# Absorption by an Optical Dipole Antenna in a Structured Environment

Authors: E. Castanié; R. Vincent; R. Pierrat; R. Carminati
Journal: International Journal of Optics
 (2012)

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## Abstract

We compute generalized absorption and extinction cross-sections of an optical dipole nanoantenna
in a structured environment. The expressions explicitly show the influence of radiation reaction and
the local density of states on the intrinsic absorption properties of the antenna. Engineering the
environment could allow to modify the overall absorption as well as the frequency and the linewidth
of a resonant antenna. Conversely, a dipole antenna can be used to probe the photonic environment,
in a similar way as a quantum emitter.


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## Body

## 1. Introduction

It is well known that the emission frequency and linewidth of a dipole quantum emitter is modified by its local environment [1–4]. The linewidth directly depends on the photonic local density of states (LDOS) which accounts for the number of radiative and nonradiative channels available for the emitter to relax in the ground state. The change in the emission frequency and linewidth induced by the environment can be described by considering the transition dipole as a classical dipole oscillator [2, 4]. Therefore, similar behaviors are expected for a dipole antenna (or a nanoparticle) interacting with its environment, the involved dipole being in this case the induced dipole that is responsible for scattering and absorption. Indeed, changes in the induced dipole dynamics in optical antennas have already been observed [5, 6], and the parallel with spontaneous emission dynamics has been mentioned on a qualitative phenomenological ground. Energy shifts and linewidths of plasmonic nanoparticles have also been discussed recently, based on general properties of damped harmonic oscillators [7]. A connection between LDOS maps and the scattering pattern of plasmonic structures has been established in a specific imaging configuration [8]. In this context, it seems that a general discussion of the influence of the environment on the absorption of an optical dipole antenna or nanoparticle would be useful. The purpose of this paper is to address this question, using a rigorous framework based on scattering theory, and to illustrate the conclusions on a simple example.In this paper, we investigate the role of the environment on the absorption cross-section of an optical dipole antenna using a rigorous theoretical framework. We show that it is possible to modify the overall absorption and its spectral properties by engineering the environment, and in particular the photonic LDOS. Conversely, it is possible to probe the environment using a resonant nanoantenna, specific measurements being able to produce LDOS maps. In Sections2 and 3, we derive the exact expressions of the dressed electric polarizability of a dipole antenna in an arbitrary environment and deduce the expression of the generalized absorption and extinction cross-sections. In Section 4, we discuss qualitatively the physical mechanisms affecting both the resonance frequency and the linewidth of a resonant antenna, using a simplified model. In Section 5 we study numerically a simple but realistic example, based on the rigorous expression derived in Section 2. This allows us to illustrate the general trends and to give orders of magnitude. In Section 6, we summarize the main conclusions.


## 2. Dressed Polarizability

This section is devoted to the computation of the dressed polarizability of an optical dipole antenna or nanoparticle (i.e., the polarizability that accounts for the interaction with the environment). To proceed, we follow the same procedure that has been used previously to compute the polarizability in vacuum [9–11]. We consider an electrically small particle (the generic term particle will be used to denote either a subwavelength optical antenna or a nanoparticle) of volume V and of permittivity ε(ω) embedded in an arbitrary environment, the particle lying at position r0 (see Figure 1). We assume that position r0 lies in vacuum (the local refractive index at r0 is assumed to be unity). To describe light propagation in the environment, we use the electric dyadic Green function G which connects the electric field at position r to an electric dipole source at point r′ through the relation E(r,ω)=μ0ω2G(r,r′,ω)p(r′). We denote by Eext the field in the environment in the absence of the particle (exciting field). The total electric field E at point r and at frequency ω reads(1)E(r,ω)=Eext(r,ω)+k02∫VG(r,r′,ω)[ε(ω)-1]×E(r′,ω)d3r′,
where k0=ω/c, c being the speed of light in vacuum. The approximation of electrically small particle amounts to considering that the electric field is uniform inside the particle. Under this condition, the expression of the total electric field inside the particle (at point r0) becomes(2)E(r0,ω)=Eext(r0,ω)+k02[ε(ω)-1]E(r0,ω)×∫VG(r0,r′,ω)d3r′.
We now split the integral of the Green dyadic into its singular part -L/k02 and its nonsingular part VGreg(r0,r0,ω) where we have assumed that Greg(r0,r′,ω) is constant over the volume of the nanoparticle. Note that L is real since it corresponds to the singularity of the Green tensor at a point that lies in vacuum (the Green tensor is computed in the absence of the particle) [12–14]. Equation (2) becomes(3)E(r0,ω)={k02V[ε(ω)-1]Greg(r0,r0,ω)I+[ε(ω)-1]L-k02V[ε(ω)-1]Greg(r0,r0,ω)}-1Eext(r0,ω).
The expression of the polarizability follows be writing the induced electric dipole moment of the particle in the form(4)p(r0,ω)=∫VP(r′,ω)d3r′=Vϵ0[ϵ(ω)-1]E(r0,ω)=ϵ0α(ω)Eext(r0,ω).
The last line defines the dressed polarizability α(ω), that in the most general situation is a tensor. Inserting (3) into (4), one obtains(5)α(ω)=V[ϵ(ω)-1]×{I+[ϵ(ω)-1]L-k02V[ϵ(ω)-1]Greg(r0,r0,ω)}-1.
A more useful expression of the dressed polarizability is obtained by defining a reference polarizablity α0(ω). A usual choice for this reference is the quasi-static polarizability of the particle in vacuum [11], that reads(6)α0(ω)=V[ϵ(ω)-1]{I+[ϵ(ω)-1]L}-1.
Note that in the case of a spherical particle, the singularity (or depolarization) dyadic is L=I/3 so that α0(ω) would simplify into the well-known (scalar) quasi-static expression α0=3V(ϵ-1)/(ϵ+2). Using (5) and (6), the dressed polarizability has the final form:(7)α(ω)=α0(ω){I-k02Greg(r0,r0,ω)α0(ω)}-1.
This expression is the main result of this section. It shows that the dressed polarizability of a particle depends on the environment, the influence of the environment being fully described by the non-singular part of the dyadic Green function VGreg(r0,r0,ω). Note that (7) is the explicit expression of the effective polarizability discussed in [4].Figure 1
Optical dipole antenna of arbitrary shape in a structured environment. A pointr0 inside the antenna is used to define its position.For a resonant antenna or nanoparticle (e.g., supporting a plasmon resonance), it is instructive to rewrite (7) in the form:(8)α(ω)-1=α0(ω)-1-k02Greg(r0,r0,ω).
The resonance frequency of the dressed polarizability is solution of the equation Re[α0-1(ω)-k02Greg(r0,r0,ω)]=0, while the linewidth is given by Im[α0-1(ω)-k02Greg(r0,r0,ω)]. The influence of the environment on the resonance lineshape is made explicit by this simple analysis.


## 3. Generalized Absorption and Extinction Cross-Sections

The expression of the dressed polarizability is the starting point to compute generalized absorption and extinction cross-sections in an arbitrary environment. To carry out this derivation, we start with the expression of the time-averaged power absorbed inside the particle, given by(9)Pa=12∫VRe[j(r′,ω)⋅E*(r′,ω)]d3r′,
where j(r′,ω)=-iωϵ0[ϵ(ω)-1]E(r′,ω) is the current density induced in the particle. As the electric field is assumed to be uniform inside the particle, the absorbed power becomes(10)Pa=ωVϵ0Im⁡ϵ(ω)2|E(r0,ω)|2.
Using (4), it can be rewritten as(11)Pa=ωϵ0Im⁡ϵ(ω)2V|ϵ(ω)-1|2|α(ω)Eext(r0,ω)|2.
To define a generalized absorption cross-section, we have to introduce an incident local energy flux ϕext. Since the exciting field at the position of the particle is Eext(r0,ω), we define the incident local energy flux using the expression for a plane wave ϕext=|Eext(r0,ω)|2/(2μ0c). This definition is arbitrary, but has the advantage to coincide with the standard one when the particle lies in a homogeneous medium. The generalized absorption cross-section is then given by the ratio Pa/ϕext. Using the relation Im[α0][α0α0*]-1=Imϵ(ω)/[V|ϵ(ω)-1|2]I (see Appendix A for a proof), we obtain the final expression of the generalized absorption cross-section:(12)σa(ω)I=k0Im⁡[α0(ω)][α0(ω)α0*(ω)]-1|α(ω)Eext(r0,ω)|2|Eext(r0,ω)|2.
Equation (12) is a central result of this paper. It deserves some remarks before we analyze its consequences. Although (12) involves tensor notations, the absorption cross-section σa(ω) is a scalar quantity. Expression (12) is exact and has been obtained under the only assumption that the electric field is uniform inside the particle (approximation of electrically small particle). It can be used, together with (7), to discuss the influence of the environment on the optical properties of any particle (or antenna) satisfying this condition. For a nonabsorbing material, the imaginary part of the permittivity ϵ(ω) vanishes, and the quasi-static polarizability α0 is real. The term Im[α0(ω)] in (12) implies σa(ω)=0, as it should be. Finally, let us emphasize that the generalized absorption cross-section that we have defined really describes the change of the intrinsic absorption of the particle induced by the environment (or in other word of the absorption probability given a local incident power). Its proper normalization by the local incident energy flux clearly distinguishes this effect on the absorbed power from that due to a mere change of the local incident power. It is also important to stress that although the generalized absorption cross-section that we have defined is a scalar, it depends on the orientation of the local exciting electric field, that encodes the anisotropy of the environment.Following the same procedure, it is also possible to compute the extinction cross-section, starting from the expression of the power extracted from the external field by the nanoparticle. The latter can be written in the form [11]:(13)Pe=12∫VRe[j(r′,ω)⋅Eext*(r′,ω)]d3r′.
One obtains(14)σe=k0Im⁡[α(ω)Eext(r0,ω)⋅Eext*(r0,ω)]|Eext(r0,ω)|2.
As for the generalized absorption cross-section, this expression is exact under the assumption of an electrically small particle. In the following, we will focus our attention on the absorption cross-section, but the analyses and the general trends can be translated to the extinction situation, that can be relevant to specific experimental configurations and type of measurements.


## 4. Qualitative Discussion

Equation (12) can be used to compute the absorption cross-sections in a given environment. For realistic geometries, the computation can only be performed numerically (we will study a simple example in Section 5). For example, it is possible to use an iteration scheme to solve numerically the Dyson equation which is the closed form of the equation governing the Green function similar to (1) [15]. Nevertheless, in order to get some insight based on simple analytical formulas, we will study an oversimplified situation. First, we consider a spherical nanoparticle of volume V, small enough to be consistent with the electric dipole approximation that we use throughout this paper. For such a shape, the singular part of the Green tensor is simply given by L=I/3 [12, 13]. Second, we assume that the nanosphere is embedded in an environment that preserves for Greg(r0,r0,ω) the same symmetry as that of free space (i.e., Greg(r0,r0,ω)=Greg(r0,r0,ω)I). This is an unrealistic hypothesis (it would be strictly valid only for a homogeneous medium or a medium with cubic symmetry), but we shall use it only to discuss qualitatively general trends. Under these hypotheses, the quasi-static polarizability reduces to α0(ω)=3V[ϵ(ω)-1]/[ϵ(ω)+2], and the dressed polarizability takes the form:(15)α(ω)=α0(ω)1-k02Greg(r0,r0,ω)α0(ω).
The absorption cross-section becomes(16)σa(ω)=k0Im⁡[α0(ω)]|α(ω)|2|α0(ω)|2.
It is clear in this expression that in absence of polarization anisotropy induced by the environment, the absorption cross-section does not depend on the exciting field (this is not the case in (12)).In order to get a simple model of a resonant optical dipole antenna, we consider a metallic nanoparticle described by Drude permittivityϵ(ω)=1-ωp2/(ω2+iωγ), where ωp is the plasma frequency, and γ is the intrinsic collision rate that describes absorption losses in the bulk material. The real and imaginary parts of the Green tensor, that both influence the absorption cross-section, have a well-defined meaning. In order to make this more explicit, we introduce the photonic LDOS ρ(r0,ω), connected to the imaginary part of the Green tensor by(17)ρ(r0,ω)=6ωπc2Im⁡[Greg(r0,r0,ω)].
We also introduce ϕ(r0,ω) that describes the influence of the real part of the non-singular Green tensor in a similar way:(18)ϕ(r0,ω)=6ωπc2Re[Greg(r0,r0,ω)].
Using these definitions, the dressed polarizability of the metallic nanoparticle reads(19)α(ω)=3Vω02[ω02{1-π2Vωϕ(r0,ω)}-ω2-iω{γ+π2Vω02ρ(r0,ω)}]-1,
where ω0=ωp/3 is the plasmon resonance frequency of the bare nanoparticle in the quasi-static limit. This expression naturally leads to the introduction of an effective frequency Ωeff2(ω)=ω02{1-πVωϕ(r0,ω)/2} such that the resonant frequency of the particle in the environment is solution of the equation Ωeff2(ω)-ω2=0. Similarly, an effective linewidth γeff(ω)=γ+πVω02ρ(r0,ω)/2 can be introduced.From (12) and (19), we can obtain the expression of the absorption cross-section in the simplified scalar model:(20)σa(ω)=3Vω02cω2γ[Ωeff2(ω)-ω2]2+ω2γeff2(ω).
Equation (20), together with the expressions of Ωeff(ω) and γeff(ω), shows that the real part of the Green function contributes to a change of the resonance frequency, while the imaginary part (the LDOS) changes the linewidth. This is the same behavior as that known for a dipole emitter (either quantum or classical), although in the present situation we deal with the dipole induced inside the particle by the external field. It is interesting to note that the effective line width γeff(ω) can only be larger than the intrinsic linewidth γ because of its dependance on the LDOS which is a positive quantity.The resonant behavior ofσa(ω) and the influence of the LDOS (through γeff(ω)) deserve to be analyzed more precisely. Due to the frequency dependence of both Ωeff(ω) and γeff(ω), the resonance lineshape is in general not a Lorentzian profile. Moreover, Ωeff(ω) and γeff(ω) are not independent, since the real and imaginary parts of the Green function are connected by Kramers-Kronig relations. It is nevertheless possible to derive the expression of the generalized absorption cross-section at resonance. The resonance frequency ωa satisfies dσa(ωa)/dω=0. As described in Appendix B, using this implicit equation, it is possible to express σa(ωa) in the form:(21)σa(ωa)=3γVω02c×[ωa4[Ωeff2(ωa)-2ωaΩeff′(ωa)Ωeff(ωa)+ωa2]2γeff2(ωa){ωa4[Ωeff2(ωa)-2ωaΩeff′(ωa)Ωeff(ωa)+ωa2]21+ωa4[Ωeff2(ωa)-2ωaΩeff′(ωa)Ωeff(ωa)+ωa2]2×γeff′2(ωa)ωa4[Ωeff2(ωa)-2ωaΩeff′(ωa)Ωeff(ωa)+ωa2]2}]-1,
where the superscript ' denotes a first-order derivative. This expression shows that both the LDOS and its first-order derivative influence the amplitude of the generalized absorption cross-section, through γeff2(ωa) and γeff′2(ωa), respectively. An increase of both quantities tends to decrease the absorption cross-section. In the particular case of an environment for which the spectral dependence of the LDOS can be neglected [γeff′2(ω)=0], we end up with σa(ωa)∝1/γeff2(ωa). This result can be qualitatively explained in simple terms. The first step in the absorption process by a metallic nanoparticle is the excitation of the conduction electron gas. Then, relaxation can occur either by radiative (emission of scattered light) or nonradiative channels (absorption due to electron-phonon collisions). Increasing the photonic LDOS increases the weight of radiative channels and therefore reduces absorption. The role of the LDOS in this process is essentially the same as that in the spontaneous decay rate of a quantum emitter by coupling to radiation.


## 5. Metallic Nanoparticle Interacting with a Perfect Mirror

In order to illustrate the effects discussed above on a real example and to get orders of magnitudes (i.e., to establish the possibility of experiments), we study quantitatively in this section the generalized absorption cross-section of a silver nanosphere, with radiusR=15nm, interacting with a flat perfectly conducting surface (perfect mirror). The geometry of the system is shown in Figure 2. To describe the silver nanoparticle, we use the tabulated values of the bulk permittivity ϵ(ω) taken from [16].Figure 2
Geometry of the system: A spherical dipole nanoparticle interacts with a perfect mirror. The dashed sphere corresponds to the image dipole.To compute the generalized absorption cross-section of the nanosphere, we use the exact expression equation (12). In order to compute relative changes, we define the normalized cross-section σan(ω)=σa(ω)/σavac(ω), where σavac(ω) is the absorption cross-section of the bare nanosphere in vacuum:(22)σavac(ω)=k0Im⁡[α0(ω)]|αvac(ω)α0(ω)|2.
The vacuum polarizability αvac(ω) is given by(23)αvac=α0(ω){1-ik036πα0(ω)}-1,
with α0(ω)=3V[ϵ(ω)-1]/[ϵ(ω)+2] [10, 11]. The calculation of σan(ω) requires the calculation of the exciting field Eext and of the Green function Greg(r0,r0,ω) in the geometry in Figure 2. This is a straightforward application of the image method, given in Appendix C for completeness.We show in Figure3(a) the variations of normalized LDOS (ratio between the full LDOS and the LDOS in vacuum) versus both the wavelength and the distance d between the mirror and the center of the nanoparticle. Figure 3(b) (red solid line) displays a section corresponding to λ=400 nm in Figure 3(a). We observe the well-known oscillations due to interferences between incident and reflected waves on the mirror [2]. In the near-field regime corresponding to d≪λ, the relative variations of the LDOS are on the order of 10%. These plots of the LDOS will be helpful in the qualitative analysis of the variations of the generalized absorption cross-section.(a) map of the normalized LDOSρ(r0,ω)/ρvac(ω), with ρ(r0,ω)=2ω/(πc2)Im[TrGreg(r0,r0,ω)] and ρvac(ω) the LDOS in vacuum, versus both the wavelength λ and the distance d between the mirror and the center of the nanoparticle. The vertical dashed line is a guide to precise the wavelength at which panel (b) has been plotted. (b) distance dependence of the LDOS (red solid line) and of the partial LDOS (blue and black dashed lines) defined by ρii(r0,ω)=2ω/(πc2)Im[Greg,ii(r0,r0,ω)] with i=x,y,z for λ=400nm. The partial LDOS ρii(r0,ω) drives the dynamics of a dipole oriented along direction i, while the LDOS sums up the contributions of the three orientations. Due to symmetry in the geometry in Figure 2, the partial LDOS along x and y is equal. In all calculations, the minimum distance d≃2R has been chosen at the limit of validity of the dipole approximation [17].
(a)(b)To study the influence of the mirror onσa(ω), we first consider an s-polarized illumination (the incident plane wave has an electric field linearly polarized along the direction y). In this case, the induced electric dipole in the nanosphere is oriented along y. As a consequence, σa(ω) is independent of the direction of incidence (angle θ in Figure 2). In Figure 4(a), we represent the variations of the normalized absorption cross-section σan(ω) (generalized absorption cross-section divided by free-space cross-section) versus both the wavelength λ and the distance d between the mirror and the center of the nanoparticle. The plasmon resonance, corresponding to λ≃360 nm, is visible for d<100 nm. Figure 4(b) displays a section view of Figure 4(a) at λ=361 nm. We observe oscillations of the absorption cross-section, as a clear signature of the influence of the mirror. The relative variations are on the order of 5% for distances d between 50 and 250nm. The behavior of σan(ω) can be compared to that of the partial LDOS ρyy(r0,ω) in Figure 3(b). The oscillations are in opposition, in agreement with the qualitative analysis presented in Section 4: An increase of the LDOS tends to decrease the absorption cross-section.(a) map of the normalized absorption cross-sectionσan versus both the wavelength λ and the distance d between the mirror and the nanosphere. The vertical dashed line is a guide to precise the wavelength at which panel (b) has been plotted. Inset: plot of the absorption cross-section as a function of the wavelength for d=30nm. (b) plot of σan and of the partial LDOS ρyy(r0,ω) versus the distance d for λ=361nm. s-polarized illumination.
(a)(b)The case of an illumination with ap-polarized plane wave (i.e., with an electric field in the x-z plane) can be analyzed in a similar manner. In this case, the electric dipole induced in the nanosphere depends on the direction of incidence θ. We have chosen θ=45° for the sake of illustration (note that θ=0 would lead to the same behavior as that observed with s-polarized illumination). Figures 5(a) and 5(b) are the same as Figures 4(a) and 4(b), but for p-polarized illumination. We observe a similar behavior of σan, with oscillations corresponding to relative variations of a few percent. Close to resonance, and for d=30nm (which corresponds to strong nanoparticle mirror interaction in this simple system), the relative variation of the absorption cross-section is of the order of 20%. Finally, let us note that significant changes are observed in the near-field regime only. For d>λ/2, the influence of interactions with the environment remains weak.(a) same as Figure4 for an illumination with a p-polarized plane wave, at an angle of incidence θ=45o. Both the partial LDOS ρxx(r0,ω) and ρzz(r0,ω) are displayed in (b) since both influence the generalized cross-section in this situation.
(a)(b)


## 6. Conclusion

We have described the influence of the environment on the absorption cross-section of an optical dipole antenna or a nanoparticle, based on a rigorous framework. We have derived a generalized form of the absorption cross-section, based on the only assumption that the electric field is uniform inside the antenna (electric dipole approximation). In the case of a resonant nanoparticle (plasmon resonance), we have analyzed qualitatively the role of the environment on the resonance frequency and on the linewidth. In particular, we have identified the role of the photonic LDOS and shown that an increase of the LDOS results in a reduction of the generalized absorption cross-section. These effects have been illustrated on the simple example of a metallic nanoparticle interacting with a perfect mirror. In the field of optical nanoantennas, these results could be exploited along two directions. First, engineering the LDOS around an optical nanoantenna could allow some control of both the resonance frequency, and more interestingly on the level of absorption. Since high absorption remains a serious drawback of metallic nanoantenna, it might be possible to reduce absorption by an appropriate structuration of the environment. Second, measuring changes in the resonance lineshape of a metallic nanoparticle, as performed, for example, in [18], should allow a direct mapping of the LDOS, without using fluorescent emitters. Finally, let us comment on the possibility of measuring σain situ. A potential method could be based on photothermal detection, in which a probe beam probes the temperature increase of the nanoparticle due to absorption. Such methods already offer the possibility of sensitive detection of nanoparticles in complex environments [19–22].



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