1 Thermodynamics of light and heat
Control and optimization of energy conversion processes involving photon absorption and radiation require detailed understanding of thermodynamic properties of radiation as well as its interaction with matter [1–5]. Historically, thermodynamic treatment of electromagnetic radiation began over a century ago with Planck applying the thermodynamic principles established for a gas of material particles to an analogous “photon gas” . In particular, he showed that thermodynamic parameters, such as the energy, volume, temperature, and pressure can be applied to electromagnetic radiation, reflecting the dual wave-particle nature of photons. In this section, we will review the general thermodynamic principles governing photon propagation and interaction with matter, as well as the evolution of theoretical understanding of these phenomena since original work by Planck [2, 6–16].
1.1 Photon statistics, temperature, and chemical potential
Photons are gauge bosons for electromagnetism and are characterized by their energy ℏω = hc/λ and momentum ℏk, where h = 2πℏ is the Planck’s constant, c is the vacuum speed of light, λ is the photon wavelength, ω is the angular frequency, and k is the photon wavevector [17, 18]. Photons can also have angular momentum, including both spin and orbital components [19–21]. The former is associated with the circular polarization of the electromagnetic waves, while the latter originates from electromagnetic phase gradients. Owing to the weakness of inelastic photon–photon scattering process, photons do not exchange energy and thus do not reach thermal equilibrium among themselves during propagation. To account for energy conservation in the interactions of photons with matter, which may lead to the thermalization of a “photon gas”, the concept of temperature T can be additionally introduced. At thermal equilibrium at temperature T, the mean occupation numbers of photons obey the Bose–Einstein statistics and are defined as , where kB is the Boltzmann constant. The electromagnetic energy density of radiation in a material per unit frequency ω is defined via the Planck’s formula as [1, 2], while the intensity of thermal radiation from the material surface defined based on the power flow, per unit projected area, per unit solid angle, per unit frequency, is Iω = υg · U/4π for isotropic radiation. The parameters D(ω) and υg are the photon density of states (DOS) and group velocity, respectively. In the case of the free-space radiation, the wellknown expressions for these parameters are D = ω2/π2c3 and υg = c. The total power radiated from a blackbody surface per unit area (emissive power) can be found by integrating Iω over the whole frequency (ω) and angular (ϕ, θ) ranges: , where the factor cos θ accounts for the surface view factor (and is known as the
Lambert’s cosine law). For a blackbody source at temperature T emitting into the vacuum, I = σT4, where σ is the Stefan–Boltzmann constant.
In general, the number of photons in a photon gas is not conserved. However, light emission and absorption processes involve interactions of photons with other quasiparticles, such as electrons, plasmons, excitons, polaritons, etc., and these interactions obey the conservation laws for energy, momentum, and angular momentum. Thus the number of photons created or annihilated during these interactions cannot always be unrestricted. As a result, photons may derive not only their temperature, but also chemical potential [9–11, 23–26] from these interactions. However, the classical form of the Planck’s law is only applicable to the blackbody radiation generated by incandescent sources and characterized by a zero photon chemical potential μγ = 0. This formalism cannot properly describe other non-equilibrium absorption–emission processes, such as luminescence, lasing, gas discharge, laser cooling, or Bose–Einstein condensate  formation.
The introduction of the concept of the photon chemical potential enables establishing relations between the number of photons and the number of other quasiparticles photons interact with. These interactions can be modeled in analogy with chemical reactions (i.e., equilibrium is reached when the sum of the chemical potentials, including that of photons, is zero). For example, the distribution of photons emitted at temperature T as a result of recombination of electrons in the conduction band and holes in the valence band of a semiconductor takes the modified form , where μγ = μe + μh. μe and μh are the chemical potentials of the electron and holes in the emitter [9, 11, 28–30]. It should be noted that these chemical potential values can only be established after charge carriers reach thermal quasiequilibrium among themselves within each energy band, forming the quasi-Fermi energy levels for the electron (Fe) and hole (Fh) distributions in the conduction and valence bands, respectively, so that μγ = Fe – Fh.
The chemical potential of photons can be introduced by several methods, including photoexcitation, electrical injection, and parametric coupling . For example, photoexcitation of charge carriers in a semiconductor results in the formation of the separate quasi-Fermi levels for electrons and holes, and emission of photons carrying positive chemical potential. This is a typical situation for the operation of photovoltaic (PV) cells [29, 32] (see section 1.2) and the efficiency enhancement mechanism in thermophotonic cells and up-converters [33–36] (see section 3.2). Upon substituting the modified photon distribution function into the Planck radiation law, we can observe that photons with a positive chemical potential carry higher energy per photon state than thermally emitted photons at the same emitter temperature. This effect is illustrated in Figure 1a, which compares photon spectra from sources at varying temperatures and with varying positive chemical potential. Another important distinction from the blackbody spectrum is that the spectra of photons emitted with a chemical potential have a low-energy cut-off, which is defined by, for example, the electronic bandgap of the emitter material (Figure 1a). If under the external bias applied to the emitter material Fh becomes larger than Fe, photons with negative chemical potential are emitted, which carry less energy than the photons in the blackbody spectrum (Figure 1b). This situation is typical for the operation of thermoradiative (TR)  cells (see section 1.2), hot-electron energy converters  and optical rectennas [39, 40].
1.2 Photon entropy and light energy conversion limits
Another important thermodynamic characteristic of light is photon entropy [2, 3, 9, 26, 41–43]. Understanding the entropy of photons helps to establish the fundamental upper limits for the processes involving conversion of light energy into work and vice versa, including PVs, light generation, and optical refrigeration [3, 15, 29, 44–49]. For a photon flux with a given photon DOS and a distribution function N(ω), the expression for the entropy per photon state has the following form: , which is applicable to both equilibrium and non-equilibrium cases [2, 6]. At the thermal equilibrium, the entropy reaches its maximum and the photon occupation numbers obey Bose–Einstein statistics, . The entropy flux leaving the surface of a blackbody source can be calculated via integration over photon energy and direction of light propagation, and equals 4/3 · σT3[2, 6]. This expression deviates from the conventional definition of the entropy flow for thermal processes driven by heat conduction, Q/T, assuming the heat flow Q is equivalent to the total integrated photon power flow I = σT4. Figure 2a compares the entropy content (i.e., a ratio of the entropy flux to the power flux, S/I) of radiation for varying temperatures and chemical potentials with that corresponding to heat conduction (S/I = T–1). It can be clearly seen that the entropy content of blackbody emission is higher than that of heat conduction. However, as the chemical potential increases, the entropy of radiation decreases and tends to zero when the lasing condition (μγ → ℏω) is reached [9, 28]. The low entropic content of lasers and other coherent sources makes possible optical refrigeration, that is, anti-Stokes fluorescent cooling [50–52], which is discussed in more detail in section 3.2. Figure 2a also shows that high-temperature emission is characterized by lower entropy content than the low-temperature one for any value of the chemical potential of photons.
From the above discussion it follows that depending on the origin or radiation, light can be either worse (S/I > T–1) or better (S/I < T–1) source of energy to extract work from, compared to heat conduction. This has important consequences in the maximum energy conversion efficiency achievable in different types of engines, depending on whether energy is delivered to and from the engine via heat conduction or radiation. A schematic of an engine together with a heat source and a heat sink is shown in Figure 2b. The heat is delivered to the engine via radiation and the entropy is transferred to the heat sink via heat conduction. The engine emits photons back to the environment at temperature T, which is lower than the temperature of the heat source Th. We assume that the heat sink is at temperature Tc = 300 K, and model the sun as a blackbody emitter with a temperature of Th = 6000 K. The general expression for the engine efficiency is also shown in Figure 2b, which depends on the temperatures of individual elements and on the mechanisms of the energy delivery to and entropy rejection from the engine.
In particular, if heat is delivered to an engine via blackbody radiation (Ih) and the engine rejects entropy to the environment via blackbody radiation (Sr) and heat conduction (Ss), the heat can be converted to work at a maximum efficiency that is less than the classical Carnot efficiency limit . This efficiency is known as the Landsberg efficiency [3, 44] (Figure 2c, blue dotted line), which is calculated under the assumptions that the heat source is the sun and there is no irreversible entropy generation in the engine (Sg = 0). Landsberg efficiency reaches its maximum value if T = Tc, taking a more familiar form: . For the sun as the heat source, ηL = 93.3%, representing the upper bound of the solar energy conversion efficiency. For comparison, the efficiency of the ideal Carnot engine  reaches 95% efficiency for Th = 6000 K (gray dotted line in Figure 2c). It has recently been noted that the ultimate efficiency of photon energy conversion can exceed the Landsberg limit in the case of a terrestrial heat source, which can absorb and recycle the heat re-emitted by the engine, yielding . Landsberg efficiency for terrestrial sources at different temperatures Th is shown in Figure 2c as teal lines, which reach the Carnot limit when T = Th, and exceed solar Landsberg efficiency for Th = 6000 K and T > Tc.
However, the Landsberg limit can only be approached in time non-reciprocal systems [26, 54] due to the entropy generation resulting from a local non-equilibrium between photon absorption and emission rates in the absorber material [10, 26]. The entropy generated in the processes of the photon absorption and thermal re-emission is [28, 55]. Accounting for this entropy generation, the solar energy conversion efficiency in an engine with a blackbody absorber takes a more general form: [26, 56], which is plotted as a function of the engine temperature in Figure 2c (red solid line). This effi-
ciency reaches its maximum value of 85.3% at T ≈ 2500 K for a blackbody absorber. However, high efficiencies can be reached at lower temperatures of the absorber if selective surfaces are used (see section 2.1).
The entropy generation in photon energy converters stems from the power mismatch between the incoming radiation and the spontaneous emission of the absorber, and can be mitigated by allowing more degrees of freedom to tailor the spontaneous emission. One example is using the infinite-junction solar cells, where each junction independently interacts with incoming photons at each frequency [28, 29]. Another approach is using a stack of two (or more) independently operated PV cells of the same material, but different thicknesses . Although not explicitly discussed in the original publication , this strategy enables tuning of two independent photon chemical potentials in individual cells to match the incoming radiation and suppress entropy generation.
To maximize the generated power, engines typically have to be operated away from their point of the lowest entropy generation. For example, in the engines that convert solar energy into an electrical current collected at voltage V (e.g., PV cells), entropy generation is minimized in the open circuit voltage regime, yet to maximize power output, the cell needs to operate at a lower voltage (Figure 2d). This reduces the chemical potential of re-emitted photons (Figure 2d, red lines), and increases the irreversible entropy generated in the cell (Figure 2d, blue lines). The inability of a PV cell to utilize the photon energy in excess of the PV cell voltage (together with the loss of the photons with the energies below the bandgap) results in the limiting efficiency of a single-junction PV cell–known as the Shockley–Queisser limit [29, 32]–to deviate significantly from the maximum efficiency discussed in Figure 2c. It also results in the PV cells heating, which further reduces cell efficiency due to increased energy loss through reradiation (see Figure 1a, 1c), and forces cell operation at an even lower voltage to mitigate this loss (dotted lines in Figure 2d, T = 400 K).
Finally, efficiency of some energy converters, such as hot-electron cells  and TR cells  is maximized if they are operated at a negative voltage to reduce radiative losses at high temperatures. As illustrated in Figure 2e, TR cells–to which heat is delivered via conduction and the entropy is rejected via radiation–reach their highest efficiency when operated under large negative voltage, which minimizes radiation and reduces irreversible entropy generation in the cell. However, the highest power is generated under operation at a smaller negative voltage, and is accompanied by the irreversible entropy production. The limiting efficiency of a TR cell can be further increased if it is only capable of emitting near-monochromatic lowenergy radiation (dotted lines in Figure 2e), albeit at the price of the reduced power generation.
1.3 The role of electron and photon densities of states and the photon angular momentum
In addition to temperature and photon chemical potential, the intensity and spectrum of radiation emitted by an object can also be modified by manipulating the photon DOS [14, 58–66]. Furthermore, most materials do not emit as blackbodies, and an energy-dependent “gray body” factor typically needs to be introduced to account for intrinsic material properties, which can be tailored by material engineering. For example, for a gray body semiconductor exhibiting an electronic bandgap and thus emitting photons carrying chemical potential, the emission rate is typically calculated via the van Roosbroeck-Shockley equation: [67–69]. This equation is valid for emitters exhibiting a quasi-thermal equilibrium within their respective electronic bands, including excited and ground state electrons, and also for μγ.
It should be noted that the absorptance coefficient α(ω) is the rate of photon absorption under the condition of detailed balance between the emission and absorption process, that is, under a certain quasi-equilibrium electron and hole distributions. As such, unlike the case of the blackbody emission, α(ω) depends not only on the photon energy and temperature, but also on the rate of the carrier excitation, for example, photoexcitation or electrical injection. This can be shown by calculating the emission rate by applying Einstein’s theory of spontaneous and stimulated emission, R(ω) = D(ω) · σ(ω) · fu (1 – fl), which is proportional to the product of the absorption rate σ(ω), the probability of the excited electron state being occupied fu and the ground state being unoccupied (1 – fl) [68, 69]. fu and fu are the Fermi–Dirac distributions of charge carries in the emitter material. The absorption rate σ(ω) is calculated under the condition that the upper state is empty and the lower state is full, and thus is uniquely defined by the available charge carrier DOS inside the material and by the transition selection rules imposed by momentum conservation [68, 69]. Accordingly, the material absorption rate can be tailored by engineering the electron DOS, for example, via electron confinement effects. This can yield highly spectrally coherent emission spectra from quantum dots and wells [16, 70–72] as will be discussed in section 2.3. Furthermore, as the emission rate depends on the rate of the carrier excitation, α(ω) = σ(ω) · (fl – fu), the emission spectra can be also manipulated via a combination of increased temperature and either optical pumping or electrical injection [15, 73, 74] (see section 3.2).
Finally, the photon DOS and group velocity can significantly deviate from their free space values in structured photonic environments with a profound effect on the spectral characteristics of the emitter. The photon DOS defines the number of states in the momentum space between k and k + dk per unit volume and solid angle ω that are available for a photon to occupy in 3D space as: D(k)dk = k2Ωdk/(2π)3. DOS as a function of photon energy is expressed via the photon dispersion relation: D(ω) = Ω/ (2π)3 · k2(ω) · dk/dω[17, 18, 63]. It can be seen that high DOS values can be reached for high-momentum optical states and/or for states with flat dispersion characteristics.
The easiest way to increase the momentum of an optical state, and thus its DOS, is by increasing the refractive index n. The dispersion relation for an isotropic bulk material with refractive index has a well-known form , which is shown in Figure 3a for n = 1 (dotted line). The photon DOS of an isotropic bulk material with index n > 1 for both light polarizations is enhanced compared to vacuum, Dn(ω) = n3ω2/π2c3. The radiative intensity is, in turn, proportional to n2 since radiative transport requires multiplication with the group velocity of light, c/n. This effect can be utilized to maximize light absorption for PV applications [22, 66, 75, 76] and to design high-index radiation extractors for fluorescent  and thermal [77, 78] emission. In anisotropic media, photon DOS has a more complicated expression, taking different values for ordinary and extraordinary rays .
As the photon DOS is inversely proportional to the light group velocity , trapped or guided modes with high photon momenta and/or flat dispersion can have DOS significantly exceeding that of bulk materials [14, 58–66, 80–82]. As a result, radiative intensity from photonic structures supporting such states can be resonantly enhanced beyond the n2 limit of bulk dielectrics. In particular, resonant effects associated with the excitation of surface polariton waves [61, 63, 83, 84] can be used to strongly modify a material’s absorptance and emittance.
Surface polaritons are electromagnetic surface modes existing in metals and polar materials, such as silver, gold, silicon carbide (SiC), and silica (SiO2). Surface phonon polariton (SPhP) modes result from the hybridization of photons and transverse optical phonons, while surface plasmon polaritons (SPPs) are formed owing to the hybridization of photons and volume plasmons–collective oscillations of free electrons. Figure 3a shows the dispersion characteristic of a SPhP mode on a SiC-air interface. The flat region of the dispersion curve corresponds to the excitation of the SPhP at the interface, and is characterized by a strong resonant enhancement of the local density of photon states (LDOS), as shown in Figure 3b[61, 63]. The high longitudinal momentum associated with surface polariton modes is a manifestation of the angular momentum of photons involved in the circulating powerflow along the material interface [85–87]. Although the highlongitudinal-momentum photon states only exist in the sub-wavelength region near the interface, they can be utilized to enhance thermal emission provided that the emitter and the extractor (or the absorber) are coupled through the near field [12, 63, 72, 83, 88–96]. Near-field coupling between SPP or SPhP modes on multiple material interfaces also enables engineering photonic metamaterials characterized by hyperbolic photon dispersion, known as hyperbolic metamaterials (HMMs) [63, 65, 97–100] HMMs are highly anisotropic, and the spectral energy density of photons in HMMs drastically differs from that predicted by Planck’s blackbody theory. The Stefan–Boltzmann law for hyperbolic media has been shown to be a quadratic (rather than fourth order) function of the temperature . HMMs are also characterized by high photon DOS in broad frequency bands, which can be utilized for engineering solar absorbers [101, 102] and thermal emitters both in the near and far field [63, 103, 104] (see section 5.1).
Confined quantized photon states in optical nanostructures can be also used to enhance and tailor energy extraction via photon emission in both near and far field regimes. These photon states include guided modes in thin films [62, 75, 80, 105–107], fibers and nanowires [108–111], trapped modes and localized polariton modes of optical micro- and nano-cavities [59, 62, 81, 112–115], and photonic crystal defect modes [116, 117]. Thermal emission extraction via engineering photon LDOS in micro/nanostructures builds upon the obvious parallels with the electronic DOS engineering in quantum wells, wires, and dots [62, 105].
Figure 3a shows the dispersion characteristics of highmomentum whispering gallery modes (WGMs) trapped in a 5-micron TiO2 microsphere (i.e. a thermal dot) by total internal reflection [112, 118]. WGMs are characterized by a high angular photon momentum , defined by the mode quantum number l. The linear tangential momentum reaches a high value on the sphere surface. Its role in the generation of the high photon LDOS is analogous to the role of the high inplane photon momentum of surface polaritons on planar interfaces. The photon LDOS on the microsphere surface is shown in Figure 3b as the red line and features sharp peaks corresponding to the WGM excitations at discrete frequencies. Each WGM has a frequency degeneracy of 2l + 1, due to several allowed azimuthal momentum quantum numbers m = –l, ... l for each angular momentum number l[112, 118]. This degeneracy–which may be removed in micro- and nano-cavities of more complex geometries or due to near-field electromagnetic coupling [114, 120, 121]–further increases the LDOS of the high-k WGM states.
Although WGM states exhibit high LDOS, curvature of a sphere or cylinder results in total internal reflection that is not as ideal as for planar interfaces. As a result of this curvature, it is possible for these modes to leak energy into the far field, thus enabling radiation extraction and external coupling. In fact, this very argument can also be applied in the case of particles supporting localized surface polariton modes as well. In Figure 3c, we plot the absorption efficiency for a SiC microsphere, which we calculated using Mie theory [59, 84] as the ratio of the sphere’s scattering cross-sections to its geometrical cross-section (blue solid line). The two sharp peaks observed in Figure 3c correspond to the excitation of the localized SPhP modes at the frequencies within the Restrahlen band of SiC characterized by a negative dielectric permittivity, and trapped WGMs outside of this band. From the detailed balance principle, the absorptance spectra in Figure 3c can be used to calculate the corresponding emittance from the sphere into the angular element dΩk as εk(ω) = αk(ω) . The absorptance and emittance can be further enhanced via far-field electromagnetic coupling between microspheres arranged into a square-lattice array with the period on the order of radiation wavelength (red solid line).
Figure 3c illustrates that individual high-DOS wavelength-scale absorbers can exhibit absorption crosssections that are larger than the corresponding geometrical cross-sections [84, 122], which demonstrates the possibility of emittance that is higher than a blackbody  as well as the possibility for generating spectrally coherent thermal light. Indeed, thermal emission from wavelengthscale particles and nanowires [84, 110, 123] is among the few known examples of far-field radiation exceeding the blackbody limit. The emittance or absorptance of extended arrays of individual nanoscale emitters, which is calculated per unit surface area rather than the localized emitters’ surface area, cannot exceed the blackbody limit . Nevertheless, long-range electromagnetic coupling in such arrays can enable highly localized heating via photon absorption, and, by reciprocity, enhanced light extraction from nanoscale thermal emitters.
It is important to note that DOS modification via trapped photon states (e.g., WGMs) does not necessarily rely on the excitation of surface modes in the emitter material, and thus offers more flexibility in their spectral design. As seen in Figure 3, trapped photons states can be excited at frequencies much higher than those typical for SPhP excitation, which offers applications in optical energy conversion schemes, such as thermophotovoltaics [62, 105, 124].
2 Heat is the new light: manipulation and harvesting of thermal emission
Spontaneous emission, including thermal emission, typically yields incoherent and unpolarized light. The ability to control the frequency, spectral coherence and directionality of thermal and thermally enhanced fluorescent radiation would be a significant benefit for applications, including solar energy harvesting, radiative cooling, sensing, and spectroscopy. In this section, we review the stateof-the art and remaining challenges associated with spectrally shaping the spontaneous emission via engineering of both the electron and photon densities of states. DOS engineering has been successfully used in the past to either enhance or inhibit light absorption, fluorescence rates, Raman scattering efficiency, and near-field energy transfer for applications, such as on-chip communications and sensing [115, 118, 125–132]. However, the broadband nature of thermal emission and the temperature dependence of the photon state occupancies make photon DOS engineering for heat extraction more challenging.
2.1 Selective surfaces for solar thermal energy generation
The incorporation of spectral selectivity in radiative absorbers and emitters can benefit many applications, most notably, in the field of solar thermal energy conversion. Solar thermal energy converters with blackbody receivers suffer from re-emission losses at high temperatures . In Figure 4a, we illustrate this challenge by comparing the spectral photon energy fluxes for AM1.5  solar radiation and thermally emitted infrared (IR) radiation from a blackbody at high temperatures. Typically, solar ther-
mal receivers require a high level of solar concentration to overcome these losses. However, achieving high optical concentration, for example, by using a large heliostat field may not only be costly, but also introduces additional energy losses, which reduce overall system efficiency and can have negative environmental impact.
To suppress re-emission losses, a receiver with a stepwise emittance, as shown in the inset to Figure 4a, needs to be engineered [15, 135–138]. Ideally, such a receiver would feature a complete absorptance across most of the solar spectrum, and zero emittance at lower frequencies overlapping with the thermal emission spectra. As illustrated in Figure 4b, even a non-ideal receiver with 90% solar absorptance and 10% IR emittance can increase the maximum possible efficiency of the solar energy conversion. The better functionality is achieved due to the ability to reach higher receiver temperatures at low solar concentrations (Figure 4c). The values in Figure 4b, c for each solar concentration have been calculated by optimizing the transitional frequency separating high-absorptance and low-emittance spectral regions to yield the highest equilibrium temperature of the receiver. Due to the presence of atmospheric absorption bands in the solar spectrum, the equilibrium temperature does not vary smoothly with the solar concentration, as evidenced by the kinks in Figure 4c.
At this point, it should be mentioned that the receiver designs presented above with high solar absorptance and low thermal emittance do not violate the Kirchhoff’s law. Although the common corollary of the Kirchhoff’s law is typically assumed to be that a good absorber has to be a good emitter, and by contrast a poor absorber, a poor emitter, it is important to realize that terrestrial absorbers operate at temperatures much lower than the temperature of the Sun. Thus these receivers are not in thermal equilibrium with solar radiation. They, however, obey the general form of the Kirchhoff’s law, also known as the principle of detailed balance, ε(ω, θ, ϕ, T) = α(ω, θ, ϕ, T), where ε(ω, θ, ϕ, T) is the directional spectral emittance, α(ω, θ, ϕ, T) is the directional spectral absorptance, and the angles θ, ϕ specify light propagation direction.
Absorbers with angular selectivity can offer even higher energy conversion efficiencies for solar thermal energy conversion applications (red solid line in Figure 3b). Unlike conventional (Lambertian) emitters with isotropic emission patterns, angular-selective emitters can only absorb/emit light within a narrow angular range . As sunlight illuminating the Earth surface is highly collimated, such receivers can still achieve perfect absorptance of solar energy . To calculate the efficiency shown in Figure 4b, the angular-selective receiver is assumed to exhibit no spectral selectivity. The combination of both spectral and angular selectivity can yield an even higher efficiency at low solar concentrations. Angular selectivity would also benefit a myriad of other applications, including solar receivers, thermophotovoltaic (TPV) energy converters, and energy-efficient directional incandescent light sources.
Spectral and angular selectivity can be achieved by using external filters or by designing the absorber to emit
selectively in different directions. Several possible approaches to achieve thermal emission with angular selectivity are illustrated in Figure 5. The first approach shown in Figure 5a is based on a reflective cavity with an aperture [142–144]. Thermally emitted photons propagating in the direction close to the normal to the emitter surface escape the cavity through the aperture. However, photons emitted at larger angles are reflected back to the emitter and re-absorbed, thus dramatically reducing thermal emission losses. The aperture also allows sunlight to illuminate and heat the receiver. Similarly, multilayered dielectric Bragg filters with spectrally and angleselective properties recently demonstrated by Soljacic and colleagues (Figure 5b) can also be used to recycle photons emitted at angles that differ from the chosen direction of emission  or at frequencies outside of a select frequency band . This approach also allows combining spectral and angular selectivity by designing the filter to have omnidirectional reflectance within chosen frequency range(s). The selective filter can also be attached directly to the emitter surface [137, 146, 147].
Asymmetric nano- and micro-scale objects supporting localized optical resonances can also exhibit highly nonisotropic angular emission patterns as illustrated in Figure 5c for the case of a notched WGM microdisk. Local perturbations in symmetrical emitters can help to match the momentum of the high-k trapped modes to the low-k propagating modes in free space, thus facilitating far-field extraction of the optical energy. In particular, Boriskina has previously predicted that localized indentations can be used to generate highly directional light emission from WGM microcavities [148, 149], which has been subsequently proven experimentally .
Finally, long-range electromagnetic coupling effects in gratings or photonic crystals can provide momentum matching of propagating photons in free space to high-k polariton modes supported by metals, doped semiconductors, or polar dielectrics. This long-range coupling yields highly directional thermal emission from gratings at select frequencies corresponding to the excitation of high-LDOS surface modes [151, 152] Some examples of directional thermal sources based on gratings will be discussed in section 2.3. Gratings can also be designed to provide spectral selectivity for light absorption and thermal emission. This functionality is illustrated in Figure 6a, which shows calculated absorptance spectra for single- and multipleperiodic hafnium (Hf) gratings. Hf was chosen for this demonstration for use in a high temperature solar receiver as this metal forms a stable native oxide layer, which is advantageous for high-temperature operation in air rather than in vacuum, and can also be used to further improve solar absorption. It can be seen in Figure 6a that the metal surface spectral selectivity can be improved by patterning the metal surface, and is tunable by the pattern geometry and symmetry properties. The emittance of the patterned surface drops sharply in the long-wavelength spectral range above 3 micron, which can help prevent re-emission losses at high temperatures. Other patterned metal surfaces–including tungsten (W), tantalum (Ta) and gold (Au)–have been demonstrated to provide similar or even better spectral selectivity [138, 153, 154].
Despite the good performance of such structures for creating thermal emission selectivity, the fabrication of large-scale micro- and nano-scale patterns at the emitter surface can be a technologically challenging and costly endeavor. To address this challenge, the development of spectrally selective emitters with simpler geometries is highly desirable. One recently proposed approach to achieve spectral selectivity and suppress thermal emission is to cover a solar receiver with a layer of transparent silica aerogel. The aerogel provides efficient thermal insulation  and helps to reduce the IR emittance of the receiver, offering a simple planar technological solution to improve the efficiency of a solar thermal energy converter. Another possible solution to achieving spectral selectivity, which will be discussed in the next section, is to place thin film emitters on top of optimally designed substrates or embed them into planar Fabry–Perot optical cavities. Selective absorbers and emitters designed using this approach have been successfully demonstrated both theoretically and experimentally [107, 156–159].
2.2 Mesoscale resonant structures for passive radiative cooling
Unlike solar thermal receivers, PV solar converters need to operate at low temperatures. However, low-energy photons cannot be converted to electricity in PV cells; instead, they contribute to parasitic heating of the device. To alleviate this problem and to increase efficiency of PV cells, it was recently proposed by Shanhui Fan and colleagues to combine high solar absorption with high thermal emission in the IR spectral range [160, 161]. Radiative cooling of PV cells and other devices requires development of nanostructures and materials with drastically different electromagnetic response in the visible and IR frequency ranges. For this application, high absorptance in the visible range needs to be accompanied by the high emittance in the IR region. The IR emittance should ideally peak in the frequency range corresponding to the atmospheric transparency window in 8–13 micron wavelength range [162–166]. A selective emitter radiating strongly in this range is thus exposed to the clear sky enabling the use of the outer space as a very low temperature heat sink. Radiative cooling can be achieved by choosing an optimal combination of material and optical properties.
This approach to tailor the spectral properties of solar receivers is illustrated in Figure 6b, which shows the simulated absorptance and emittance spectra of a multilayer absorber with an 80-nm thick layer of amorphous silicon (a-Si) as the active layer for potential PV applications. The 130-nm silica (SiO2) spacer underneath the a-Si layer is supported by a gold reflector and thus acts as a planar Fabry–Perot cavity. Constructive interference of incident and reflected light within this cavity can lead to an increase in solar absorption. The absorptance in the visible frequency range drops sharply at the frequency corresponding to the a-Si material bandgap. In turn, radiative cooling of this structure can be achieved as a result of IR emittance enhanced by the SPhP mode excitation within the Restrahlen band of a 700-nm silica layer on top of the a-Si film, which spectrally overlaps with the atmospheric transparency window. This layer simultaneously serves as the transparent anti-reflective coating in the visible range, which helps to enhance solar absorption in a-Si. In the structure reported in Figure 6b, we have numerically optimized the thicknesses of each individual layer to increase IR emittance and to simultaneously enhance solar absorption. More complicated photonic crystal structures have been designed to achieve even higher IR emission for the PV cell cooling applications [166, 167].
Personalized cooling technology is another example of an application where optical spectral selectivity can be beneficial. Conventional personal cooling is typically achieved through heat conduction and convection. However, past studies have shown the human body to be a very efficient emitter of IR radiation , which suggests radiative cooling can also be an effective cooling mechanism. Most conventional fabrics are opaque to IR radiation (see Figure 6c) and block thermal emission from the body to the environment. Ideal fabrics for personalized cooling applications thus need to exhibit spectral selectivity in their transmittance characteristics. They should enable IR transmission to directly pass through clothing, thus maximizing radiative cooling, while ensuring that the fabric is opaque at visible wavelengths. We have recently demonstrated that resonant electromagnetic effects in microfibers can provide a basis for the development of a new wearable technology for personalized cooling .
The fabrics with the required spectrally selective transmittance spectra were designed using a combination of optimal material composition and structural photonic engineering. Synthetic polymers that support few vibrational modes were identified as candidate materials to reduce intrinsic material absorption in the IR wavelength range. Individual fibers were designed to be comparable in size to visible wavelengths to achieve strong light scattering and thus remain optically opaque to the human eye. At the same time, they are too thin to support trapped photon states at IR wavelengths. This reduces the photon LDOS in microfibers and minimizes the interaction of the fabrics with IR light, resulting in high transmission in this spectral range.
As illustrated in Figure 6c, the designed fabrics are indeed opaque for the visible light, yet transparent for the IR thermal radiation emitted by the human body. Compared to conventional personal cooling technologies, these fabrics can provide a fully passive means to cool the human body regardless of the person’s physical activity level. The anticipated effect of the new optical–thermal polymer fabrics (tailored into a short sleeve shirt and pants) will be the increase in the body cooling rate by at least 23 W . This would enable thermally regulated interior environments, such as offices or homes, to raise the summer HVAC temperature set points from 75 to 79°F, resulting in significant energy savings .
2.3 Nanophotonic incandescent sources: coherent, polarized, and twisted thermal light
Spectral and angular selectivity of radiation is a signature of the temporal and spatial coherence of the thermal emitter. Many of the above approaches to increase coherence of the thermally emitted light have been pursued both theoretically and experimentally, as illustrated in Figure 7. Coherent thermal emitters can potentially be used as tunable light sources for sensing and spectroscopy, especially in the far-IR range, where hardly any coherent sources are available . They can also play an important role in optical communications and solar and waste heat energy harvesting, for example, via a TPV energy conversion process [49, 138, 172–174] or optical rectification [39, 40]. The degree of coherence for a radiation source with a known spectral distribution I(ω) can be calculated as , where τ is the time delay between interfering light sources, which is determined by the optical path difference Δ as τ = 2Δ/υg[175–177]. The coherence length is typically defined as the optical path difference at which the degree of coherence reaches 10%. The coherence length of thermal blackbody radiation scales inversely with temperature of the source and equals about 0.6 micron for the sunlight  and about 4 micron for the radiation from an incandescent emitter at T ∼ 775 K . However, resonant enhancement of photon and electron DOS in the emitter via a combination of optical and quantum confinement effects can yield nanoand micro-scale thermal sources with coherence and polarization characteristics of emitted photons deviating significantly from blackbody radiation. This is important for thermal emission manipulation via optical interference, as only [partially] coherent light exhibits interference phenomena, while completely incoherent light sources contribute additively to the intensity at any point of space. Furthermore, the temporal and spatial coherence of the thermal emitter are manifested in the spectral and angular selectivity of emission, which stem from the positionmomentum and time-energy uncertainty principles, and can be utilized in the photon energy conversion schemes.
For example, it has been shown by Greffet and others that planar sources supporting surface polariton modes yield quasi-monochromatic near-field radiation with the coherence length larger than the emitted photon wavelength . Thermal sources with geometries that provide matching of the high momentum of these surface modes to the free space radiation may exhibit even longer coherence length than planar near-field emitters made of the same material [180, 181]. These coherent far-field direc-
tional thermal sources can be shaped as nanowire antennas shown in Figure 7a or planar gratings of either parallel  or concentric [182, 183] grooves as shown in Figure 7b, 7c. For example, the coherence length of thermal emission from individual Ti/Pt nanowires of 125 nm in width was experimentally measured to be at least 20 μm at T = 773 K, which is much larger than expected for a blackbody emitter . Such thermal sources with sizes on the order or smaller than the wavelength of emitted photons are especially interesting, as they can exhibit global coherence if the coherence length is comparable to or exceeds the wavelength. In turn, the coherence length of the near-IR tungsten grating emitter shown in Figure 7b is measured to be about 106 micron at T = 623 K . This value exceeds the coherence length of the blackbody emission and is approaching a coherence length of a CO2 laser. Other coherent thermal emitters based on periodic one-dimensional gratings and two-dimensional photonic crystals with emission peaks observed in near-to-far-IR frequency range have been demonstrated experimentally by using metals and polar dielectrics [180, 181, 184–189].
Thermal emission from coherent nanoscale sources quite often exhibits a significant degree of polarization . For example, radiation from heated thin nanowires supporting localized plasmon and polariton waves is strongly polarized in the direction orthogonal to the wire [191, 192]. As the polarization direction of emitted light follows the orientation of nanoscale emitters, thermal emission from nanopatterned surfaces can be tailored by introducing local anisotropy of individual emitters’ orientation. As shown in Figure 7d[181, 193, 194], local anisotropy can be introduced by gradually rotating the direction of nanorod antennas patterned on a planar substrate. It has been shown experimentally by Hasman and colleagues that thermal radiation emitted by such a surface exhibits photon momentum characteristics associated with the emission from a revolving medium. This phenomenon is known as the angular Doppler effect [181, 193, 194], and is a manifestation of the spin–orbit interaction of emitted light. Spin–orbit interactions are also a basis for other interesting optical effects, such as photon analogs of spin-Hall [195–197], Magnus , and Coriolis  effects, which paves the road to many exciting applications of coherent nanoscale thermal sources in the emerging field of spinoptics.
Finally, thermal emission can be controlled by simultaneous engineering of photon LDOS and electron DOS in the material. The latter modifies intrinsic absorption characteristics of the material and can be achieved by using quantum confinement effects, for example, in quantum wells as shown in Figure 7e[16, 70, 71]. In this structure, quantum-well intersubband transitions strongly modify material absorption properties, which–in combination with photon DOS modification due to a periodic arrangement of nanoscale emitters–results in a dramatic narrowing of the spectral and angular range of emitted radiation. Likewise, monolayer materials, such as graphene demonstrate unusual electronic and optical properties due to the electron confinement in the monolayer plane. Embedding a graphene layer inside a planar optical microcavity as shown in Figure 7f provides a way to modify graphene emission characteristics and to achieve highly spectrally selective thermal emission .
The devices shown in Figure 7e, 7f can be pumped by electrical current injection, which heats up the emitter due to scattering of injected electrons. If the optical modal structure of the thermal source inhibits radiation of longwavelength photons, the thermal energy accumulates inside the emitter in the form of the energy of phonons and “hot” charge carriers, which leads to the emitter self-heating. As a result, emitter can reach significantly higher temperatures under the same input power and thermal management conditions as compared not only to the blackbody reference, but also to the same material in the absence of photon confinement effects [16, 70, 200]. Furthermore, at high temperatures, the thermal conductivity of the suspended graphene is significantly reduced due to the strong Umklapp phonon–phonon scattering , which also suppresses lateral heat dissipation and leads to spatial localization of hot electrons. As a result, the efficiency and brightness of thermal emission is further increased, making possible realization of thermal graphene sources emitting in the visible range .
3 Thermal up- and down-conversion of photon energy
Thermal energy storage and recycling inside emitters with spectral- and angular-selective characteristics can be used to achieve thermal up- and down-conversion of photon energy via the process of photon absorption and subsequent controlled thermal re-emission. This is illustrated in Figure 8a, b, which schematically show photon absorbers and thermal emitters with angular- and frequency-selective surfaces. The absorbed photons are coupled to another surface via heat conduction and re-emitted in desirable frequency range. By adjusting the spectral selectivity of the absorbing and emitting surfaces, either up- or downconversion process can theoretically be achieved. Solar TPV energy conversion platforms effectively make use of the photon down-conversion process shown in Figure 8a
to convert the broadband solar spectrum to a narrowband thermal emission spectrum, which peaks at lower photon energy tuned to fit the electron bandgap of a PV cell [138, 146, 203–207]. Thermal up-conversion of photon energy (Figure 8b) is more challenging, yet could be highly promising for applications in waste heat harvesting and in development of tunable photon sources.
3.1 Thermal up-conversion
We have recently predicted  that solar-to-electricity conversion efficiency higher than the conventional Shockley–Queisser limit for PV cells  can be achieved in a hybrid platform that combines a single-junction solar cell and a thermal up-converter, as illustrated in Figure 8c. Within such a hybrid scheme, photons with energies below the bandgap of the PV cell are absorbed by the up-converter, which heats up and re-emits photons with higher energies towards the cell. To make this process possible, both front and back surfaces of the up-converter must have carefully designed angular- and frequency-selective emittance characteristics. The front surface should provide a perfect absorption of sunlight across the solar spectrum, and prevent re-emission of photons at lower frequencies. Additionally, it should reduce re-emission of photons with energies overlapping with the solar spectrum, which requires the surface to exhibit angular as well as spectral selectivity. This can be achieved, for example, via the use of an external cavity with an aperture or a selective filter as shown in Figure 5a, 5b. In turn, the emitter surface should only allow emission of photons with energies above the PV cell bandgap.
The maximum efficiency of a hybrid device utilizing the thermal up-conversion scheme can reach 73% for the ideal selective emittance characteristics (perfect solar absorption and perfect thermal emission blocking) of the up-converter surfaces under illumination by the nonconcentrated sunlight (Figure 8d) . Reaching high up-conversion efficiency requires raising the up-converter temperature, which for the commonly used PV materials–for example, Si, GaAs, CdTe, and GaAsP–nevertheless was predicted to lie within practically achievable 900–1600 K range. Non-ideal up-converter surfaces that allow for reasonable absorption and emission losses still yield limiting efficiency values exceeding 45% for moderate optical concentration of 300 suns (Figure 8d). The observed increase in the predicted conversion efficiency is a result of better matching of the PV cell bandgap energy to the energy of incoming photons, which reduces irreversible entropy generation in the PV cell. For the ideal angular and spectral characteristics of the up-converter surfaces, the entropy creation rate in the up-converter is much lower than that in the PV cell, which explains high maximum efficiency levels shown in Figure 8d. However, the increase in the radiation losses from the up-converter with non-ideal characteristics results in the increase in the entropy creation rate in the up-converter (see section 1.2), which is reflected in the drop in the hybrid device efficiency. Successful realization of such hybrid platform could offer new opportunities for reaching higher levels of solar energy conversion efficiency under low levels of optical concentration [15, 208].
3.2 Laser cooling and heat-assisted luminescence
Anti-Stokes luminescence is another example of a process based on thermally induced up-conversion of the photon energy. The thermal up-conversion process discussed in the previous section relies on the energy storage as the phonon or free electron energy, accompanied by controlled photon re-emission in thermal equilibrium with the material. The photon up-conversion via anti-Stokes luminescence instead makes use of a non-equilibrium photon emission as a result of radiative recombination of electron-hole pairs assisted by electron–phonon scattering, as schematically shown in Figure 9a. This process results in the emission of photons carrying chemical potential (see section 1.1) and with energies that are higher than the energy of photons in the optical pump, which forms a basis for optical refrigeration (also called laser refrigeration or anti-Stokes fluorescent cooling) [50–52]. Optical refrigeration can be achieved by irradiating a luminescent material at a frequency on the low energy tail of its absorption band, which is followed by spontaneous emission of more energetic photons in the process of the anti-Stokes luminescence (Figure 9b). The extra energy of emitted photons is extracted from the lattice phonons, which results in the cooling of the material. The anti-Stokes luminescence can also be observed under material pumping via electron injection [209–212].
Although optical refrigeration was originally proposed by Pringsheim almost a century ago , the progress in this field was stymied for decades, first, by the concerns for possible violation of the thermodynamics second law  and later, by the lack of high-purity materials. Landau helped to resolve the controversy with the second law violation by proper accounting for the entropy of light emitted in the process of spontaneous isotropic anti-Stokes fluorescence  (see section 1.2). In turn, progress in materials engineering yielded materials with high internal quantum efficiency, which enabled successful experimental demonstrations of the optical refrigeration, mostly of rare-Earth-doped grasses [42, 51, 52], starting with the experiments of Epstein and co-authors . The efficiency of the laser cooling process scales with the material absorption efficiency ηabs and the external quantum efficiency ηext as ηc = ηabs · ηext · (λp/λf) – 1, where λp is the wavelength of the optical pump, and is the wavelength of the spontaneous anti-Stokes fluorescent emission. Accordingly, a lot of effort in increasing this efficiency has been directed to material engineering in order to increase the pump photon absorption rate and to suppress non-radiative decay due to multi-phonon emission processes. In particular, electron DOS engineering with quantum wells, dots, and impurity bands has been explored to increase the cooling efficiency [64, 210, 214–217]. However, the external quantum efficiency can be strongly affected by the photon DOS in the emitter and its near-field neighborhood, which paves the way to the potential efficiency increase via photonic engineering [51, 64, 218].
The role that the photon DOS engineering can play in boosting the efficiency of the optical refrigeration is two-
fold. First, a fluorescence peak can be blue-shifted by suppressing the photon DOS in a spectral range above the pump wavelength λp, thus decreasing λf. Additionally, an increase of the radiative rate at the blue-shifted emission wavelength could increase the external quantum efficiency ηext. Photonic crystals  and planar surfaces supporting surface-plasmon polariton modes [64, 220] have been theoretically proposed by Khurgin as promising means to improve the cooling efficiency, however, they have not been experimentally demonstrated to date. Two successful examples of the nanophotonic structures that improve the efficiency of the optical refrigeration are shown in Figure 9c, 9d. The structure in Figure 9c makes use of the n2 emission rate enhancement (see section 1.3) in a high-index absorber. The absorber is coupled to a luminescent emitter across a nanoscale gap, which provides thermal insulation and enhances photon extraction via frustrated total internal reflection process, that is, photon tunneling across the gap [51, 221]. High-index photon extractors shaped as domes, which are directly attached to the luminescent emitter have also been experimentally demonstrated . In turn, the use of optically thin nanobelt cryocoolers (Figure 9d) [218, 222] enables suppression of the photon DOSinside the luminescent material and thus increases the external quantum efficiency. Instead of getting trapped inside the material and optically recycled until they are re-absorbed, up-converted photons can escape the nanobelt structure, resulting in its temperature reduction. Likewise, photon DOS engineering has potential to improve cooling of solids via the process of spontaneous anti-Stokes Raman scattering .
Finally, as the heat-enhanced anti-Stokes spontaneous emission and scattering processes enable photon energy up-conversion, they can be used to increase the efficiency of solar energy conversion processes. One possible realization of a hybrid solar energy converter using heat-assisted photoluminescence has recently been proposed [15, 73, 74, 224–226], and is schematically illustrated in Figure 9b. In such a converter, solar radiation is absorbed in a low-bandgap photo-luminescent emitter, which is kept at high temperature. The heat sink is replaced with a PV cell with the bandgap energy higher than the bandgap of the emitter. The up-converted photons emitted in the process of the anti-Stokes luminescence gain enough energy to be harvested by the high-bandgap PV cell. This enables converting thermal energy into electrical work at high voltage, which yields enhanced device efficiency. Such a hybrid conversion platform has been theoretically predicted to reach maximum efficiency of 70% at operating temperatures below 1000°C. Operation at even lower temperatures (< 500 K) can be achieved if the thermal gradient is maintained by a hot electron-hole gas rather than by a hot lattice, such as, for example, in a hot-carrier solar cell operated at open circuit . Recent experiments demonstrated 30% up-conversion efficiency by using a InGaAs/GaAsP quantum well up-converter, where the thermal gradient was maintained by steadystate Auger heating of charge carriers .
4 Bridging heat conduction and radiation on the nanoscale
As discussed above, tremendous progress has been made in understanding and controlling thermal emission, which resulted in successful demonstrations of coherent thermal sources. However, unless thermal emitters are operated at high temperatures, they are only suitable for low power applications, especially when compared to conventional coherent emission sources, such as lasers and light emitting diodes as well as alternative heat transfer mechanisms, such as heat conduction and convection. At realistic emitter temperatures, the power output of thermal sources and optical energy converters is low, even if they can theoretically operate at very high efficiencies. One approach to boost the power output relies on storing energy in the form of non-equilibrium excitations, with subsequent emission of photons that carry chemical potential. This enables generation of a higher energy flux than equilibrium blackbody radiation at the same temperature of the emitter (see Figure 1a). This approach forms the basis for the operation of the hybrid energy converter based on the heat-enhanced anti-Stokes luminescence (Figure 9b) [15, 73, 74, 224]. Another approach makes use of the dramatic enhancement of the local photon DOS in the near-field of a thermal emitter to increase the radiative power of a thermal source . Past studies have successfully demonstrated both theoretically and experimentally that by separating an emitter and an absorber by distances comparable to the wavelength of radiation, it is possible to enhance radiative transfer by several orders of magnitude beyond the blackbody limit [12, 90, 91, 93–96, 99, 227–232].
4.1 Near-field DOS enhancement & resonant energy transfer
The latter approach is demonstrated in Figure 10a, which compares the photon energy flux spectrum of a blackbody emitter with the corresponding spectra for a thin-film “thermal well” emitter [62, 105], collected in the far- and the near-field, respectively. It can be seen in Figure 10a that the photon DOS modification in thin-film emitters can be used to efficiently suppress long-wavelength far-field thermal radiation (blue solid line). The photon DOS suppression below cut-off frequencies of the guided modes trapped in the thin film by the total internal reflection is analogous to the case of the nanobelt cryocooler [218, 222] discussed in section 3.2. This spectral selectivity translates into high theoretically predicted efficiency of TPV platforms using thin film emitters and thin film PV cells . However, the total energy flux delivered by photons from the emitter to the PV cell drops dramatically below the blackbody emitter level, which would reduce the power output of a TPV platform. The observed drop in the power flux is due to an inability of the high-momentum guided modes in the thin film to couple to the free-space propagating modes that carry energy away from the emitter into the far field (top inset in Figure 10a). In contrast, if the same emitter and the PV cell are coupled through the near field, the radiative energy flux is significantly enhanced and can exceed the blackbody level by orders of magnitude while retaining spectral selectivity (red solid line). The basis for the observed enhancement is the efficient coupling of the high-k trapped waveguide modes across the vacuum gap, which results in the enhanced tunneling of emitted photons into the absorber (middle inset in Figure 10a).
Even more dramatic enhancement of the near-field radiative heat transfer rate can be achieved by using nearfield emitters and absorbers supporting surface polariton modes, which exhibit significant photon DOS enhancement at resonance, as explained in section 1.3. Figure 10b presents calculated near-field heat flux spectra between planar emitters and absorbers made of either aluminum zinc oxide (AZO, blue solid line) or SiC (teal solid line) and coupled across a 20-nm wide vacuum gap . Both spectra exhibit resonant peaks due to the electromagnetic coupling of surface plasmon–polariton modes in AZO and phonon–polariton modes in SiC across the vacuum gap (bottom inset in Figure 10a). These peaks exceed the blackbody limit by orders of magnitude. Figure 10b also illustrates that further radiative heat flux enhancement can be achieved if the emitter and the absorber are shaped as ultra-thin films (compare the red solid line with the blue one). The additional enhancement has been attributed to the significant spectral broadening of the emission spectra due to coupling between SPP modes on both sides of each thin film [72, 233]. Similarly, mode-coupling-induced spectrum broadening and enhancement of the radiative heat flux has been predicted and demonstrated for thinfilm SPhP emitters [92, 93, 234–237] as well as for metamaterial [98, 103, 104, 147, 186, 192, 238, 239] emitters composed of multiple thin films (or nanowires) supporting polariton modes.
4.2 Bridging conduction and radiation
To date, most of the calculations of both the far-field thermal emission and the near-field radiative energy transfer
have relied upon macroscopic Maxwell equations—either exact or under various approximations. Although the continuum electromagnetic models smear out the atomic details, they are applicable in most practical cases. However, these details cannot be ignored when the separation between thermal emitters and absorbers approaches atomic length scales. As a result, the electrodynamic theory developed by Rytov [7, 8] to model the near-field radiative heat transfer, which is based on the fluctuation–dissipation theorem , diverges as the gap between an emitter and absorber approaches zero (see Figure 10c), which is unphysical. Accordingly, a mechanistic atomic-scale description of the transfer mechanisms is required for more accurate prediction of energy transfer at very small separations between two bodies.
To develop such an approach, we utilized the Green’s function formalism using lattice dynamics with the microscopic Maxwell equations . By using the new approach, we investigated the mechanisms underlying energy transport between two ionic slabs in the near-field radiation regime down to contact within a single unified formalism . Figure 10c shows the calculated values of conductance plotted as a function of slab separation for small gaps to show the discrepancy between our approach (dots) and Rytov theory (solid line) near contact. The Rytov theory demonstrates the unphysical divergence near contact whereas our theory is able to yield a finite contact conductance. The new model resolves the zero-gap divergence issue and provides a computational tool to probe the conductance from the near-field radiation regime down to contact in a unified manner. Interestingly, the new results show that near-field radiative heat flux at very small gaps can be enhanced even stronger than previously predicted via continuous electromagnetic models.
5 Discussion: remaining challenges and outlook
Despite the tremendous progress in understanding various mechanisms of thermal emission manipulation and applying this knowledge to develop new device designs, many challenges still remain, both fundamental and technological.
5.1 Progress and challenges in materials engineering and fabrication
For example, fabrication of nanoscale gaps between an emitter and absorber remains a significant technological challenge. As a result, experimental demonstration of high-efficiency near-field TPV platforms is lacking despite many promising conceptual proposals. However, radiative heat transfer between a nanoscale tip and a planar surface
can be achieved at very narrow separations. This offers many interesting technological applications, including thermal radiation scanning tunneling microscopy [243–246], high-resolution thermal lithography , and heatassisted magnetic recording [247–249], where nanoscale thermal emitters are used to heat a magnetic recording medium. The progress in this field will also benefit optical refrigeration and photon up-conversion applications, where the figure of merit can be improved by using the near-field fluorescence extraction mechanism [220, 250].
Continued progress in materials engineering is also essential for the development of new material platforms with optical properties tuned to yield high photon DOS at various frequencies from the visible to the far-IR [171, 251–253]. In particular, dynamically tunable thermal emitters are of high interest with applications to sensing, spacecraft thermal management, and thermal camouflage. Materials that actively alter their thermal emittance through phase change have been investigated for this purpose, most notably, vanadium dioxide (VO2), which undergoes an insulator-to-metal transition at 68°C [254, 255]. This leads to the thermal emission reduction if the temperature is increased above the transition temperature, contrary to the blackbody emission trend, and offers applications in IR camouflage . However, unique properties of VO2 can also be used to design metamaterial emitters that emit strongly at temperatures above the phase transition as illustrated in Figure11a,11b. The emitter shown in Figure11a has a periodic structure composed of thin layers of VO2 and magnesium fluoride (MgF2), which is a transparent dielectric in mid-IR, and is supported by an aluminum (Al) back reflector. At low temperatures, the multi-layer structure is largely transparent in the IR, and thus the overall emittance is governed by the Al mirror, resulting in a low emittance (Figure 11a). In contrast, at high temperatures, VO2 becomes metallic and the multi-layer structure undergoes a transition to become a hyperbolic metamaterial, which exhibits enhanced emission across the entire IR wavelength range due to its hyperbolic photon dispersion [63, 65, 97–100] (Figure 11b). Such metamaterial emitters with variable heat rejection can be useful for terrestrial and spacecraft thermal management applications .
VO2 emitters can also be used to achieve strong dynamic modification of the near-field heat transfer, especially in combination with polar materials, such as SiO2 or SiC (Figure 11c). A thin film of VO2 in its metallic phase supports SPP modes, which enhance the near-field radiative heat flux at high temperatures and screen the SPhP mode of the silica substrate (red solid line). When the VO2 film becomes transparent in its insulator phase, it enables the SPhP mode to transfer energy across the nanoscale gap between the emitter and the absorber, resulting in a dramatic spectral transformation of the near-field heat flux (blue solid line). It should be noted that in the case of lowtemperature operation, the radiative near-field heat flux from a VO2 surface is dominated by the strong contribution from the SPhP polariton modes supported by the insulator phase of VO2 at low frequencies (above 20 μm in wavelength) .
Active tuning of thermal emission via external electric or magnetic fields could enable higher switching rates, but to date, has only been demonstrated in a handful of materials. These include fast modulation of the intersubband emission of the quantum well p–i–n diodes  and tuning of the graphene thermal emission  via application of gate bias, which varies the carrier density in the emitter material. Emission properties of perovskite-structure ferroelectric materials can also be modulated by application of an external DC electric field, as illustrated in Figure 11d, and temperature . However, as this process is most effective near the Curie temperature–that is, phase transition temperature between ferroelectric and paraelectric phases–development of ferroelectric materials with high Curie temperatures is necessary for practical applications. Other types of phase-change or voltage-tunable materials that can be explored for developing tunable thermal emitters include W-VO2 alloys , ITO , and Ge2Sb2Te5 (GST)  just to name a few. Achieving material stability at high temperatures and outside of vacuum environment is also a big challenge that needs to be overcome [15, 154, 264].
5.2 Advances and challenges in fundamental understanding and nanophotonic design
Some fundamental aspects of the light absorption, emission, as well as light-to-work energy conversion are still under investigation. In particular, the search is still ongoing for the optimum conditions to achieve higher-thanblackbody emittance of coherent nanoscale sources or by reciprocity, enhanced resonant absorption at select frequencies. Some success in increasing the absorption cross-sections has been achieved by tuning the geometry and material composition of nanoscale emitters to achieve near-degeneracy of several trapped photon modes of different polarization and angular momentum in a narrow spectral range [265, 266]. Metamaterial hyperlenses have been theoretically predicted to yield selective absorber heating and, by reciprocity, enhanced light extraction from nanoscale thermal sources into the far field [78, 267, 268]. It has also been proposed that extraordinarily large absorption cross-sections of nanoscale resonators can be achieved by embedding them into a material with near-zero refractive index . Recent progress in designing and fabricating low-loss zero-index metamaterials operating at various frequency ranges [270–273] makes feasible practical realization of this approach. The role of collective effects  caused by the interference between multiple coherent thermal sources in thermal emission enhancement, radiation wave front shaping, and focusing still needs to be revealed [275, 276]. In particular, fundamental and technological solutions for thermal emission focusing can help to overcome challenges in realizing the near-field coupling schemes.
Fundamental studies on the entropy and information content of correlated light fields generated by coherent thermal sources are also important [277–279], especially in the processes of light absorption and emission away from thermal equilibrium, when light–matter interactions occur over time scales too short for the thermalization process to take place. This is illustrated by a recent striking demonstration of efficient optical refrigeration via the heat transport between a thermal bath and a non-equilibrium exciton–polariton fluid . Other theoretical studies predict that a modification of a photonic system coupling to the thermal bath via parametric oscillations may create an effective chemical potential for photons even in thermodynamic equilibrium . This offers potential applications in quantum electrodynamics and optomechanics.
Finally, addressing the issues associated with heat removal from the laser gain media require detailed understanding of the energy and entropy of the photons, electrons, and phonons in laser systems [41, 281–284]. Development of a complete theoretical framework connecting the fundamental atomic physics, thermodynamics, and material science associated with photon absorption, emission, and non-radiative thermal transport phenomena at nano/micro and macro scales is necessary to address these issues.
The authors would like to thank Laureen Meroueh, Kenneth McEnaney, Lee Weinstein, Marin Soljacic, Shanhui Fan, Carmel Rotschild, Peter Bermel, Philippe Ben-Abdallah, David McClosky, Calinda M. Yew, Baratunde Cola, and Richard M. Osgood for helpful discussions. This work was supported by DOE-BES Award No. DE-FG02-02ER45977 (for thermal emission tailoring and near-field radiative heat transport), the ARPA-E award DE-AR0000471 (for hybrid full spectrum harvesting), and the “Solid State Solar-Thermal Energy Conversion Center (S3TEC)”, funded by the US Department of Energy, Office of Science, and Office of Basic Energy, Award No. DE-SC0001299/DE-FG02-09ER46577 (for TPV applications).
Planck M., The theory of heat radiation, P. Blackston’s sons co (1914).Google Scholar
Landau L., Lifshitz E., Statistical Physics, Part 1, Course Theor. Physics, vol. 5, Institute of Physical Problems, USSR Academy of Sciences, Moscow (1980).Google Scholar
Landsberg P. T., Tonge G., Thermodynamic energy conversion efficiencies, J. Appl. Phys. 51(7), R1–R20 (1980).Google Scholar
Ruppel W., Wurfel P., Upper limit for the conversion of solar energy, IEEE Trans. Electron Dev. 27(4), 877–882 (1980).Google Scholar
De Vos A., Pauwels H., On the thermodynamic limit of photovoltaic energy conversion, Appl. Phys. A Mater. Sci. Process. 25(2), 119–125, Springer Berlin / Heidelberg (1981).Google Scholar
Landau L., On the thermodynamics of photoluminescence, J. Phys. 10, 503–506 (1946).Google Scholar
Rytov S. M. M., Theory of electric fluctuations and thermal radiation, Air Force Cambridge Research Center, Bedford, MA (1959).Google Scholar
Rytov S. M., Kravtsov Y. A.., Tatarskii V. I., Principles of statistical radiophysics, Springer-Verlag, New York (1987).Google Scholar
Wurfel P., The chemical potential of radiation, J. Phys. C Solid State Phys. 15(18), 3967, IOP Publishing (1982).Google Scholar
Wurfel P., Ruppel W., The flow equilibrium of a body in a radiation field, J. Phys. C Solid State Phys. 18(15), 2987–3000, IOP Publishing (1985).Google Scholar
Ries H., Thermodynamics of Quantum Conversion of Light, Zeitschrift für Phys. Chemie 1(1), 133–140 (1998).Google Scholar
Rousseau E., Siria A., Jourdan G., Volz S., Comin F., Chevrier J., Greffet J.-J., Radiative heat transfer at the nanoscale, Nat Phot. 3(9), 514–517, Nature Publishing Group (2009).Google Scholar
Song B., Fiorino A., Meyhofer E., Reddy P., Near-field radiative thermal transport: From theory to experiment, AIP Adv. 5(5), 053503, AIP Publishing (2015).Google Scholar
Bermel P., Boriskina S. V., Yu Z., Joulain K., Control of radiative processes for energy conversion and harvesting, Opt. Express 23(24), A1533–A1540, Optical Society of America (2015).Google Scholar
Boriskina S. V., Green M. A., Catchpole K., Yablonovitch E., Beard M. C., Okada Y., Lany S., Gershon T., Zakutayev A., et al., Roadmap on optical energy conversion, J. Opt. (2016).Google Scholar
Inoue T., De Zoysa M., Asano T., Noda S., Realization of narrowband thermal emission with optical nanostructures, Optica 2(1), 27, Optical Society of America (2015).Google Scholar
Levi A. F. J., Applied quantum mechanics, Cambridge Univ. Press (2006).Google Scholar
Chen G., Nanoscale energy transfer and conversion, Oxford University Press (2005).Google Scholar
Allen L., Padgett M. J., Babiker M., Wolf E., IV The Orbital Angular Momentum of Light, [Progress in Optics], Elsevier, 291–372 (1999).Google Scholar
Mazilu M., Optical eigenmodes; spin and angular momentum, J. Opt. 13(6), 064009, IOP Publishing (2011).Google Scholar
Bliokh K. Y., Rodriguez-Fortuno F. J., Nori F., Zayats A. V., Spinorbit interactions of light, Optics, 23 (2015).Google Scholar
Yablonovitch E., Statistical ray optics, J. Opt. Soc. Am. 72(7), 899–907 (1982).Google Scholar
Landsberg P. T., Photons at non-zero chemical potential, J. Phys. C Solid State Phys. 14(32), L1025–L1027, IOP Publishing (1981).Google Scholar
Ries H., Mcevoy A. J. J., Rles H., Mcevoy A. J. J., Chemical potential and temperature of light aFA, J. Photochem. Photobiol. A Chem. 59(1), 11–18 (1991).Google Scholar
Badescu V., Time-dependent and steady-state statistics of photons at nonzero chemical potential, J. Phys. Condens. Matter 3(33), 6509–6521, IOP Publishing (1991).Google Scholar
Green M. A., Third Generation Photovoltaics: Advanced Solar Energy Conversion (Springer Series in Photonics), Springer (2005).Google Scholar
Klaers J., Schmitt J., Vewinger F., Weitz M., Bose-Einstein condensation of photons in an optical microcavity., Nature 468(7323), 545–548, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved. (2010).Google Scholar
Green M., Energy, entropy and efficiency, [Third Generation Photovoltaics], T. Kamiya, B. Monemar and H. Venghaus, Eds., Springer Berlin Heidelberg, 21–34 (2006).Google Scholar
Henry C. H., Limiting efficiencies of ideal single and multiple energy gap terrestrial solar cells, J. Appl. Phys. 51(8), 4494–4500 (1980).Google Scholar
Markvart T., The thermodynamics of optical étendue, J. Opt. A Pure Appl. Opt. 10(1), 015008 (2008).Google Scholar
Hafezi M., Adhikari P., Taylor J. M., A chemical potential for light, Quantum Physics; Statistical Mechanics; Optics, 7 (2014).Google Scholar
Shockley W., Queisser H. J., Detailed balance limit of efficiency of p-n junction solar cells, J. Appl. Phys. 32(3), 510–519 (1961).Google Scholar
Harder P. N., Green M. A., Thermophotonics, Semicond. Sci. Technol. 18(5), S270 (2003).Google Scholar
Farrell D. J., Sodabanlu H., Wang Y., Sugiyama M., Okada Y., Can a Hot-Carrier Solar Cell also be an Efficient Upconverter?, IEEE J. Photovoltaics 5(2), 571–576 (2015).Google Scholar
Farrell D. J., Sodabanlu H., Wang Y., Sugiyama M., Okada Y., A hot-electron thermophotonic solar cell demonstrated by thermal up-conversion of sub-bandgap photons., Nat. Commun. 6, 8685, Nature Publishing Group (2015).Google Scholar
Xue J., Zhao Y., Oh S.-H., Herrington W. F., Speck J. S., Den-Baars S. P., Nakamura S., Ram R. J., Thermally enhanced blue light-emitting diode, Appl. Phys. Lett. 107(12), 121109, AIP Publishing (2015).Google Scholar
Strandberg R., Theoretical efficiency limits for thermoradiative energy conversion, J. Appl. Phys. 117(5), 055105, AIP Publishing (2015).Google Scholar
Ross R. T., Nozik A. J., Efficiency of hot-carrier solar energy converters, J. Appl. Phys. 53(5), 3813, American Institute of Physics (1982).Google Scholar
Joshi S., Moddel G., Efficiency limits of rectenna solar cells: Theory of broadband photon-assisted tunneling, Appl. Phys. Lett. 102(8), 083901, AIP Publishing (2013).Google Scholar
Lerner P. B., Miskovsky N. M., Cutler P. H., Mayer A., Chung M. S., Thermodynamic analysis of high frequency rectifying devices: Determination of the efficiency and other performance parameters, Nano Energy 2(3), 368–376 (2013).Google Scholar
Ruan X. L., Rand S. C., Kaviany M., Entropy and efficiency in laser cooling of solids, Phys. Rev. B 75(21), 214304 (2007).Google Scholar
Epstein R. I., Buchwald M. I., Edwards B. C., Gosnell T. R.., Mungan C. E., Observation of laser-induced fluorescent cooling of a solid, Nature 377(6549), 500–503 (1995).Google Scholar
Mashaal H., Gordon J. M., Basic limit for the efficiency of coherence-limited solar power conversion, Opt. Lett. 39(17), 5130–5133, Optical Society of America (2014).Google Scholar
Landsberg P. T., Evans D. A., Thermodynamic Limits for Some Light-Producing Devices, Phys. Rev. 166(2), 242–246, American Physical Society (1968).Google Scholar
Gordon J. M., A simple derivation of work and efficiency limits for blackbody radiation converters, Am. J. Phys. 61(9), 821, American Association of Physics Teachers (1993).Google Scholar
Boriskina S. V., Tong J. K., Ferry V. E., Michel J., Kildishev A. V., Breaking the limits of optical energy conversion, Opt. Photonics News(July/Aug), 50–53 (2015).Google Scholar
Alharbi F. H., Kais S., Theoretical limits of photovoltaics efficiency and possible improvements by intuitive approaches learned from photosynthesis and quantum coherence, Renew. Sustain. Energy Rev. 43, 1073–1089 (2015).Google Scholar
Luque A., Martí A., Theoretical limits of photovoltaic conversion, [Handbook of Photovoltaic Sci. Eng.], John Wiley & Sons, Ltd, 113–151 (2003).Google Scholar
Harder N.-P., Wurfel P., Theoretical limits of thermophotovoltaic solar energy conversion, Semicond. Sci. Tech. 18(5), S151 (2003).Google Scholar
Pringsheim P., Zwei Bemerkungen über den Unterschied von Lumineszenz und Temperaturstrahlung, Z. Phys. 57, 739–746 (1929).Google Scholar
Sheik-Bahae M., Epstein R. I., Optical refrigeration, Nat. Photonics 1(12), 693–699, Nature Publishing Group (2007).Google Scholar
Nemova G., Kashyap R., Laser cooling of solids, Reports Prog. Phys. 73(8), 086501 (2010).Google Scholar
Carnot N. L. S., Reflections on the motive power of heat (1824).Google Scholar
Ries H., Complete and reversible absorption of radiation, Appl. Phys. B Photophysics Laser Chem. 32(3), 153–156 (1983).Google Scholar
De Vos A., Pauwels H., Comment on a thermodynamical paradox presented by P. Wurfel, J. Phys. C Solid State Phys. 16(36), 6897 (1983).Google Scholar
Wurfel P., Physics of solar cells: from principles to new concepts, WILEY-VCH Verlag GmbH &Co. KGaA, Weinheim (2005).Google Scholar
Yu Z., Sandhu S., Fan S., Efficiency above the Shockley-Queisser limit by using nanophotonic effects to create multiple effective bandgaps with a single semiconductor., Nano Lett. 14(1), 66–70, American Chemical Society (2014).Google Scholar
Purcell E. M., Spontaneous emission probabilities at radio frequencies, Phys. Rev. 69(11-12), 674, American Physical Society (1946).Google Scholar
Bohren C. F., Huffman D. R., Absorption and scattering of light by small particles, Wiley-VCH 98, Weinheim, Germany (1983).Google Scholar
Luo C., Narayanaswamy A., Chen G., Joannopoulos J. D., Thermal Radiation from Photonic Crystals: A Direct Calculation, Phys. Rev. Lett. 93(21), 213905 (2004).Google Scholar
Joulain K., Mulet J.-P., Marquier F., Carminati R., Greffet J.-J., Surface electromagnetic waves thermally excited: Radiative heat transfer, coherence properties and Casimir forces revisited in the near field, Surf. Sci. Reports 57(3-4), 59–112 (2005).Google Scholar
Boriskina S. V., Tong J., Weinstein L., Hsu W.-C., Huang Y.., Chen G., Thermal emission shaping and radiative cooling with thermal wells, wires and dots, Adv. Photonics 2015, IT2A.3, OSA, Washington, D.C. (2015).Google Scholar
Boriskina S. V., Ghasemi H., Chen G., Plasmonic materials for energy: From physics to applications, Mater. Today 16(10), 375–386 (2013).Google Scholar
Khurgin Y., Improving the efficiency of laser cooling of semiconductors by means of bandgap engineering in electronic and photonic domains, [Optical refrigeration], R. I. Epstein and M. Sheik-Bahae, Eds., WILEY-VCH Verlag, 169–196 (2009).Google Scholar
Jacob Z., Smolyaninov I. I., Narimanov E. E., Broadband Purcell effect: Radiative decay engineering with metamaterials, Appl. Phys. Lett. 100(18), 181104–181105, AIP (2012).Google Scholar
Callahan D. M., Munday J. N., Atwater H. A., Solar cell light trapping beyond the ray optic limit, Nano Lett. 12(1), 214–218, American Chemical Society (2012).Google Scholar
van Roosbroeck W., Shockley W., Photon-Radiative Recombination of Electrons and Holes in Germanium, Phys. Rev. 94(6), 1558–1560 (1954).Google Scholar
Lasher G., Stern F., Spontaneous and Stimulated Recombination Radiation in Semiconductors, Phys. Rev. 133(2A), A553–A563 (1964).Google Scholar
Bhattacharya R., Pal B., Bansal B., On conversion of luminescence into absorption and the van Roosbroeck-Shockley relation, Appl. Phys. Lett. 100(22), 222103, AIP Publishing (2012).Google Scholar
De Zoysa M., Asano T., Mochizuki K., Oskooi A., Inoue T., Noda S., Conversion of broadband to narrowband thermal emission through energy recycling, Nat. Photonics 6(8), 535–539, Nature Publishing Group (2012).Google Scholar
Inoue T., De Zoysa M., Asano T., Noda S., Single-peak narrowbandwidth mid-infrared thermal emitters based on quantum wells and photonic crystals, Appl. Phys. Lett. 102(19), 191110, AIP Publishing (2013).Google Scholar
Boriskina S., Tong J., Huang Y., Zhou J., Chiloyan V., Chen G., Enhancement and Tunability of Near-Field Radiative Heat Transfer Mediated by Surface Plasmon Polaritons in Thin Plasmonic Films, Photonics 2(2), 659–683, Multidisciplinary Digital Publishing Institute (2015).Google Scholar
Manor A., Martin L. L., Rotschild C., Optical refrigeration for ultra-efficient photovoltaics, SPIE OPTO, R. I. Epstein, D. V. Seletskiy and M. Sheik-Bahae, Eds., 93800L, International Society for Optics and Photonics (2015).Google Scholar
Manor A., Martin L., Rotschild C., Conservation of photon rate in endothermic photoluminescence and its transition to thermal emission, Optica 2(6), 585, Optical Society of America (2015).Google Scholar
Yu Z. F., Raman A., Fan S. H., Fundamental limit of nanophotonic light trapping in solar cells, Proc. Natl. Acad. Sci. USA 107(41), 17491–17496 (2010).Google Scholar
Yu Z., Raman A., Fan S., Fundamental limit of light trapping in grating structures, Opt. Express 18(S3), A366–A380, OSA (2010).Google Scholar
Yu Z., Sergeant N. P., Skauli T. T., Zhang G., Wang H., Fan S., Enhancing far-field thermal emission with thermal extraction, Nat. Commun. 4, 1730, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved (2013).Google Scholar
Shi J., Liu B., Li P., Ng L. Y., Shen S., Near-field energy extraction with hyperbolic metamaterials, Nano Lett 15(2), 1217–1221, American Chemical Society (2015).Google Scholar
Biehs S.-A., Lang S., Petrov A. Y., Eich M., Ben-Abdallah P., Blackbody Theory for Hyperbolic Materials, Phys. Rev. Lett. 115(17), 174301 (2015).Google Scholar
Saeta P. N., Ferry V. E., Pacifici D., Munday J. N., Atwater H. A., How much can guided modes enhance absorption in thin solar cells?, Opt. Express 17(23), 20975–20990, OSA (2009).Google Scholar
Grandidier J., Callahan D. M., Munday J. N., Atwater H. A., Gallium Arsenide Solar Cell Absorption Enhancement Using Whispering Gallery Modes of Dielectric Nanospheres, IEEE J. Photovoltaics 2(2), 123–128 (2012).Google Scholar
Jacob Z., Kim J. Y., Naik G. V., Boltasseva A., Narimanov E. E., Shalaev V. M., Engineering photonic density of states using metamaterials, Appl. Phys. B 100(1), 215–218 (2010).Google Scholar
Shen S., Narayanaswamy A., Chen G., Surface phonon polaritons mediated energy transfer between nanoscale gaps., Nano Lett. 9(8), 2909–2913, American Chemical Society (2009).Google Scholar
Bohren C. F., How can a particle absorb more than the light incident on it?, Am. J. Phys. 51(4), 323–327, AAPT (1983).Google Scholar
Tong J., Mercedes A., Chen G., Boriskina S. V., Local field topology behind light localization and metamaterial topological transitions, [Singular and Chiral Nanoplasmonics], S. V. Boriskina and N. I. Zheludev, Eds., Pan Stanford, 259–284 (2014).Google Scholar
Bliokh K. Y., Nori F., Transverse spin of a surface polariton, Phys. Rev. A 85(6), 061801 (2012).Google Scholar
Rosenblatt G., Feigenbaum E., Orenstein M., Circular motion of electromagnetic power shaping the dispersion of Surface Plasmon Polaritons, Opt. Express 18(25), 25861–25872, OSA (2010).Google Scholar
Volokitin A. I., Persson B. N. J., Near-field radiative heat transfer and noncontact friction, Rev. Mod. Phys. 79(4), 1291–1329, American Physical Society (2007).Google Scholar
Pendry J. B., Radiative exchange of heat between nanostructures, J. Phys. Condens. Matter 11(35), 6621 (1999).Google Scholar
Narayanaswamy A., Shen S., Hu L., Chen X. Y., Chen G., Breakdown of the Planck blackbody radiation law at nanoscale gaps, Appl. Phys. A. Mater. Sci. Proces. 96(2), 357–362 (2009).Google Scholar
Biehs S.-A., Rousseau E., Greffet J.-J., Mesoscopic description of radiative heat transfer at the nanoscale, Phys. Rev. Lett. 105(23), 234301 (2010).Google Scholar
Ben-Abdallah P., Joulain K., Drevillon J., Domingues G., Nearfield heat transfer mediated by surface wave hybridization between two films, J. Appl. Phys. 106(4), 044306 (2009).Google Scholar
Basu S., Francoeur M., Maximum near-field radiative heat transfer between thin films, Appl. Phys. Lett. 98(24), 243120, AIP (2011).Google Scholar
Basu S., Zhang Z. M., Fu C. J., Review of near-field thermal radiation and its application to energy conversion, Int. J. Energy Res. 33(13), 1203–1232 (2009).Google Scholar
Basu S., Zhang Z. M., Maximum energy transfer in near-field thermal radiation at nanometer distances, J. Appl. Phys. 105(9), 093535, AIP Publishing (2009).Google Scholar
van Zwol P. J., Joulain K., Ben-Abdallah P., Chevrier J., Phonon polaritons enhance near-field thermal transfer across the phase transition of VO2, Phys. Rev. B 84(16), 161413 (2011).Google Scholar
Poddubny A., Iorsh I., Belov P., Kivshar Y., Hyperbolic metamaterials, Nat. Photonics 7(12), 948–957, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved. (2013).Google Scholar
Guo Y., Jacob Z., Thermal hyperbolic metamaterials, Opt. Express 21(12), 15014–15019 (2013).Google Scholar
Biehs S.-A., Tschikin M., Messina R., Ben-Abdallah P., Super-Planckian near-field thermal emission with phononpolaritonic hyperbolic metamaterials, Appl. Phys. Lett. 102(13), 131106, AIP Publishing (2013).Google Scholar
Noginov M. A., Li H., Barnakov Y. A., Dryden D., Nataraj G., Zhu G., Bonner C. E., Mayy M., Jacob Z., et al., Controlling spontaneous emission with metamaterials, Opt. Lett. 35(11), 1863–1865, OSA (2010).Google Scholar
Corrigan T. D., Park D. H., Drew H. D., Guo S.-H., Kolb P. W., Herman W. N., Phaneuf R. J., Broadband and mid-infrared absorber based on dielectric-thin metal film multilayers, Appl. Opt. 51(8), 1109–1114, Optical Society of America (2012).Google Scholar
Sergeant N. P., Pincon O., Agrawal M., Peumans P., Design of wide-angle solar-selective absorbers using aperiodic metaldielectric stacks, Opt. Express 17(25), 22800–22812, Optical Society of America (2009).Google Scholar
Biehs S.-A., Tschikin M., Ben-Abdallah P., Hyperbolic Metamaterials as an Analog of a Blackbody in the Near Field, Phys. Rev. Lett. 109(10), 104301 (2012).Google Scholar
Molesky S., Dewalt C. J., Jacob Z., High temperature epsilonnear-zero and epsilon-near-pole metamaterial emitters for thermophotovoltaics, Opt. Express 21 Suppl 1(January), A96–A110, Optical Society of America (2013).Google Scholar
Tong J. K., Hsu W.-C., Huang Y., Boriskina S. V., Chen G., Thin-film “Thermal Well” emitters and absorbers for highefficiency thermophotovoltaics, Optics, Sci. Reports 5, 10661 (2015).Google Scholar
Kats M. A., Blanchard R., Genevet P., Capasso F., Nanometre optical coatings based on strong interference effects in highly absorbing media, Nat. Mater. 12(1), 20–24, Nature Publishing Group (2013).Google Scholar
Narayanaswamy A., Mayo J., Canetta C., Infrared selective emitters with thin films of polar materials, Appl. Phys. Lett. 104(18), 183107, AIP Publishing (2014).Google Scholar
Cao L., White J. S., Park J.-S., Schuller J. A., Clemens B. M., Brongersma M. L., Engineering light absorption in semiconductor nanowire devices, Nat. Mater. 8(8), 643–647, Nature Publishing Group (2009).Google Scholar
Krogstrup P., Jřrgensen H. I., Heiss M., Demichel O., Holm J. V., Aagesen M., Nygard J., Fontcuberta i Morral A., Singlenanowire solar cells beyond the Shockley–Queisser limit, Nat. Photonics 7(4), 306–310, Nature Publishing Group (2013).Google Scholar
Schuller J. A., Taubner T., Brongersma M. L., Optical antenna thermal emitters, Nat. Photonics 3(11), 658–661, Nature Publishing Group (2009).Google Scholar
Tong J. K., Hsu W.-C., Eon Han S., Burg B. R., Zheng R., Shen S., Chen G., Direct and quantitative photothermal absorption spectroscopy of individual particulates, Appl. Phys. Lett. 103(26), 261104 (2013).Google Scholar
Matsko A. B., Ilchenko V. S., Optical resonators with whispering-gallery modes-part I: basics, IEEE J. Sel. Top. Quantum Electron. 12(1), 3–14 (2006).Google Scholar
Ilchenko V. S., Matsko A. B., Optical resonators with whispering-gallery modes-part II: applications, IEEE J. Sel. Top. Quantum Electron. 12(1), 15–32 (2006).Google Scholar
Benson T. M., Boriskina S. V., Sewell P., Vukovic A., Greedy S. C., Nosich A. I., Micro-optical resonators for microlasers and integrated optoelectronics, [Frontiers in Planar Lightwave Circuit Technology, Volume 216 of the series NATO Science Series II: Mathematics, Physics and Chemistry], Springer, 39–70 (2006).Google Scholar
Boriskina S. V., Reinhard B. M., Spectrally and spatially configurable superlenses for optoplasmonic nanocircuits, Proc. Natl. Acad. Sci. U. S. A. 108(8), 3147–3151 (2011).Google Scholar
Yablonovitch E., Gmitter T. J., Meade R. D., Rappe A. M., Brommer K. D., Joannopoulos J. D., Donor and acceptor modes in photonic band structure, Phys. Rev. Lett. 67(24), 3380, American Physical Society (1991).Google Scholar
Ben-Abdallah P., Ni B., Single-defect Bragg stacks for highpower narrow-band thermal emission, J. Appl. Phys. 97(10), 104910, AIP Publishing (2005).Google Scholar
Vahala K. J., Optical microcavities, Nature 424(6950), 839–846 (2003).Google Scholar
Johnson B. R., Theory of morphology-dependent resonances: shape resonances and width formulas, J. Opt. Soc. Am. A 10(2), 343–352, OSA (1993).Google Scholar
Boriskina S. V., Sewell P., Benson T. M., Nosich A. I., Accurate simulation of two-dimensional optical microcavities with uniquely solvable boundary integral equations and trigonometric Galerkin discretization, J. Opt. Soc. Am. A. Opt. Image Sci. Vis. 21(3), 393–402 (2004).Google Scholar
Boriskina S. V., Theoretical prediction of a dramatic Q-factor enhancement and degeneracy removal of whispering gallery modes in symmetrical photonic molecules, Opt. Lett. 31(3), 338–340 (2006).Google Scholar
Boriskina S. V., Tong J. K., Hsu W.-C., Weinstein L., Huang X., Loomis J., Xu Y., Chen G., Hybrid optical-thermal devices and materials for light manipulation and radiative cooling, Proc. SPIE 9546, Act. Photonic Mater. VII, 95461U (2015).Google Scholar
Hu L., Chen G., Analysis of optical absorption in silicon nanowire Arrays for photovoltaic applications, Nano Lett. 7(11), 3249–3252 (2007).Google Scholar
Dyachenko P. N., do Rosário J. J., Leib E. W., Petrov A. Y., Störmer M., Weller H., Vossmeyer T., Schneider G. A., Eich M., Tungsten band edge absorber/emitter based on a monolayer of ceramic microspheres, Opt. Express 23(19), A1236, Optical Society of America (2015).Google Scholar
Vernooy D. W., Furusawa A., Georgiades N. P., Ilchenko V. S., Kimble H. J., Cavity QED with high-Q whispering gallery modes, Phys. Rev. A 57(4), R2293, American Physical Society (1998).Google Scholar
Gopinath A., Boriskina S. V., Premasiri W. R., Ziegler L., Reinhard B. M., Dal Negro L., Plasmonic nanogalaxies: multiscale aperiodic arrays for surface-enhanced Raman sensing, Nano Lett. 9(11), 3922–3929 (2009).Google Scholar
Benson T. M., Boriskina S. V., Sewell P., Vukovic A., Nosich A. I., Janyani V., Al-Jarro A., Sakhnenko N., Smotrova E. I., et al., Micro-resonators: simulation and application, Proc. CAOL 2005. Second Int. Conf. Adv. Optoelectron. Lasers, 2005. 1 (2005).Google Scholar
Wang J., Yang L., Boriskina S. V., Reinhard B. M. B. M., Yan B., Reinhard B. M. B. M., Spectroscopic ultra-trace detection of nitro-aromatic gas vapor on rationally designed nanoparticle cluster arrays, Anal. Chem. 83(6), 2243–2249 (2011).Google Scholar
Muskens O. L., Giannini V., Sanchez-Gil J. A., Gomez Rivas J., Strong enhancement of the radiative decay rate of emitters by single plasmonic nanoantennas, Nano Lett. 7(9), 2871–2875, American Chemical Society (2007).Google Scholar
Pelton M., Modified spontaneous emission in nanophotonic structures, Nat. Photonics 9(7), 427–435, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved (2015).Google Scholar
Giannini V., Fernández-Domínguez A. I., Sonnefraud Y., Roschuk T., Fernández-García R., Maier S. A., Controlling light localization and light–matter interactions with nanoplasmonics, Small 6(22), 2498–2507, WILEY-VCH Verlag (2011).Google Scholar
Ahn W., Hong Y., Boriskina S. V., Zhao X., Reinhard B. M., Template-guided self-assembly of discrete optoplasmonic molecules and extended optoplasmonic arrays, Nanophotonics 4(1), 250–260 (2015).Google Scholar
Ho C. K., Iverson B. D., Review of high-temperature central receiver designs for concentrating solar power, Renew. Sustain. Energy Rev. 29, 835–846 (2014).Google Scholar
ASTM International West Conshohocken PA., ASTM Standard G173-03: Standard tables for reference solar spectral irradiances: direct normal and hemispherical on 37° tilted surface (2008).Google Scholar
Badescu V., Spectrally and angularly selective photothermal and photovoltaic converters under one-sun illumination, J. Phys. D Appl. Phys. 38(13), 2166 (2005).Google Scholar
McEnaney K., Kraemer D., Chen G., Direct heat-to-electricity conversion of solar energy, An. Rev. Heat Transf. 15, 179–230 (2012).Google Scholar
Bermel P., Lee J., Joannopoulos J. D., Celanovic I., Soljacic M., Selective solar absorbers, An. Rev. Heat Transf. (2012).Google Scholar
Yeng Y. X., Ghebrebrhan M., Bermel P., Chan W. R., Joannopoulos J. D., Soljačić M., Celanovic I., Enabling hightemperature nanophotonics for energy applications, Proc. Natl. Acad. Sci. U. S. A. 109(7), 2280–2285 (2012).Google Scholar
McEnaney K., Modeling of solar thermal selective surfaces and thermoelectric generators, MIT (2010).Google Scholar
Shen Y., Ye D., Celanovic I., Johnson S. G., Joannopoulos J. D., Soljačić M., Optical broadband angular selectivity, Science 343(6178), 1499–1501 (2014).Google Scholar
Blanco M. J., Marti J. G., Alarcan-Padilla D. C., Theoretical efficiencies of angular-selective non-concentrating solar thermal systems, Sol. Energy 76(6), 683–691 (2004).Google Scholar
Weinstein L., Kraemer D., McEnaney K., Chen G., Optical cavity for improved performance of solar receivers in solarthermal systems, Sol. Energy 108, 69–79 (2014).Google Scholar
Weinstein L. A., Hsu W.-C., Yerci S., Boriskina S. V., Chen G., Enhanced absorption of thin-film photovoltaic cells using an optical cavity, J. Opt. 17(5), 055901, IOP Publishing (2015).Google Scholar
Braun A., Katz E. A., Feuermann D., Kayes B. M., Gordon J. M., Photovoltaic performance enhancement by external recycling of photon emission, Energy Environ. Sci. 6(5), 1499, The Royal Society of Chemistry (2013).Google Scholar
Ilic O., Bermel P., Chen G., Joannopoulos J. D., Celanovic I., Soljacic M., Tailoring high temperature radiation and the resurrection of the incandescent source, Nat. Nanotech. (2016).Google Scholar
Lenert A., Bierman D. M., Nam Y., Chan W. R., Celanović I., Soljačić M., Wang E. N., A nanophotonic solar thermophotovoltaic device, Nat. Nanotechnol. 9(2), 126–130, Nature Publishing Group (2014).Google Scholar
Bermel P., Harradon M., Soljacic M., Celanovic I., Joannopoulos J. D., Yeng Y., Ghebrebrhan M., Tailoring photonic metamaterial resonances for thermal radiation, Nanoscale Res. Lett. 6, 549 (2011).Google Scholar
Boriskina S. V., Benson T. M., Sewell P., Nosich A. I., Q factor and emission pattern control of the WG modes in notched microdisk resonators, IEEE J. Sel. Top. Quantum Electron. 12(1), 52–88 (2006).Google Scholar
Boriskina S. V., Benson T. M., Sewell P. D., Nosich A. I., Directional emission, increased free spectral range, and mode Q-factors in 2-D wavelength-scale optical microcavity structures, IEEE J. Sel. Top. Quantum Electron. 12(6), 1175–1182 (2006).Google Scholar
Wang Q. J., Yan C., Yu N., Unterhinninghofen J., Wiersig J., Pflügl C., Diehl L., Edamura T., Yamanishi M., et al., Whispering-gallery mode resonators for highly unidirectional laser action, Proc. Natl. Acad. Sci. U. S. A. 107(52), 22407–22412 (2010).Google Scholar
Laroche M., Arnold C., Marquier F., Carminati R., Greffet J.-J., Collin S., Bardou N., Pelouard J.-L., Highly directional radiation generated by a tungsten thermal source, Opt. Lett. 30(19), 2623, Optical Society of America (2005).Google Scholar
Arnold C., Marquier F., Garin M., Pardo F., Collin S., Bardou N., Pelouard J.-L., Greffet J.-J., Coherent thermal infrared emission by two-dimensional silicon carbide gratings, Phys. Rev. B 86(3), 035316 (2012).Google Scholar
Bermel P., Ghebrebrhan M., Chan W., Yeng Y. X., Araghchini M., Hamam R., Marton C. H., Jensen K. F., Soljacic M., et al., Design and global optimization of high-efficiency thermophotovoltaic systems, Opt. Express 18(S3), A314–A334, OSA (2010).Google Scholar
Rinnerbauer V., Ndao S., Xiang Yeng Y., Senkevich J. J., Jensen K. F., Joannopoulos J. D., Soljačić M., Celanovic I., Geil R. D., Large-area fabrication of high aspect ratio tantalum photonic crystals for high-temperature selective emitters, J. Vac. Sci. Technol. B Microelectron. Nanom. Struct. 31(1), 011802, American Institute of Physics (2013).Google Scholar
Chen G., Wang E. N., Boriskina S. V., McEnaney K., Ghasemi H., Yerci S., Lenert A., Yang S., Miljkovic N., et al., Internallyheated thermal and externally-cool photovoltaic cascade solar system for the full solar spectrum utilization, US 20150053266 A1 (2015).Google Scholar
Kats M. A., Byrnes S. J., Blanchard R., Kolle M., Genevet P., Aizenberg J., Capasso F., Enhancement of absorption and color contrast in ultra-thin highly absorbing optical coatings, Appl. Phys. Lett. 103(10), 101104, AIP Publishing (2013).Google Scholar
Roberts A. S., Chirumamilla M., Thilsing-Hansen K., Pedersen K., Bozhevolnyi S. I., Near-infrared tailored thermal emission from wafer-scale continuous-film resonators, Opt. Express 23(19), A1111, Optical Society of America (2015).Google Scholar
Jang M. S., Brar V. W., Sherrott M. C., Lopez J. J., Kim L., Kim S., Choi M., Atwater H. A., Tunable large resonant absorption in a midinfrared graphene Salisbury screen, Phys. Rev. B 90(16), 165409 (2014).Google Scholar
Langlais M., Prod’homme P., Bru H., Ben-Abdallah P., High temperature layered absorber for thermo-solar systems, J. Quant. Spectrosc. Radiat. Transf. 149, 8–15 (2014).Google Scholar
Zhu L., Raman A., Wang K. X., Anoma M. A., Fan S., Radiative cooling of solar cells, Optica 1(1), 32, Optical Society of America (2014).Google Scholar
Safi T. S., Munday J. N., Improving photovoltaic performance through radiative cooling in both terrestrial and extraterrestrial environments, Opt. Express 23(19), A1120, Optical Society of America (2015).Google Scholar
Nilsson T. M. J., Niklasson G. A., Radiative cooling during the day: simulations and experiments on pigmented polyethylene cover foils, Sol. Energy Mater. Sol. Cells 37(1), 93–118 (1995).Google Scholar
Eriksson T. S., Granqvist C. G., Radiative cooling computed for model atmospheres, Appl. Opt. 21(23), 4381–4388, Optical Society of America (1982).Google Scholar
Granqvist C. G., Radiative cooling to low temperatures: General considerations and application to selectively emitting SiO films, J. Appl. Phys. 52(6), 4205, AIP Publishing (1981).Google Scholar
Gentle A. R., Smith G. B., Radiative heat pumping from the Earth using surface phonon resonant nanoparticles, Nano Lett. 10(2), 373–379, American Chemical Society (2010).Google Scholar
Raman A. P., Anoma M. A., Zhu L., Rephaeli E., Fan S., Passive radiative cooling below ambient air temperature under direct sunlight, Nature 515(7528), 540–544, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved, (2014).Google Scholar
Rephaeli E., Raman A., Fan S., Ultrabroadband photonic structures to achieve high-performance daytime radiative cooling, Nano Lett. 13(4), 1457–1461, American Chemical Society (2013).Google Scholar
Steketee J., Spectral emissivity of skin and pericardium, Phys. Med. Biol. 18(5), 686–694, IOP Publishing (1973).Google Scholar
Tong J. K., Huang X., Boriskina S. V., Loomis J., Xu Y., Chen G., Infrared-transparent visible-opaque fabrics for wearable personal thermal management, ACS Photonics 2(6), 150609075019003, American Chemical Society (2015).Google Scholar
Ball P., Material witness: Could polythene clothes be cool?, Nat. Mater. 14(9), 865, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved, (2015).Google Scholar
Feng K., Streyer W., Zhong Y., Hoffman A. J., Wasserman D., Photonic materials, structures and devices for Reststrahlen optics, Opt. Express 23(24), A1418, Optical Society of America (2015).Google Scholar
Laroche M., Carminati R., Greffet J.-J. J., Near-field thermophotovoltaic energy conversion, J. Appl. Phys. 100(6), 063704, AIP (2006).Google Scholar
Narayanaswamy A., Chen G., Surface modes for near field thermophotovoltaics, Appl. Phys. Lett. 82(20), 3544–3546, AIP (2003).Google Scholar
Chester D., Bermel P., Joannopoulos J. D., Soljacic M., Celanovic I., Design and global optimization of highefficiency solar thermal systems with tungsten cermets, Opt. Express 19 Suppl 3(S3), A245–A257, OSA (2011).Google Scholar
Kano Y., Wolf E., Temporal Coherence of Black Body Radiation, Proc. Phys. Soc. 80(6), 1273–1276, IOP Publishing (1962).Google Scholar
Mehta C. L., Coherence-time and effective bandwidth of blackbody radiation, Nuovo Cim. 28(2), 401–408 (2008).Google Scholar
Klein L. J., Hamann H. F., Au Y.-Y., Ingvarsson S., Coherence properties of infrared thermal emission from heated metallic nanowires, Appl. Phys. Lett. 92(21), 213102, AIP Publishing (2008).Google Scholar
Donges A., The coherence length of black-body radiation, Eur. J. Phys. 19(3), 245–249, IOP Publishing (1998).Google Scholar
Carminati R., Greffet J.-J., Near-Field Effects in Spatial Coherence of Thermal Sources, Phys. Rev. Lett. 82(8), 1660–1663 (1999).Google Scholar
Greffet J.-J., Carminati R., Joulain K., Mulet J.-P., Mainguy S., Chen Y., Coherent emission of light by thermal sources, Nature 416(6876), 61–64, Macmillian Magazines Ltd. (2002).Google Scholar
Hasman E., Kleiner V., Dahan N., Gorodetski Y., Frischwasser K., Balin I., Manipulation of Thermal Emission by Use of Micro and Nanoscale Structures, J. Heat Transfer 134(3), 031023 (2012).Google Scholar
Han S. E., Norris D. J., Beaming thermal emission from hot metallic bull’s eyes, Opt. Express 18(5), 4829–4837, Optical Society of America (2010).Google Scholar
Stanley R., Plasmonics in the mid-infrared, Nat. Photonics 6(7), 409–411, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved, (2012).Google Scholar
Puscasu I., Schaich W. L., Narrow-band, tunable infrared emission from arrays of microstrip patches, Appl. Phys. Lett. 92(23), 233102, AIP Publishing (2008).Google Scholar
Costantini D., Lefebvre A., Coutrot A.-L., Moldovan-Doyen I., Hugonin J.-P., Boutami S., Marquier F., Benisty H., Greffet J.-J., Plasmonic Metasurface for Directional and Frequency-Selective Thermal Emission, Phys. Rev. Appl. 4(1), 014023 (2015).Google Scholar
Liu X., Tyler T., Starr T., Starr A. F., Jokerst N. M., Padilla W. J., Taming the blackbody with infrared metamaterials as selective thermal emitters, Phys. Rev. Lett. 107(4), 45901, American Physical Society (2011).Google Scholar
Hesketh P. J., Zemel J. N., Gebhart B., Polarized spectral emittance from periodic micromachined surfaces. II. Doped silicon: Angular variation, Phys. Rev. B 37(18), 10803–10813 (1988).Google Scholar
Hesketh P. J., Zemel J. N., Gebhart B., Organ pipe radiant modes of periodic micromachined silicon surfaces, Nature 324(6097), 549–551 (1986).Google Scholar
Pralle M. U., Moelders N., McNeal M. P., Puscasu I., Greenwald A. C., Daly J. T., Johnson E. A., George T., Choi D. S., et al., Photonic crystal enhanced narrow-band infrared emitters, Appl. Phys. Lett. 81(25), 4685, AIP Publishing (2002).Google Scholar
Sandus O., A Review of Emission Polarization, Appl. Opt. 4(12), 1634, Optical Society of America (1965).Google Scholar
Bimonte G., Cappellin L., Carugno G., Ruoso G., Saadeh D., Polarized thermal emission by thin metal wires, New J. Phys. 11(3), 033014, IOP Publishing (2009).Google Scholar
Öhman Y., Polarized thermal emission from narrow tungsten filaments, Nature 192(4799), 254–254 (1961).Google Scholar
Frischwasser K., Yulevich I., Kleiner V., Hasman E., Rashbalike spin degeneracy breaking in coupled thermal antenna lattices, Opt. Express 19(23), 23475–23482, Optical Society of America (2011).Google Scholar
Dahan N., Gorodetski Y., Frischwasser K., Kleiner V., Hasman E., Geometric Doppler Effect: Spin-Split Dispersion of Thermal Radiation, Phys. Rev. Lett. 105(13), 136402 (2010).Google Scholar
Bliokh K. Y., Niv A., Kleiner V., Hasman E., Geometrodynamics of spinning light, Nat. Photonics 2(12), 748–753, Nature Publishing Group (2008).Google Scholar
Hosten O., Kwiat P., Observation of the Spin Hall effect of light via weak measurements, Science (80-.). 319(5864), 787–790 (2008).Google Scholar
Shitrit N., Bretner I., Gorodetski Y., Kleiner V., Hasman E., Optical Spin Hall Effects in Plasmonic Chains, Nano Lett. 11(5), 2038–2042, American Chemical Society (2011).Google Scholar
Dooghin A. V., Kundikova N. D., Liberman V. S., Zel’dovich B. Y., Optical Magnus effect, Phys. Rev. A 45(11), 8204–8208 (1992).Google Scholar
Bliokh K. Y., Gorodetski Y., Kleiner V., Hasman E., Coriolis effect in optics: Unified geometric phase and Spin-Hall effect, Phys. Rev. Lett. 101(3), 030404 (2008).Google Scholar
Engel M., Steiner M., Lombardo A., Ferrari A. C., v. Lohneysen H., Avouris P., Krupke R., Löhneysen H. V., Avouris P., et al., Light-matter interaction in a microcavity-controlled graphene transistor, Nat. Commun. 3, 906, Nature Publishing Group (2012).Google Scholar
Dorgan V. E., Behnam A., Conley H. J., Bolotin K. I., Pop E., High-field electrical and thermal transport in suspended graphene, Nano Lett. 13(10), 4581–4586, American Chemical Society (2013).Google Scholar
Kim Y. D., Kim H., Cho Y., Ryoo J. H., Park C.-H., Kim P., Kim Y. S., Lee S., Li Y., et al., Bright visible light emission from graphene, Nat. Nanotechnol. 10(8), 676–681, Nature Publishing Group (2015).Google Scholar
Andreev V. M., Vlasov A. S., Khvostikov V. P., Khvostikova O. A., Gazaryan P. Y., Sorokina S. V., Sadchikov N. A., Solar Thermophotovoltaic Converters Based on Tungsten Emitters, J. Sol. Energy Eng. 129(3), 298 (2007).Google Scholar
Swanson R. M., A proposed thermophotovoltaic solar energy conversion system, Proc. IEEE 67(3), 446–447 (1979).Google Scholar
Spirkl W., Ries H., Solar thermophotovoltaics: An assessment, J. Appl. Phys. 57(9), 4409–4414, AIP (1985).Google Scholar
Ungaro C., Gray S. K., Gupta M. C., Solar thermophotovoltaic system using nanostructures, Opt. Express 23(19), A1149, Optical Society of America (2015).Google Scholar
Rephaeli E., Fan S., Absorber and emitter for solar thermophotovoltaic systems to achieve efficiency exceeding the Shockley-Queisser limit, Opt. Express 17(17), 15145–15159, OSA (2009).Google Scholar
Boriskina S. V., Chen G., Exceeding the solar cell Shockley-Queisser limit via thermal up-conversion of low-energy photons, Opt. Commun. 314, 71–78 (2014).Google Scholar
Seo T. H., Shin G., Kyoung Kim B., Choi C.-J., Lee C., Jong Kim M., Suh E.-K., Enhancement of light output power in ultraviolet light emitting diodes using graphene film on selfassembled Au nanocluster by agglomeration process, J. Appl. Phys. 114(22), 223105, AIP Publishing (2013).Google Scholar
Yen S.-T., Lee K.-C., Analysis of heterostructures for electroluminescent refrigeration and light emitting without heat generation, J. Appl. Phys. 107(5), 054513, AIP Publishing (2010).Google Scholar
Dousmanis G. C., Mueller C. W., Nelson H., Petzinger K. G., Evidence of Refrigerating Action by Means of Photon Emission in Semiconductor Diodes, Phys. Rev. 133(1A), A316–A318 (1964).Google Scholar
Berdahl P., Radiant refrigeration by semiconductor diodes, J. Appl. Phys. 58(3), 1369, AIP Publishing (1985).Google Scholar
Vavilov S. I., Photoluminescence and thermodynamics, J. Phys. USSR 10, 499–501 (1946).Google Scholar
Yu S.-Q., Wang J.-B., Ding D., Johnson S. R., Vasileska D., Zhang Y.-H., Impact of electronic density of states on electroluminescence refrigeration, Solid. State. Electron. 51(10), 1387–1390 (2007).Google Scholar
Lopez-Sanchez O., Alarcon Llado E., Koman V., Fontcuberta I Morral A., Radenovic A., Kis A., Light Generation and Harvesting in a van der Waals Heterostructure, Mesoscale and Nanoscale Physics, ACS Nano (2014).Google Scholar
Nemova G., Kashyap R., Laser cooling with PbSe colloidal quantum dots, J. Opt. Soc. Am. B 29(4), 676, Optical Society of America (2012).Google Scholar
Khurgin J. B., Role of bandtail states in laser cooling of semiconductors, Phys. Rev. B 77(23), 235206 (2008).Google Scholar
Zhang J., Li D., Chen R., Xiong Q., Laser cooling of a semiconductor by 40 kelvin, Nature 493(7433), 504–508, Nature Publishing Group, a division of Macmillan Publishers Limited. All Rights Reserved, (2013).Google Scholar
Khurgin J. B., Band gap engineering for laser cooling of semiconductors, J. Appl. Phys. 100(11), 113116, AIP Publishing (2006).Google Scholar
Khurgin J. B., Surface Plasmon-Assisted Laser Cooling of Solids, Phys. Rev. Lett. 98(17), 177401 (2007).Google Scholar
Martin R. P., Velten J., Stintz A., Malloy K. J., Epstein R. I., Sheik-Bahae M., Hasselbeck M. P., Imangholi B., Boyd S. T. P., et al., Nanogap experiments for laser cooling: a progress report, Proc. SPIE 6461, Laser Cool. Solids, 64610H (2007).Google Scholar
Li D., Zhang J., Wang X., Huang B., Xiong Q., Solid-state semiconductor optical cryocooler based on CdS nanobelts, Nano Lett. 14(8), 4724–4728, American Chemical Society (2014).Google Scholar
Chen Y.-C., Bahl G., Raman cooling of solids through photonic density of states engineering, Optica 2(10), 893, Optical Society of America (2015).Google Scholar
Manor A., Kruger N., Rotschild C., Entropy driven multiphoton frequency up-conversion, CLEO/QELS Conf. Proc., QF2D.1, Osa, Washington, D.C. (2013).Google Scholar
Buckner B. D., Heeg B., Power generation by thermally assisted electroluminescence: like optical cooling, but different, Proc. SPIE 6907, Laser Refrig. Solids, 69070I, 2008, 9 November 2015.Google Scholar
Ekins-Daukes N. J., Ballard I., Calder C. D. J., Barnham K. W. J., Hill G., Roberts J. S., Photovoltaic efficiency enhancement through thermal up-conversion, Appl. Phys. Lett. 82(12), 1974, AIP Publishing (2003).Google Scholar
Rousseau E., Laroche M., Greffet J.-J., Radiative heat transfer at nanoscale: Closed-form expression for silicon at different doping levels, J. Quant. Spectrosc. Radiat. Transf. 111(7/8), 1005–1014 (2010).Google Scholar
Ben-Abdallah P., Joulain K., Fundamental limits for noncontact transfers between two bodies, Phys. Rev. B 82(12), 121419 (2010).Google Scholar
Hu L., Narayanaswamy A., Chen X., Chen G., Near-field thermal radiation between two closely spaced glass plates exceeding Planck’s blackbody radiation law, Appl. Phys. Lett. 92(13), 133106 (2008).Google Scholar
Basu S., Francoeur, M., Near-field radiative transfer based thermal rectification using doped silicon, Appl. Phys. Lett. 98(11), 113106 (2011).Google Scholar
Miller O. D., Johnson S. G., Rodriguez A. W., Shapeindependent limits to near-field radiative heat transfer, Optics, 6 (2015).Google Scholar
Polder D., Van Hove M., Theory of Radiative Heat Transfer between Closely Spaced Bodies, Phys. Rev. B 4(10), 3303–3314 (1971).Google Scholar
Economou E. N., Surface Plasmons in Thin Films, Phys. Rev. 182(2), 539–554 (1969).Google Scholar
Miller O. D., Johnson S. G., Rodriguez A. W., Effectiveness of Thin Films in Lieu of Hyperbolic Metamaterials in the Near Field, Phys. Rev. Lett. 112(15), 157402 (2014).Google Scholar
Song B., Ganjeh Y., Sadat S., Thompson D., Fiorino A., Fernández-Hurtado V., Feist J., Garcia-Vidal F. J., Cuevas J. C., et al., Enhancement of near-field radiative heat transfer using polar dielectric thin films, Nat. Nanotechnol. 10(3), 253–258, Nature Publishing Group (2015).Google Scholar
Othman M. A. K., Guclu C., Capolino F., Graphene-based tunable hyperbolic metamaterials and enhanced near-field absorption, Opt. Express 21(6), 7614–7632 (2013).Google Scholar
Francoeur M., Mengüç M. P., Vaillon R., Local density of electromagnetic states within a nanometric gap formed between two thin films supporting surface phonon polaritons, J. Appl. Phys. 107(3), 034313, AIP Publishing (2010).Google Scholar
Liu X. L., Zhang R. Z., Zhang Z. M., Near-field thermal radiation between hyperbolic metamaterials: Graphite and carbon nanotubes, Appl. Phys. Lett. 103(21), 213102, AIP Publishing (2013).Google Scholar
Liu B., Shi J., Liew K., Shen S., Near-field radiative heat transfer for Si based metamaterials, Opt. Commun. 314, 57–65 (2014).Google Scholar
Novotny L., Hecht B., Principles of nano-optics, Cambridge University Press (2006).Google Scholar
Tian Z., Esfarjani K., Chen G., Enhancing phonon transmission across a Si/Ge interface by atomic roughness: Firstprinciples study with the Green’s function method, Phys. Rev. B 86(23), 235304, American Physical Society (2012).Google Scholar
Chiloyan V., Garg J., Esfarjani K., Chen G., Transition from near-field thermal radiation to phonon heat conduction at sub-nanometer gaps, Nat. Commun., 6755, Nature Publishing Group (2015).Google Scholar
De Wilde Y., Formanek F., Carminati R., Gralak B., Lemoine P.-A., Joulain K., Mulet J.-P., Chen Y., Greffet J.-J., Thermal radiation scanning tunnelling microscopy, Nature 444(7120), 740–743 (2006).Google Scholar
Jones A. C., Raschke M. B., Thermal infrared near-field spectroscopy, Nano Lett. 12(3), 1475–1481, American Chemical Society (2012).Google Scholar
Babuty A., Joulain K., Chapuis P.-O., Greffet J.-J., De Wilde Y., Blackbody Spectrum Revisited in the Near Field, Phys. Rev. Lett. 110(14), 146103 (2013).Google Scholar
Kittel A., Müller-Hirsch W., Parisi J., Biehs S.-A., Reddig D., Holthaus M., Near-Field Heat Transfer in a Scanning Thermal Microscope, Phys. Rev. Lett. 95(22), 224301 (2005).Google Scholar
Kryder M. H., Gage E. C., McDaniel T. W., Challener W. A., Rottmayer R. E., Erden M. F., Heat Assisted Magnetic Recording, Proc. IEEE 96(11), 1810–1835 (2008).Google Scholar
Stipe B. C., Strand T. C., Poon C. C., Balamane H., Boone T. D., Katine J. A., Li J.-L., Rawat V., Nemoto H., et al., Magnetic recording at 1.5 Pb m-2 using an integrated plasmonic antenna, Nat. Photonics 4(7), 484–488, Nature Publishing Group (2010).Google Scholar
Challener W. A., Peng C., Itagi A. V., Karns D., Peng W., Peng Y., Yang X., Zhu X., Gokemeijer N. J., et al., Heat-assisted magnetic recording by a near-field transducer with efficient optical energy transfer, Nat. Photonics 3(4), 220–224, Nature Publishing Group (2009).Google Scholar
Chen K., Santhanam P., Sandhu S., Zhu L., Fan S., Heat-flux control and solid-state cooling by regulating chemical potential of photons in near-field electromagnetic heat transfer, Phys. Rev. B 91(13), 134301 (2015).Google Scholar
Law S., Adams D. C., Taylor A. M., Wasserman D., Midinfrared designer metals, Opt. Express 20(11), 12155–12165, OSA (2012).Google Scholar
Naik G. V., Schroeder J. L., Ni X., Kildishev A. V., Sands T. D., Boltasseva A., Titanium nitride as a plasmonic material for visible and near-infrared wavelengths, Opt. Mater. Express 2(4), 478–489, OSA (2012).Google Scholar
Naik G. V., Kim J., Boltasseva A., Oxides and nitrides as alternative plasmonic materials in the optical range, Opt. Mater. Express 1(6), 1090–1099, OSA (2011).Google Scholar
Kats M. A., Sharma D., Lin J., Genevet P., Blanchard R., Yang Z., Qazilbash M. M., Basov D. N., Ramanathan S., et al., Ultrathin perfect absorber employing a tunable phase change material, Appl. Phys. Lett. 101(22), 221101, AIP Publishing (2012).Google Scholar
Qazilbash M. M., Brehm M., Chae B.-G., Ho P.-C., Andreev G. O., Kim B.-J., Yun S. J., Balatsky A. V., Maple M. B., et al., Mott Transition in VO2 Revealed by Infrared Spectroscopy and Nano-Imaging, Science (80-.). 318(5857), 1750–1753 (2007).Google Scholar
Kats M. A., Blanchard R., Zhang S., Genevet P., Ko C., Ramanathan S., Capasso F., Vanadium Dioxide as a Natural Disordered Metamaterial: Perfect Thermal Emission and Large Broadband Negative Differential Thermal Emittance, Phys. Rev. X 3(4), 041004 (2013).Google Scholar
Otanicar T. P., Smith R., Dai L., Phelan P. E., Swaminathan R., Applicability of Controllable Nanoparticle Radiative Properties for Spacecraft Heat Rejection, J. Thermophys. Heat Transf., 1–6, American Institute of Aeronautics and Astronautics (2015).Google Scholar
Inoue T., De Zoysa M., Asano T., Noda S., Realization of dynamic thermal emission control, Nat. Mater. 13(10), 928–931, Nature Publishing Group (2014).Google Scholar
Brar V. W., Sherrott M. C., Jang M. S., Kim S., Kim L., Choi M., Sweatlock L. A., Atwater H. A., Electronic modulation of infrared radiation in graphene plasmonic resonators, Nat. Commun. 6, 7032, Nature Publishing Group (2015).Google Scholar
Huang Y., Boriskina S. V., Chen G., Electrically tunable nearfield radiative heat transfer via ferroelectric materials, Appl. Phys. Lett. 105(24), 244102, AIP Publishing (2014).Google Scholar
Paik T., Hong S.-H., Gaulding E. A., Caglayan H., Gordon T. R., Engheta N., Kagan C. R., Murray C. B., Solution-processed phase-change VO(2) metamaterials from colloidal vanadium oxide (VO(x)) nanocrystals, ACS Nano 8(1), 797–806, American Chemical Society (2014).Google Scholar
Yi F., Shim E., Zhu A. Y., Zhu H., Reed J. C., Cubukcu E., Voltage tuning of plasmonic absorbers by indium tin oxide, Appl. Phys. Lett. 102(22) (2013).Google Scholar
Chen Y. G., Kao T. S., Ng B., Li X., Luo X. G., Luk’yanchuk B., Maier S. A., Hong M. H., Hybrid phase-change plasmonic crystals for active tuning of lattice resonances, Opt. Express 21(11), 13691–13698, Optical Society of America (2013).Google Scholar
Lee H.-J., Smyth K., Bathurst S., Chou J., Ghebrebrhan M., Joannopoulos J., Saka N., Kim S.-G., Hafnia-plugged microcavities for thermal stability of selective emitters, Appl. Phys. Lett. 102(24), 241904, American Institute of Physics (2013).Google Scholar
Ladutenko K., Belov P., Peńa Rodríguez O., Mirzaei A., Miroshnichenko A., Shadrivov I., Superabsorption of light by nanoparticles, Nanoscale, The Royal Society of Chemistry (2015).Google Scholar
Mirzaei A., Shadrivov I., Miroshnichenko A., Kivshar Y. S., Superabsorption of Light by Multilayer Nanowires, Nanoscale 7(42), 17658–17663, The Royal Society of Chemistry (2015).Google Scholar
Simovski C., Maslovski S., Nefedov I., Kosulnikov S., Belov P., Tretyakov S., Hyperlens makes thermal emission strongly super-Planckian, Photonics Nanostructures – Fundam. Appl. 13, 31–41 (2015).Google Scholar
Ding D., Minnich A. J., Selective radiative heating of nanostructures using hyperbolic metamaterials, Opt. Express 23(7), A299–A308, Optical Society of America (2015).Google Scholar
Zhou M., Shi L., Zi J., Yu Z., Extraordinarily Large Optical Cross Section for Localized Single Nanoresonator, Phys. Rev. Lett. 115(2), 023903 (2015).Google Scholar
Moitra P., Yang Y., Anderson Z., Kravchenko I. I., Briggs D. P., Valentine J., Realization of an all-dielectric zero-index optical metamaterial, Nat. Photonics 7(10), 791–795, Nature Publishing Group (2013).Google Scholar
Dong J.-W., Chang M.-L., Huang X.-Q., Hang Z. H., Zhong Z.-C., Chen W.-J., Huang Z.-Y., Chan C. T., Conical Dispersion and Effective Zero Refractive Index in Photonic Quasicrystals, Phys. Rev. Lett. 114(16), 163901 (2015).Google Scholar
Boriskina S. V., Quasicrystals: Making invisible materials, Nat. Photonics 9(7), 422–424, Nature Publishing Group (2015).Google Scholar
Huang X., Lai Y., Hang Z. H., Zheng H., Chan C. T., Dirac cones induced by accidental degeneracy in photonic crystals and zero-refractive-index materials, Nat. Mater. 10(8), 582–586, Nature Publishing Group (2011).Google Scholar
Boriskina S. V., Povinelli M., Astratov V. N., Zayats A. V., Podolskiy V. A., Collective phenomena in photonic, plasmonic and hybrid structures, Opt. Express 19(22), 22024 (2011).Google Scholar
Zhou M., Yi S., Luk T. S., Gan Q., Fan S., Yu Z., Analog of superradiant emission in thermal emitters, Phys. Rev. B 92(2), 024302 (2015).Google Scholar
Sokhoyan R., Atwater H. A., Cooperative behavior of quantum dipole emitters coupled to a zero-index nanoscale waveguide, Optics, ArXiV (2015).Google Scholar
Narayanaswamy A., Zheng Y., Theory of thermal nonequilibrium entropy in near-field thermal radiation, Phys. Rev. B 88(7), 075412 (2013).Google Scholar
Barnett S. M., Phoenix S. J. D., Entropy as a measure of quantum optical correlation, Phys. Rev. A 40(5), 2404–2409 (1989).Google Scholar
Maghrebi M. F., Jaffe R. L., Kardar M., Nonequilibrium quantum fluctuations of a dispersive medium: Spontaneous emission, photon statistics, entropy generation, and stochastic motion, Phys. Rev. A – At. Mol. Opt. Phys. 90(1) (2014).Google Scholar
Klembt S., Durupt E., Datta S., Klein T., Baas A., Léger Y., Kruse C., Hommel D., Minguzzi A., et al., Exciton-Polariton Gas as a Nonequilibrium Coolant, Phys. Rev. Lett. 114(18), 186403 (2015).Google Scholar
Bowman S. R., Lasers without internal heat generation, IEEE J. Quantum Electron. 35(1), 115–122 (1999).Google Scholar
Nemova G., Kashyap R., Thin-disk athermal laser system, Opt. Commun. 319, 100–105 (2014).Google Scholar
Tolman R. C., Fine P. C., On the irreversible production of entropy, Rev. Mod. Phys. 20(1), 51–77, American Physical Society (1948).Google Scholar
Mungan C. E., Thermodynamics of radiation-balanced lasing, 1075–1082 (2003).Google Scholar