Diffuse Surface Scattering in the Plasmonic Resonances of Ultra-Low Electron Density Nanospheres

Diffuse Surface Scattering in the Plasmonic Resonances of Ultra-Low Electron Density Nanospheres

Abstract

Localized surface plasmon resonances (LSPRs) have recently been identified in extremely diluted electron systems obtained by doping semiconductor quantum dots. Here we investigate the role that different surface effects, namely electronic spill-out and diffuse surface scattering, play in the optical properties of these ultra-low electron density nanosystems. Diffuse scattering originates from imperfections or roughness at a microscopic scale on the surface. Using an electromagnetic theory that describes this mechanism in conjunction with a dielectric function including the quantum size effect, we find that the LSPRs show an oscillatory behavior both in position and width for large particles and a strong blueshift in energy and an increased width for smaller radii, consistent with recent experimental results for photodoped ZnO nanocrystals. We thus show that the commonly ignored process of diffuse surface scattering is a more important mechanism affecting the plasmonic properties of ultra-low electron density nanoparticles than the spill-out effect.

Diffuse surface scattering, localized surface plasmon resonances, semiconductor quantum dots
\alsoaffiliation

Department of Applied Physics and Gothenburg Physics Centre, Chalmers University of Technology, SE-412 96 Göteborg, Sweden

Surface plasmons in metals have been studied for a long time Ritchie (1957); Raether (1998); Liebsch (1997). However, in the last few years, the behavior of plasmon resonances in nanosystems has become a hot topic due to numerous applicationsMaier (2007), having been made possible by considerable progress in both calculating and measuring the optical properties of nanoparticles. A particularly interesting example concerns the energy shift experienced by the localized surface plasmon resonances (LSPRs) of nanospheres as a function of the size, as well as the corresponding modification in the plasmon width Scholl et al. (2012); Raza et al. (2013); Peng et al. (2010); Baida et al. (2009); Townsend and Bryant (2012); Lermé et al. (2010).

Recently, it was discovered that doped semiconductor quantum dots with a high concentration of carriers in the conduction band show, when illuminated, absorption resonances attributed to the excitation of surface plasmons Luther et al. (2011); Buonsanti et al. (2011); Naik et al. (2012); Faucheaux and Jain (2013); Faucheaux et al. (2014); Schimpf et al. (2014). Not only are doped semiconductor nanocrystals emerging as a new class of plasmonic structures for their remarkable properties of tuning and switching on/off the plasmon energy Faucheaux and Jain (2013); Faucheaux et al. (2014); ? The density of electrons in such nanocrystals is low, typically two to three orders of magnitude lower than in typical metals. In terms of the classic density parameter , being the carrier density, which in units of the Bohr radius is 2-6 for common metals, in doped semiconductors is on the order of 25. Such a diluted electron gas has its absorption band in the infrared rather than in the visible part of the electromagnetic spectrum.

In previous publications Monreal et al. (2013, 2014) we analyzed how the so-called surface spill-out effect modifies the position and width of plasmonic resonances in Ag and Au nanospheres of radii smaller than 10 nm embedded in different dielectric matrices. This effect originates from the fact that the electronic density of typical high electron density metals does not have a sharp discontinuity at the geometrical surface, as assumed by the classical theory. Rather, it is a continuous function because the surface potential barrier confining the electrons is finite and smooth. These studies omitted another surface mechanism which affects local surface plasmon resonances in any geometry, and is associated with the existence of imperfections or roughness at a microscopic scale on the surface. As a consequence, some of the metal electrons arriving at the surface are reflected back in any direction Flores and García-Moliner (1977); Monreal et al. (1980, 1982). The origin of the phenomenon can be better understood in the case of planar surfaces. For an ideally flat surface, the translational invariance of space in the direction parallel to the surface implies conservation of the parallel momentum and, therefore, conservation of the parallel component of the electric current (specular scattering). However, this restriction is lifted for non-ideal surfaces, where it is possible to have diffuse scattering, and, consequently, fluctuations in the parallel current. This mechanism affects any physical phenomenon taking place at a surface and, in particular, will lead to energy broadening of the LSPRs since it breaks coherence of single scattering events. For planar surfaces or spheres with typical metallic electronic densities, the spill-out mechanism dominates over the diffuse surface scattering one at the frequencies of the surface plasmon modes, this being the reason why the second mechanism is generally neglected Feibelman (1982). However, imperfections in the shape and morphology of ultra small particles are frequent and constitute an important source for diffuse surface scattering, particularly for the low-density electron systems that we will study in this work. Similar behavior can be produced by adsorbed molecules Persson (1993); Mogensen and Kneipp (2014).

The purpose of this article is to investigate the role that spill-out and diffuse surface scattering play in the optical properties of ultra-low electron density nanosystems. Using an electromagnetic theory that describes diffuse surface scattering in conjunction with a dielectric function that includes the effect of quantization due to the small size of the particles, we find that the LSPRs show an oscillatory behavior both in position and width for particles larger than ca. 3 nm in radius and a strong blueshift in energy and an increased width for smaller radii, consistent with recent experimental results Schimpf et al. (2014). We thus show that the commonly ignored process of diffuse surface scattering is an important mechanism affecting the plasmonic properties of these systems. Based on our theory, we can also extract an effective length characterizing diffuse surface scattering which can be included in an effective dielectric function and used in simpler models.

Surface scattering mechanisms affecting the electromagnetic response of metal surfaces can be described by means of two effective complex lengths, and , where is the frequency. These are surface response functions associated with changes across the surface of the normal component of the electric field vector and of the parallel component of the displacement vector with respect to their classical counterparts, respectively Feibelman (1982). The length can be related to the electronic charge density, , induced at the surface by any external perturbation and describes the spill-out effect, while diffuse surface scattering, which provokes fluctuations in the current parallel to the metal surface, is described by ( for specular scattering) Feibelman (1982). For the case of a sphere of radius , the corresponding lengths are denoted as and and, by considering the mentioned changes in and across the sphere surface respectively, it was shown Apell and Ljungbert (1982); Apell and Penn (1983) that, in the quasi-static limit , the polarizability of the sphere can be written as

(1)

Then, in the same quasi-static limit, the optical absorption cross section can be calculated as

(2)

where is the speed of light. In eqs. (1) and (2), is the classical, local permittivity of the metal and is a frequency independent permittivity of the surrounding medium. Note that if surface effects are neglected ( and in eq. (1)), the classical results of the Mie theory are recovered.

The role that these two lengths play in the effective relaxation time of the surface plasmons in small spheres with typical electron densities characterized by 2, 3 and 4, was analyzed in Ref. Apell et al. (1984). At these densities the spill-out contribution to the surface plasmon relaxation time is much larger than the diffuse surface scattering contribution, same as for planar surfaces. However, as the electron density decreases, the spill-out contribution decreases quickly while the diffuse surface scattering one remains nearly constant (we refer the reader to Fig. 2 of Ref. Apell et al. (1984)). Therefore, one expects the relative importance of both contributions to be reversed for low enough electron densities.

These contributions can be estimated rather easily from eq. (1) and the results of Ref. Apell et al. (1984) (see Supporting Information, SI, for a detailed derivation). Assuming and , being the bulk plasma frequency, we have the classical Mie LSPR frequency of the sphere . From eqs. (1) and (2) one can obtain its full-width at half-maximum (see eq. (S6)). Substituting and by their counterparts for a planar surface ( and , respectively), a good approximation for large , we find that for a perfectly diffuse surface reflecting electrons at random, the ratio of spill-out to diffuse surface scattering contributions can be estimated as

(3)

which is cast in terms of the effective electron mass (in units of the electron mass ) and the one-electron radius (in units of the Bohr radius ), with .

Equation (3) shows that the spill-out contribution decreases for effective masses smaller than the electron mass, which is the case for the conduction electrons in doped semiconductors. Also, the ratio of the contributions of the two mechanisms to the plasmonic width decreases with increasing as . Taking the values of for - 5 reported in Ref. Liebsch (1987) and , one obtains values of decreasing from 2.5 for , to 0.5 for . This estimate, as well as a simple analysis in the SI, show that the effects of non-specular scattering become more important as the electron density is lowered and will largely overcome these of electronic spill-out for .

Having demonstrated the importance of accounting for diffuse surface scattering, we now proceed to analyze these effects in a detailed manner. A microscopic description of this effect is, however, beyond the scope of the present work. Instead we use a phenomenological theory first designed for planar surfaces Flores and García-Moliner (1977); Monreal et al. (1980, 1982) and then extended to spheres de Andrés et al. (1985). The theory embeds the real sphere in an infinite, fictitious medium having exactly the same dielectric functions. Then, a constitutive relation giving the polarization due to the free charges inside the real sphere, is written as

(4)

where is the electric field vector in the infinite medium, which, for is the actual electric field inside the sphere, is the permittivity of free space, is the dielectric tensor of the medium, accounts for interband transitions of bound electrons, and the integral extends to the whole space. In this integral, the region of space describes the excitations produced at a point inside the sphere that propagate directly to the point while the fictitious region simulates these excitations that arrive at after being reflected at the surface. Therefore, the surface properties are mimicked by the values of the electric field in the fictitious region of the infinite medium. In this work, we want the sphere surface to reflect electrons completely at random and this means that, on the average, no excitation will arrive to coming from the surface. In eq. (4), this is thus equivalent to making the electric field to be zero outside the sphere. Hence our problem consists of constructing an electric field of the form

satisfying the Maxwell equations. In general, this is not possible without adding fictitious charges/currents to the ficticious region of the medium. Here we will use a different, equivalent, procedure.

From the point of view of an electromagnetic theoretical formulation of both kinds of surface effects discussed above, one should note that the radial component deviates from its classical counterpart because of the existence of longitudinal modes localized in the surface region, which are not present in the classical formulation. Consequently, the spill-out effect can only be analyzed if a non-local longitudinal dielectric function, that is, dependent on the spatial coordinates as well as on the frequency, is included in the theory. In a similar way, a description of the diffuse surface scattering mechanism requires the use of a non-local transverse dielectric function, which, as we will see below, allows to include in the theory the excitation of transverse electron-holes pairs in addition to the classical polariton mode propagating with wave vector . Since our previous analysis shows that we can expect the spill-out effects to be small, we will neglect them completely by making the longitudinal dielectric function of the sphere a local one. However, the transverse dielectric function has to be non-local. In our approximation only depends on spatial coordinates through the difference , and it is convenient to Fourier-transform the permittivity to momentum space. We will use here the simplest possible form for a non-local transverse dielectric function

(5)

where is a wave vector, and is a constant proportional to the Fermi velocity . This form of is obtained when the whole spectrum of electron-hole pairs is substituted by just a single pair. Thus the pole of eq. (5) describes a transverse electron-hole pair dispersing in energy linearly with the wave vector. Quantum size effects (QSE) are included in the theory by means of the energy gap Monreal et al. (2013) with Gorkov and Eliashberg (1965), being the Fermi wave vector. In this model, the strength of the QSE with particle size is proportional to .

The longitudinal and transverse dielectric functions have to be equal in the limit and therefore a good approximation for is

(6)

It is convenient to solve for in a basis set of spherical vectors functions: , and represented by their quantum numbers, and the parity (even or odd) with respect to the azimuthal angle. Here and only take positive integer values. The electric field vector of a plane wave of wave vector , incident onto the sphere along the direction, can be expressed with components having ,Stratton (1941) simplyfying the problem. Then, the field in the extended medium can be written in general as

(7)

The field inside the metal sphere is a linear combination of the different normal modes that can be excited according to the proposed dielectric functions. In our case, there are no longitudinal modes because is a local dielectric function and there are two transverse modes (index ): the polariton-like mode of wave vector and one transverse electron-hole pair of wave vector (see SI for details). Thus, the field inside the extended medium can be written as

(8)

At this point, the electric field inside the sphere contains four constants, namely, and () and the electric field outside the sphere contains two constants for the scattered amplitudes of the even and odd components. However, we have four matching conditions for the electromagnetic field at the sphere surface. The missing two equations can be obtained by imposing that the free-polarization calculated from the definition of eq. (4) with the field fulfills the wave equation , inside the sphere (details in the SI).

The electric field in the medium outside the sphere, has an odd component given by

(9)

and the even component is

(10)

Solving for and allows us to calculate the absorption cross section

(11)

as scattering can be neglected in all the results we present due to the small size of our particles. In the following calculations we use the values of the parameters appropriate for ZnO nanocrystals in toluene: , , and 0.1 eV.Schimpf et al. (2014) With these values, we use the lower limit of the experimental electron density, cm, to get the experimental surface plasmon energies at the largest radii. Then, , the Fermi velocity m s and  eV.

To show clearly the effects a diffuse scattering surface produces in the plasmonic resonances, we first perform a calculation of the absorption cross section neglecting quantum size effects () and with . This value of is given by the long wave length limit of the Lindhard transverse dielectric function. The results are depicted in Fig. 1 for spheres of radii 4, 3 and 2 nm, compared to the classical results of the Mie theory Mie (1908). We can appreciate the widening of the resonances and the appearance of small oscillations on their right side which are caused by the additional propagating transverse mode. The resonance strongly blue-shifts in energy for 2 nm.

Figure 1: Effects of diffuse surface scattering as seen in absorption. Absorption cross-section normalized to surface area as a function of energy for 4, 3 and 2 nm from top to bottom. Quantum size effects are neglected (). Dashed lines: classical Mie theory; continuous lines: present theory for a totally diffuse surface. Notice the asymmetric widening of the resonance and the strong blue-shift for R = 2 nm. The inset shows a magnification of the plot in the energy region above the peak (semi-log scale) to highlight the oscillations.

From our calculated cross section we extract the position, , and the width of the resonance, , defined as the full width at half maximum. and are taken as adjustable parameters given that they have to be increased from the values and , nm, by less than 30 in order to reproduce the experimental results of Ref. Schimpf et al. (2014). A reason for this is that the value of is justified for a large system. Moreover, other values of can be found in the literature since the form of eq. (5) substitutes the whole spectrum of transverse electron-hole pairs by a single pair. With respect to , a local dielectric function for few electrons in a box has been calculated Jain (2014). It has the form of eq. (6) with , where is the number of electrons and is the side of the box. Our frequency gap scales with and particle size exactly with the same powers and a prefactor that differs by 15 if the electron density is the same in both models. Since the prefactor has to depend on the shape of the nanoparticle, a change of ca. 20 is justified.

Figure 2: The energy of the plasmonic resonance versus the sphere radius for four groups of the values of the parameters and . Dashed line: and (no QSE); dot-dashed line and nm; continuous line: and nm and dotted line: and nm. The experimental values of Ref. Schimpf et al. (2014) are represented by the black squares. By including QSE and slightly increasing the parameters involved from the basic theory there is a good account for the experimental findings.

Figure 2 shows as a function of the sphere radius. The dashed line displays the surface plasmon energy for and ; it presents small oscillations with R for radii larger that 3 nm, and then quickly blue shifts for smaller radii. When we include the quantum size effect using nm (dot-dashed line) we observe the additional blue-shift caused by this effect, which is more pronounced for the smaller radii, but the oscillations remain. If we now increase by 30 keeping the same value of (solid line) we further increase the blue-shift at small radii and also change the oscillations at large radii. When we increase both, and by 20 we obtain the dotted line which does not differ much from the previous case. In both cases the experimental results Schimpf et al. (2014) can be reproduced remarkably well. Thus a diffuse surface produces a non-negligible blue-shift of the plasmonic resonances in small spheres with a low density of electrons, a result which is not obtained in the simple theory of Ref.Apell et al. (1984) where they would be essentially unshifted.

Figure 3: The width of the plasmonic resonace versus for the the same groups of the values of the parameters as in Fig. 2. dashed line: and ; dot-dashed line and nm; continuous line: and nm and dotted line: and nm. The experimental values of Ref. Schimpf et al. (2014) are represented by the black squares. While in the simple model of Apell et al. (1984) the plasmon width would increase linearly with for all radii, the detailed model for diffuse surface scattering produces this behavior only at large radii. The width actually oscillates at intermediate radii and then increases fast at short radii. Notice that the plasmon width is much more sensitive to the values chosen for than the plasmon energy. The experimental width can be reproduced by the same set of parameters that reproduce the plasmon resonance.

Figure 3 depicts the width of the resonance as a function of , for the same set of values of and as in Fig. 2. Note that, while in the pure classical theory the width of the resonance would be equal to the bulk value eV (bottom line of Fig. 3 ), the surface scattering mechanism increases the plasmon damping linearly in for large radii. Then, for 6 nm 3 nm the width oscillates between 0.13 eV and 0.16 eV and finally, for radii smaller than ca. 3–2.5 nm the plasmon width increases again almost linearly with with a higher slope which also increases with . The experimental results of Ref. Schimpf et al. (2014) are shown by the full squares. The width is better reproduced by our calculation with the largest value of . Note also that the plasmon width is much more sensitive to the values of than the plasmon energy.

We now obtain the length from our electromagnetic theory. This can be done analytically given the simplicity of our transverse dielectric function and that we only need to consider the component of the fields having even symmetry. Using the small-argument asymptotic values of the spherical Bessel functions appearing in the electric fields of the even mode (see eq. (S36)) we get as

(12)

where is the pole of the transverse dielectric permittivity, eq. (5), and . The origin of the oscillations in and shown in Figs. 2 and 3 is clearly related to the Bessel functions appearing in eq. (12). Since (eq. (S27)), then for the values of used here and large-argument asymptotic expansions of the Bessel functions can be performed yielding

(13)

Comparing this equation with the corresponding for the planar surface, eq. (S13), which is used in simple models, we see that the correction to for a real sphere is the factor , so a large is required to get rid of the oscillatory factor to have the same limit, assuming is unimportant. Then the crossover from large values of , where the sphere can still be described by the planar surface, to small values of , is given by . The physical meaning of this relation is clear. The decay length of the transverse electron-hole pair mode is . When this length becomes shorter than the sphere diameter , the mode only feels one surface and consequently, the limit of the planar surface is reached.

Figure 4: (a) The real part and (b) the imaginary part of versus for , and eV. Red solid line: results of the full theory, eq. (12), and dashed line: results of the asymtotic expansion eq. (13). The continuous horizontal lines are the values of and , being good asymptotes for .

Figure 4 shows the real and the imaginary parts of as a function of compared to their large-argument asymptotic values given by eq. (13), for a typical value of  eV, and (no QSE). The non-zero values of at large values of are the consequence of having in this calculation, which, however, produces negligible shifts of the surface plasmon energies shown in Fig. 2. Note that, even if QSE are neglected, depends strongly on for small radii. One can note that the expansion of eq. (13) is a good approximation to for radii larger than ca. 2 nm.

Surface scattering is usually included in simple theories by means of an effective damping rate , being a constant of the order of 1. This procedure produces a linear increase of the LSPR width with and, for low electron density systems, a continuous red shift of its spectral position with decreasing Schimpf et al. (2014). While this may be a reasonable approximation for large radii, when and the main effect of surface scattering is to increase the plasmon width linearly with while the plasmon energy presents small oscillations around its classical value (Figs. 3 and 2 respectively), an effective damping rate theory cannot capture the nature of diffuse surface scattering at short radii. As already noted, is a complex quantity whose real part cannot in general be neglected. A better approximation can be obtained by defining an effective size-dependent dielectric function for a sphere containing diffuse surface scattering, , via the Rayleigh polarizability (see eq. (S45)) as

(14)

and expressed by eq. (12). Such a definition can be useful in the analysis of problems involving the dielectric function of the nanosphere.

In this article, we have investigated how different surface effects, namely electronic spill-out and diffuse scattering, impact in the optical properties of ultra-low electron density nanospheres which are experimentally accessible by electron doping of semiconductor quantum dots. We first estimated the relative contributions of spill-out to diffuse surface scattering, showing that the ratio decreases with effective electron mass and with increasing . Next, we used a more elaborated theoretical model for including the diffuse surface scattering mechanism into an electromagnetic theory. Using this model, we calculated the extinction cross-section and found that the plasmonic resonances show an oscillatory behavior both in position and width for sizes larger than ca. 3 nm in radius and a strong blueshift in energy and an increased width for smaller radii. When our model is used in conjunction with a dielectric function that includes effects of quantization due to the small size of the particles, we are able to reproduce the position and widths of the measured resonances Schimpf et al. (2014) using reasonable values of the two basic parameters, and , involved in the theory. From our formalism, we can extract the length that allows to include the effects of a diffuse surface into an effective size-dependent dielectric function, which can be useful for future work. We conclude that diffuse scattering at the surface of ultra-low electron density nanocrystals is an important mechanism affecting their plasmonic properties and has to be taken into account when designing plasmonic devices based on doped semiconductor nano structures.

{acknowledgement}

RCM acknowledges financial support from the Spanish Mineco via the project MAT2014-53432-C5-5-R. TJA thanks the Foundation of Polish Science for support via the project HOMING PLUS/2013-7/1. TJA and SPA acknowledge financial support from the Swedish Foundation for Strategic Research via the Functional Electromagnetic Metamaterials for Optical Sensing project SSF RMA 11.

{suppinfo}

Details of the simple theoretical model and estimation of spill-out and diffuse surface scattering effects. Details of the solution for the electromagnetic fields in the more detailed theory for diffuse surface scattering. Derivation of the formulae for the diffuse surface scattering length and the corresponding size-dependent dielectric function.

References

  1. Ritchie, R. H. Plasma Losses by Fast Electrons in Thin Films. Phys. Rev. 1957, 106, 874–881.
  2. Raether, H. Surface Plasmons on Smooth and Rough Surfaces and on Gratings; Springer-Verlag, 1998.
  3. Liebsch, A. Electronic Excitations at Metal Surfaces; Plenum, 1997.
  4. Maier, S. Plasmonics: Fundamentals and Applications; Springer-Verlag, 2007.
  5. Scholl, J. A.; Koh, A. L.; Dionne, J. A. Quantum Plasmon Resonances of Individual Metallic Nanoparticles. Nature 2012, 483, 421–427.
  6. Raza, S.; Stenger, N.; Kadkhodazadeh, S.; Fischer, S. V.; Kostesha, N.; Jauho, A.-P.; Burrows, A.; Wubs, M.; Mortensen, N. A. Blueshift of the Surface Plasmon Resonance in Silver Nanoparticles Studied with EELS. Nanophotonics 2013, 2, 131–138.
  7. Peng, S.; McMahon, J. M.; Schatz, G. C.; Gray, S. K.; Sun, Y. Reversing the Size-Dependence of Surface Plasmon Resonances. Proc. Natl. Acad. Sci. U.S.A. 2010, 107, 14530–14534.
  8. Baida, H.; Billaud, P.; Marhaba, S.; Christofilos, D.; Cottancin, E.; Crut, A.; Lermé, J.; Maioli, P.; Pellarin, M.; Del Fatti, N.; et al. Quantitative Determination of the Size Dependence of Surface Plasmon Resonance Damping in Single Ag@SiO Nanoparticles. Nano Lett. 2009, 9, 3463–3469.
  9. Townsend, E.; Bryant, G. W. Plasmonic Properties of Metallic Nanoparticles: The Effects of Size Quantization. Nano Lett. 2012, 12, 429–434.
  10. Lermé, J.; Baida, H.; Bonnet, C.; Broyer, M.; Cottancin, E.; Crut, A.; Maioli, P.; Del Fatti, N.; Vallée, F.; Pellarin, M. Size Dependence of the Surface Plasmon Resonance Damping in Metal Nanospheres. J. Phys. Chem. Lett. 2010, 1, 2922–2928.
  11. Luther, J. M.; Jain, P. K.; Ewers, T.; Alivisatos, A. P. Localized Surface Plasmon Resonances Arising from Free Carriers in Doped Quantum Dots. Nat. Mater. 2011, 10, 361–366.
  12. Buonsanti, R.; Llordes, A.; Aloni, S.; Helms, B. A.; Milliron, D. J. Tunable Infrared Absorption and Visible Transparency of Colloidal Aluminum-Doped Zinc Oxide Nanocrystals. Nano Lett. 2011, 11, 4706–4710.
  13. Naik, G. V.; Liu, J.; Kildishev, A. V.; Shalaev, V. M.; Boltasseva, A. Demonstration of Al:ZnO as a Plasmonic Component for Near-Infrared Metamaterials. Proc. Natl. Acad. Sci. U.S.A. 2012, 109, 8834–8838.
  14. Faucheaux, J. A.; Jain, P. K. Plasmons in Photocharged ZnO Nanocrystals Revealing the Nature of Charge Dynamics. J. Phys. Chem. Lett. 2013, 4, 3024–3030.
  15. Faucheaux, J. A.; Stanton, A. L. D.; Jain, P. K. Plasmon Resonances of Semiconductor Nanocrystals: Physical Principles and New Opportunities. J. Phys. Chem. Lett. 2014, 5, 976–985.
  16. Schimpf, A. M.; Thakkar, N.; Gunthardt, C. E.; Masiello, D. J.; Gamelin, D. R. Charge-Tunable Quantum Plasmons in Colloidal Semiconductor Nanocrystals. ACS Nano 2014, 8, 1065–1072.
  17. Monreal, R. C.; Antosiewicz, T. J.; Apell, S. P. Competition Between Surface Screening and Size Quantization for Surface Plasmons in Nanoparticles. New J. Phys. 2013, 15, 083044.
  18. Monreal, R. C.; Apell, S. P.; Antosiewicz, T. J. Surface Scattering Contribution to the Plasmon Width in Embedded Ag Nanospheres. Opt. Express 2014, 22, 24994–25004.
  19. Flores, F.; García-Moliner, F. Classical Electrodynamics of Non-Specular Conducting Surfaces. J. Phys. France 1977, 38, 863–870.
  20. Monreal, R.; García-Moliner, F.; Flores, F. Optical Properties of Non-Ideal Solid Surfaces: Phenomenological Models. Phys. Scr. 1980, 22, 155–164.
  21. Monreal, R.; García-Moliner, F.; Flores, F. Non Local Electrodynamics of Metal Film Systems. J. Phys. France 1982, 43, 901–913.
  22. Feibelman, P. J. Surface Electromagnetic Fields. Prog. Surf. Sci. 1982, 12, 287–407.
  23. Persson, B. N. J. Polarizability of Small Spherical Metal Particles: Influence of the Matix Environment. Surf. Sci. 1993, 281, 153–162.
  24. Mogensen, K. B.; Kneipp, K. Size-Dependent Shifts of Plasmon Resonance in Silver Nanoparticle Films Using Controlled Dissolution: Monitoring the Onset of Surface Screening Effects. J. Phys. Chem. C 2014, 118, 28075–28083.
  25. Apell, P.; Ljungbert, A. A General Non-Local Theory for the Electromagnetic Response of a Small Metal Particle. Phys. Scr. 1982, 26, 113–118.
  26. Apell, P.; Penn, D. R. Optical Properties of Small Metal Spheres: Surface Effects. Phys. Rev. Lett. 1983, 50, 1316–1319.
  27. Apell, P.; Monreal, R.; Flores, F. Effective Relaxation Time in Small Spheres: Diffuse Surface Scattering. Solid State Commun. 1984, 52, 971–973.
  28. Liebsch, A. Dynamical Screening at Simple-Metal Surfaces. Phys. Rev. B 1987, 36, 7378–7388.
  29. de Andrés, P.; Monreal, R.; Flores, F. Quantum Size and Nonlocal Effects in the Electromagnetic Properties of Small Metallic Spheres. Phys. Rev. B 1985, 32, 7878–7889.
  30. Gorkov, L. P.; Eliashberg, G. M. Minute Metallic Particles in an Electromagnetic Field. Sov. Phys. JETP 1965, 21, 940–947.
  31. Stratton, J. A. Electromagnetic Theory; McGraw-Hill, New York, 1941.
  32. Mie, G. Beiträge zur Optik trüber Medien, speziell Kolloidaler Metallösungen. Ann. Phys. 1908, 25, 377–445.
  33. Jain, P. K. Plasmon-in-a-Box: On the Physical Nature of Few-Carrier Plasmon Resonances. J. Phys. Chem. Lett. 2014, 5, 3112–3119.
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