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Optics Express

Optics Express

  • Editor: C. Martijn de Sterke
  • Vol. 18, Iss. 14 — Jul. 5, 2010
  • pp: 14553–14567
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Chiral metamaterials: retrieval of the effective parameters with and without substrate

Rongkuo Zhao, Thomas Koschny, and Costas M. Soukoulis  »View Author Affiliations


Optics Express, Vol. 18, Issue 14, pp. 14553-14567 (2010)
http://dx.doi.org/10.1364/OE.18.014553


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Abstract

After the prediction that strong enough optical activity may result in negative refraction and negative reflection, more and more artificial chiral metamaterials were designed and fabricated at difference frequency ranges from microwaves to optical waves. Therefore, a simple and robust method to retrieve the effective constitutive parameters for chiral metamaterials is urgently needed. Here, we analyze the wave propagation in chiral metamaterials and follow the regular retrieval procedure for ordinary metamaterials and apply it in chiral metamaterial slabs. Then based on the transfer matrix technique, the parameter retrieval is extended to treat samples with not only the substrate but also the top layers. After the parameter retrieval procedure, we take two examples to check our method and study how the substrate influences on the thin chiral metamaterials slabs. We find that the substrate may cause the homogeneous slab to be inhomogeneous, i.e. the reflections in forward and backward directions are different. However, the chiral metamaterial where the resonance element is embedded far away from the substrate is insensitive to the substrate.

© 2010 Optical Society of America

1. Introduction

Chiral metamaterials (CMMs), which are artificial materials that lack any planes of mirror symmetry, possess strong ability to rotate the plane of polarization of electromagnetic waves. This ability is called optical activity which is of great interest to many areas of science, for example, analytical chemistry and molecular biology. Recently, it was predicted that strong enough optical activity may result in negative refraction [1–6

1. J. B. Pendry, “A chiral route to negative refraction,” Science 306, 1353–1355 (2004). [CrossRef] [PubMed]

] and negative reflection [7

7. C. Zhang and T. J. Cui, “Negative reflections of electromagnetic waves in a strong chiral medium,” Appl. Phys. Lett. 91, 194101 (2007). [CrossRef]

]. After these predictions [1–7

1. J. B. Pendry, “A chiral route to negative refraction,” Science 306, 1353–1355 (2004). [CrossRef] [PubMed]

], a lot of artificial CMMs were designed and fabricated at different frequency ranges from microwaves to optical frequencies [8–22

8. J. K. Gansel, M. Thiel, M. S. Rill, M. Decker, K. Bade, V. Saile, G. V. Freymann, S. Linden, and M. Wegener, “Gold helix photonic metamaterial as broadband circular polarizer,” Science 325, 1513–1515 (2009). [CrossRef] [PubMed]

]. The basic physical quantities to characterize the optical properties of CMMs are the effective constitutive parameters. Therefore, a simple and robust method to retrieve the effective parameters for CMMs is urgently needed.

After the parameter retrieval, we give two chiral metamaterial examples: (1) twisted-crosses and (2) four-folded rotated Ω-particles. For the twisted-crosses CMMs, the resonance elements are very close to the substrate. The existence of the substrate, therefore, has a huge influence on the thin CMM slab. It causes the resonance shifts to low frequencies and induces the homogeneous slab to be inhomogeneous. In order to correct the inhomogeneity, we need to introduce a top layer, the same material as the substrate, to cover the CMM slab. The top layer will red-shift the resonance further. For the four-folded rotated Ω-particles CMMs, the resonance elements are embedded far away from the substrate. The influence of the substrate can be neglected. In the meanwhile, profiting from the retrieval method and the precise simulation, we fit the retrieval results using the analytical formulas deriving from the Ω-particle resonator model. They agree with each other very well.

The following sections are arranged as follows. In Sec. 2, we first obtain explicit analytic expressions of the retrieval parameters for free standing CMM slabs, then we extend this method to deal with the samples with the substrate and top layers. In Sec. 3, we use the parameter retrieval methods to study two CMM examples and obtain the influence of substrate/top layer on thin layer CMM slabs. Finally in Sec. 4, we present our conclusions.

2. Retrieval method

2.1. Eigen waves in chiral materials

For reciprocal (Pasteur) chiral materials [31

31. I. V. Lindell et al., Electromagnetic Waves in Chiral and Bi-Isotropic Media (Artech House, Boston · London, 1994).

, 32

32. A. Serdyukov et al., Electromagnetics of Bi-anisotropic Materials: Theory and Applications (Gordon and Breach Science Publishers, Amsterdam, 2001).

], the strength of the cross coupling between the magnetic and electric field is characterized by the parameter κ called chirality. The constitutive relations in chiral medium are usually written as [33

33. Some people (see, for instance, A. Lakhtakia et al., “Reflection of plane waves at planar achiral-chiral interfaces: independence of the reflected polarization state from the incident polarization state,” J. Opt. Soc. Am. A7, 1654 (1990).) use the Drude-Born-Fedorov relations: D = ε(B + β∇ × E), B = μ(H + β∇ × H), where β characterizes the strength of the chirality. They can be brought to the same form. The transformations between the parameters of the two systems are given in Ref. 26. [CrossRef]

]:

(DB)=(ε0εiκc0iκc0μ0μ)(EH),
(1)

where ε 0 and μ 0 are the permittivity and permeability of vacuum, ε and μ are the relative permittivity and permeability of the medium respectively. c 0 is the speed of light in vacuum. Assuming all fields to be plane waves, the source free Maxwell equations take the form:

k×H=ωD,k×E=ωB,
(2)

where k and ω are the wavevector and the angular frequency of the plane wave in the chiral medium. Inserting Eq. (1) into Eq. (2), we can get the eigenfunction of the electric field E propagating in the chiral medium:

k×(k×E)=k02(εμκ2)E2iκk0(k×E),
(3)

where k 0 = ω/c 0 is the free space wavevector. For simplicity but without loss of generality we can assume k = kẑ and obtain the eigenvectors and eigenvalues as:

E±(z)=(x̂±iŷ)E0eikz,
(4)
k±=k0(n±κ),
(5)

where n=εμ . There are two eigenmodes in chiral medium. One is the right circular polarization (RCP/+) wave and the other is the left circular polarization (LCP/−) wave. Any wave propagating though the medium can be uniquely decomposed into RCP and LCP and there is no conversion between RCP and LCP as they propagate in the chiral medium. Then we can define the index of refraction for RCP/LCP waves as:

n±=n±κ.
(6)

If κ > n, n will be negative. This constitutes an alternative approach to realize a negative refractive index as proposed earlier by Pendry [1

1. J. B. Pendry, “A chiral route to negative refraction,” Science 306, 1353–1355 (2004). [CrossRef] [PubMed]

].

A chiral medium has two important properties. One is called optical activity which characterizes the rotation of the polarization plane of a linearly polarized light as it passes through a chiral medium. Mathematically, it’s defined as the polarization azimuth rotation angle of elliptically polarized light:

θ=12[arg(T+)arg(T)],
(7)

where T + and T are the transmission coefficients for RCP and LCP waves. The other property is circular dichromism which arises from the different absorption for RCP and LCP. It characterizes the difference between the transmissions of two polarizations:

η=12tan1(T+2T2T+2+T2).
(8)

Artificial CMMs with large θ and small η are very important for applications.

Fig. 1. Schematics of the transmission and reflection coefficient of a standalone CMM slab.

2.2. Parameter retrieval for CMM slabs without substrate

A slab of reciprocal (Pasteur) chiral material looks exactly identical for waves propagating in forward or backward direction. However, for a normal incident circular polarized wave E ±(z) = ( ± )E 0 eikz along the z direction the reflected wave will be E±(z) = (x̂ ± )E0 e−ikz along the −z direction. The y component is always 90° advanced(+) / retarded(−) with respect to the x component when the wave vector changes to the opposite direction. Therefore, the polarization of the reflected wave is reversed based on our current definition of handiness in relation to the wave vector, i.e. the reflected wave of RCP (LCP) wave is LCP (RCP). Now we consider a circularly polarized plane wave normally incidents onto a CMM slab with thickness d, refractive index n ±, and impedance Z=με , as shown in Fig. 1 (note that the impedance, Z’s, of RCP and LCP waves are identical [31

31. I. V. Lindell et al., Electromagnetic Waves in Chiral and Bi-Isotropic Media (Artech House, Boston · London, 1994).

]). The amplitude of the incident wave is assumed to be unity; the amplitudes of the transmitted and reflected waves are T ± and R respectively; those of the forward and backward propagating waves inside the slab are T± and R. Applying the condition of continuity of tangential electric and magnetic fields at z = 0 and z = d, we have the following equations:

1+R=T±+R,
(9a)
1R=T±RZ,
(9b)
T±eik±d+Reikd=T±,
(9c)
T±eik±dReikdZ=T±,
(9d)

where k ± is the wave vector as defined by Eq. (5). Then eliminating T′ and R′ in Eqs. (9), we obtain the transmission and reflection coefficients:

T±=4Zeink0de±iκk0d(1+Z)2(1Z)2e2ink0d,
(10a)
R=(1Z2)(e2ink0d1)(1+Z)2(1Z)2e2ink0d.
(10b)

Equation (10b) shows that R + = R . This can be understood intuitively as follows: We know that the polarizations of RCP and LCP are reversed after being reflected. For the forward incident wave, the optical path of RCP (LCP) is n + d (nd), where d is the distance that the wave has traveled; For the backward reflected wave, the optical path is nd (n + d). Therefore, the total optical paths for RCP and LCP are all n + d + nd. They pass through the same optical path for the reflected waves, so the loss should be the same for both of them. In addition, the same impedance of the RCP and the LCP gives the same reflections for both circular polarizations on the surface. Therefore, both the reflections of the single slab should be the same.

Inverting the above Eqs. (10), the impedance Z and refractive index n ± are given below:

Z=±(1+R)2T+T(1R)2T+T,
(11a)
n±=ik0d{ln[1T±(1Z1Z+1R)]±2mπ},
(11b)

where m is an integer determined by the branches. The correct sign of the square root in Eq. (11a) and the correct branch of the logarithm in Eq. (11b) are selected according to the following conditions:

Re(Z)0,Im(n)0,
(12)

which are required by energy conservation and causality [23

23. D. R. Smith, S. Schultz, P. Markoš, and C. M. Soukoulis, “Determination of effective permittivity and permeability of metamaterials from reflection and transmission coefficients,” Phys. Rev. B 65, 195104 (2002). [CrossRef]

]. Then the remaining retrieval parameters can be obtained with the following relations: n = (n + + n )/2, κ = (n +n )/2, ε = n/Z, and μ = nZ.

Actually, we have another route to get the retrieval results. If we redefine T=T+T and R = R , according to Eqs. (10), T and R can be written as:

T=4Zeink0d(1+Z)2(1Z)2e2ink0d,
(13a)
R=(1Z2)(e2ink0d1)(1+Z)2(1Z)2e2ink0d.
(13b)

These expressions are exactly the same as those for the ordinary nonchiral materials. Therefore, we can use the traditional retrieval procedure for the nonchiral metamaterials to get the refraction index n, the impedance Z, the permeability ε and the permittivity μ [23

23. D. R. Smith, S. Schultz, P. Markoš, and C. M. Soukoulis, “Determination of effective permittivity and permeability of metamaterials from reflection and transmission coefficients,” Phys. Rev. B 65, 195104 (2002). [CrossRef]

]. Then from Eqs. (10a), we can obtain

κ=i2k0dln(T+T)=i2k0dln(T+eiϕ+Teiϕ),
(14)

where ϕ ± are the phases of T ±. Then we immediately get the refraction indexes n ± = n ± κ.

From Eqs. (14), we have

Re(κ)=ϕ+ϕ+2mπ2k0d,
(15a)
Im(κ)=lnTlnT+2k0d,
(15b)

where the integer m is determined by the condition of −π < ϕ +ϕ + 2 < π for one unit cell. We note that the real and imaginary parts of κ relate to the azimuth rotation angle θ and the circular dichromism η respectively.

2.3. Parameter retrieval for CMM slabs with substrate

The retrieval procedure discussed above identifies the scattering amplitudes of the CMM slab with those of an equivalent homogeneous slab. The retrieved effective parameters of the CMM are the parameters of this equivalent homogeneous slab and given as functions of the scattering matrix of the CMM. In this form, the retrieval procedure is only applicable if the CMM has the same symmetry as the equivalent homogeneous slab. For instance, the reflection amplitudes for a homogeneous chiral (Pasteur) slab are identical for incidence from the front or back interfaces. For a CMM on top of a substrate (for an example see Fig. 2) the scattering amplitudes do not necessarily have this property. In this case, we cannot directly apply the above retrieval procedure to the measured or simulated scattering amplitudes of the sample to obtain effective parameters.

In the experiments and simulations (for instance, the commercial software CST Microwave Studio [34

34. CST MICROWAVE STUDIO (CST MWS) is a specialist tool for the 3D EM simulation of high frequency components, http://www.cst.com/Content/Products/MWS/Overview.aspx.

]), we can easily obtain the total scattering matrix S total of the CMM/substrate slab which relates the incoming waves to the outgoing (scattered) waves. It is well known [35

35. P. Markoš and C. M. Soukoulis, Wave Propagation: From Electrons to Photonic crystals and Left-Handed Materials (Princeton University Press, Princeton, 2008).

] that any scattering matrix S corresponds to a transfer matrix M which relates the amplitudes of the in- and outgoing waves in front of the slab to those behind the slab:

S=(rttr);M=(trrtrtrt1t),
(16)

where t and r are the transmission and reflection amplitudes; the quantities without (with) prime (′) refer to wave propagation in forward (backward) direction.

Now we consider a structure of substrate/CMM/top layer as an example and assume the positive (forward) direction to be from the top layer to substrate layer. Measurement or simulation afford the total scattering matrix S total of the stack in terms of total transmission and reflection amplitudes. Using Eq. (16) we obtain the corresponding total transfer matrix M total, which factorizes into a product of the transfer matrices of the individual layers [35

35. P. Markoš and C. M. Soukoulis, Wave Propagation: From Electrons to Photonic crystals and Left-Handed Materials (Princeton University Press, Princeton, 2008).

]:

Mtotal=MsubstrateMCMMMtoplayer.
(17)

The homogeneous substrate and top layers are assumed to be known. Their transfer matrices, M substrate and M toplayer, respectively, are just the well known transfer matix of a homogeneous slab and can be calculated analytically (as the product of the transfer matix across the interface from vacuum into the homogenous slab, the diagonal transfer matrix (phase & attennuation) for the propagation within the homogeneous slab, and the inverse of the interface transfer matrix again to step out of the slab back into vacuum):

M=[Z+12ZZ12ZZ12ZZ+12Z][eink0d00eink0d][1+Z21Z21Z21+Z2],
(18)

where the impedance of Z, refractive index of n, and the thickness of d are all known parameters of the substrate or the top layer. Note that the transfer matrix of each layer is that of the slab in free space, i.e. the interface of two media can be considered as two media separated by a vacuum slab with zero thickness.

Solving the above equation [Eq. (17)], we can get the effective transfer matrix of the CMM slab standing alone in free space:

MCMM=Msubstrate1MtotalMtoplayer1.
(19)

Having extracted the effective transfer matrix of the CMM slab alone, we can use the relation [Eq. (16)] again to obtain the S parameters of the free standing CMM slab. Then the retrieval procedure given in Sec. 2.2 can be applied to the isolated S parameters of the CMM slab. And following this way, we can obtain the retrieval parameters of CMMs with substrate and/or the top layer.

3. Examples of the CMM slabs with and without substrate

In this section, we will give two examples to demonstrate that a physically meaningful retrieval can be obtained from scattering amplitudes measured for the combined system of CMM and substrate/top layer and to show how the substrate influences the retrieval parameters of the CMM slab. For this purpose, we choose the twisted-crosses CMMs which had been fabricated in the optical region by Decker et al. [21

21. M. Decker, M. Ruther, C. E. Kriegler, J. Zhou, C. M. Soukoulis, S. Linden, and M. Wegener, “Strong optical activity from twisted-cross photonic metamaterials,” Opt. Lett. 34, 2501–1503 (2009). [CrossRef] [PubMed]

] and the four-folded rotated Ω-particle CMMs which is closest to the standard chiral model.

3.1. Retrieval results of the twisted-crosses CMM slabs with and without substrate

Fig. 2. (a)–(c) are the Schematics of the twisted-crosses CMM slab. (a) free standing, (b) with substrate and top layer, and (c) with substrate only. The amplititudes, (d)–(f), and the phases, (g)–(i), are also shown correspondingly. The prime (′) denotes that the wave is incident from the opposite direction.

The structure of the twisted-crosses CMM is shown in Fig. 2. It’s composed of two gold crosses rotated against each other by an angle of 22.5°. Each arm of the crosses is a short rectangular wire with the dimension of 25nm × 56nm × 315nm. The separation between the two crosses is 37.5nm. The gold structure is embedded in a lossless dielectric with the refractive index of n = 1.41 as shown in Fig. 2(a). The structure is fabricated on the glass substrate (n=1.45) with the thickness of 500nm as illustrated in Fig. 2(c); Optionally a thin glass layer (n=1.45) with the thickness of 200nm can be placed on top of the embedded gold structure, see Fig. 2(b). The gold is modeled by a Drude model permittivity ε(ω)=εωp2ω(ω+iωc) with plasma frequency ωp = 2π × 2159THz, collision frequency ωc = 2π × 25THz, and ε = 9.07.

Fig. 3. The retrieval parameters ε, μ, κ, n , n +, η, and θ for CMM slabs. (Left) freestanding, (Middle) with substrate and top layer, and (Right) with substrate only.These results were extracted using (19).

The scattering amplitudes of the homogeneous chiral slab are the same for propagation though the slab in forward or backward direction. The simulated scattering amplitudes for the free standing CMM shown in Figs. 2(a), 2(d), and 2(g) also have this property. We can directly apply the retrieval procedure described in Sec. 2.2 and obtain the effective medium parameters. The results are given in Figs. 3.

For the CMM on susbtrate no meaningful retrieval can be obtained by applying the retrieval procedure described in Sec. 2.2 directly to the total scattering amplitudes; The presence of the substrate leads to additional scattering not originating from the CMM. It also makes the reflections in forward and backward direction unequal - an asymmetry which can never be reproduced by the homogeneous chiral slab. Only after extracting the scattering amplitudes of the CMM slab itself from the simualtion results using Eq. (19) derived in Sec. 2.3 we can apply the standard retrieval procedure described in Sec. 2.2 to the extracted CMM scattering amplitudes and obtain reasonable effective medium parameters for the CMM slab.

Even after extracting the CMM scattering amplitudes we still observe some weakly asymmetric reflections R +−R+− in forward and backward direction for the CMM on substrate in Figs. 2(f), 2(i). The extraction derived in Sec. 2.3 does only deal with the propagating modes in the system. However, there is also interaction between the CMM slabs surface regions with their environment mediated by evanescent modes. This interaction makes the surfaces of the CMM slab on substrate unequal and prevents its approximation by an equivalent homogenenous effective medium slab.

There are two possible solutions to this problem: First, we could follow the method introduced in Ref. 22

22. M. Decker, M. W. Klein, M. Wegener, and S. Linden, “Circular dichroism of planar chiral magnetic metamaterials,” Opt. Lett. 32, 856–858 (2007). [CrossRef] [PubMed]

and approximate an isotropic reflection Rav as the geometric average,

Rav=RR,
(20)

where, R (R′) is the reflection when the incident wave is from the top/vacuum (bottom/substrate) side of the CMM slab. This method has been used successfully if the anisotropy was small enough [27

27. D. R. Smith, D. C. Vier, Th. Koschny, and C. M. Soukoulis, “Electromagnetic parameter retrieval from inhomogeneous metamaterials,” Phys. Rev. E 71, 036617 (2005). [CrossRef]

]. (Note that the inhomogenization is not inherent property of the twisted-crosses CMM slab. It’s only the boundary effect of the thin layer sample. If a sufficiently transparent sample goes to bulk material with infinity thickness, this boundary effect becomes negligible.) Using this method we obtain the retrieval of the single sided CMM on sustrate shown in the right column in Fig. 3.

Second, we could cover the top side of the CMM with a second layer of substrate. This layer does not need to be very thick as the interaction via the evanescent modes with the surface layers of the CMM decays quickly. As can be seen in Figs. 2(e), 2(h) this approach lead to perfectly symmetric reflection amplitudes and allows to apply the standard retrieval procedure described in Sec. 2.2 to the extracted CMM scattering amplitudes to obtain the effective parametes of the CMM slab. The results for this case are show in the center column in Fig. 3.

Comparing the results with and without substrate, we can see that the substrate has two main influences on the CMMs. One is lowering the frequency of the resonance because the substrate increases the capacity C of the resonator and ωR~1LC . The other is the substrate may induce the homogeneous CMM to be inhomogeneous. For the structure with substrate only, the two crosses are in the different environments. For the cross near the substrate, the evanescent field leak to the substrate while for the cross near the air, the field leaks to the air, which makes the two substantially identical crosses unequal physically. Even the substrate contribution has been deducted off mathematically by using Eq. (19), the CMM slab still shows the inhomogeneous property (e.q. R +−R+−).

3.2. Retrieval results of the four-folded rotated Ω-particle CMM slabs with and without substrate

Fig. 4. Schmetics of the four-folded rotated Ω-particle CMM. The inner and outer radius of the loop are r = 5µm and R = 5.5µm. The length of each straight wire is L = 8.08µm. d = 0.5µm. a = 32µm. b = 12µm. Each Ω-particle locates at the center of each quarter of the unit cell. The silver Ω-particle is embeded in the polyimide with ε = 2.5 and loss tangent δ = 0.03. The silver is charactored by the Drude model with the surface plasmon ωp = 13.66 × 1015 rad/s and the collision frequency ωc = 2.73 × 1013 rad/s.

Not all the chiral metamaterials are so sensitive to the influence of the substrate. In the following, we will give such an example—four-folded rotated Ω-particle chiral metamaterials. The structure and the dimensional parameters are shown in Fig. 4. The incident wave is perpendicular to the CMM slab.

The amplitude and phase of the reflection and transmission are shown in Figs. 5(a)–5(d). The left is with 50µm substrate (n=1.27) only and the right is for the free standing sample. There is a strong resonance at around 1.87THz where both the amplitude and phase of the transmissions of RCP and LCP are different, which indicates very strong optical activity and circular dichromism. The interesting is that for the structure with substrate only, the extracted reflections from different directions almost overlap with each other, e.g. R = R′, even they have a large difference before the extraction using Eq. (19). Comparing the results between with [Fig. 5(a),5(c)] and without [Fig. 5(b), 5(d)] substrate, we see that the substrate almost has no influence on the Ω-particle CMMs. That is because the resonance elements, the gap of the circle magnetic resonator and the short wires for the electric resonance, are located in the middle of the unit cell. They are far away from the unit cell surface, in other words, they are far away from the substrate. The evanescent field leaked into the substrate is very little. Therefore, this kind CMM is not sensitive to the existence of the substrate.

Figures 5(e)–5(j) are the retrieval results of the optical parameters ε, μ, and κ. All these curves behave well. We fit these curves using the analytical formulas given by Eqs. (29) derived from the Ω-particle resonator model (see Appendix A). For with substrate only, the fitted parameters are as following: εb = 3.1738, μb = 0.9799, ω 0 = 1.8651THz, γ = 0.05519 ω 0, Ωε = 0.1537, Ωμ = 0.0627, and Ωκ = 0.0986. For without substrate, they are very close to those with substrate. εb = 3.1736, μb = 0.9798, ω 0 = 1.8713 THz, γ = 0.05463 ω 0, Ωε = 0.1560, Ωμ = 0.0625, and Ωκ = 0.0993. From these parameters, we can again see that the substrate has very little influence on the four-folded rotated Ω-particle CMMs. The substrate only lowers the frequency of the resonance by 0.3%.

Fig. 5. (a)–(d) are the simulation results of the amplitude and the phase of the reflection and transmission for the four-folded rotated Ω-particle CMM slabs. They are extracted using (19). R′ is the reflection for the incident wave from the opposite direction. (e)–(j) show the optical parameters ε, μ, and κ. Re/Im denotes the real/imaginary part of the value. The subscripts s and f denotes the retrieval results from the numerical simulation and the fitting results using Eqs. (29) respectively. The left is with substrate (n=1.27) only and the right is for the free standing sample.

4. Conclusion

In summary, we have analyzed the wave propagation in chiral metamaterials and followed the similar procedure that was done in ordinary metamaterials to do the parameter retrieval for CMM slabs. Based on the transfer matrix technique, we extended the parameter retrieval technique to be able to treat samples with substrates and extra top layers. We studied the influence of the substrate and top layers on the thin chiral metamaterial slabs.We found that the substrate could lower the frequency of the resonance and induce the homogeneous chiral metamaterials to be inhomogeneous. The sensitivity of the influence relates to the strength of the leaked evanescent field in the substrate. We also fitted the retrieval results using analytical expressions derived from Ω-particle chiral model based on the effective LC circuit mode. We found they agree with each other very well.

A. Derive the forms of the constitutive parameters from the Ω-particle resonator model

Fig. 6. Schematics of the single right-handed (left) and left-handed (right) Ω-particle resonators.

Figure 6 gives the schematics of the Ω-particle resonator. The structure consists of an open circular loop and two short wires. The area of the loop is S = πr 2 and the length of each wire is l. The wires are perpendicular to the loop and connected to the ends of the open loop. If the Ω-particle is in a homogeneous external field, the driving electric potential can be written as:

U=2lE0±μ0SḢ0,
(21)

where ± signs correspond to right-handed and left-handed helix resonators, The hat-dot denotes the first time derivative. Applying the effective RLC circuit model, we have

Lİ+qC+RI=U,I=q̇.
(22)

Let α=lL , β=μ0AL , γ=RL , and ω02=1LC . Then assuming the external fields are plane waves, ~ e−iωt, and considering stationary solutions, we get the following equation:

(ω2iωγ+ω02)q=αE0±iωβH0,
(23)

then, we have

q=αω2iωγ+ω02E0±iωβω2iωγ+ω02H0.
(24)

Therefore, the electric dipole, p = q l, and the magnetic dipole, m = ±I A = ± A, can be written as:

p=α1ω02ω2iωγE0+±iωβ1ω02ω2iωγH0,
(25a)
m=iωαAω02ω2iωγE0+ω2βAω02ω2iωγH0,
(25b)

where, αA=1μ0βl , l = l 0, and A = A 0; 0 is the unit vector along the direction of the wires, i.e., the up direction. The electric polarization and the magnetic polarization are defined as P=ΣpV0 and M=ΣmV0 respectively, where the summation is done in the unit cell and V 0 denotes the volume of the unit cell. Assuming there are N resonators in one unit cell, the electric polarization and the magnetic polarization can be written as:

P=NV0αlω02ω2iωγE+NV0±iωβlω02ω2iωγH,
(26a)
M=NV0iωαAω02ω2iωγE+NV0ω2βAω02ω2iωγH.
(26b)

Here, the directions of l and A are merged into E 0 and H 0 to form the vectors of E and H.

Inserting Eqs. (26) to the relation D = ε 0 E + P and B = μ 0 H + μ 0 M, we have

D=ε0E+αlNV0ω02ω2iωγE+±iωβlNV0ω02ω2iωγH,
(27a)
B=μ0H+iμ0ωαANV0ω02ω2iωγE+ω2μ0βANV0ω02ω2iωγH.
(27b)

Comparing Eqs. (27) with Eq. (1), we can obtain the relative permittivity ε, permeability μ, and the chirality κ:

ε=1+αlNV0ε0ω02ω2iωγ,
(28a)
μ=1+ω2βANV0ω02ω2iωγ,
(28b)
κ=±ωβlc0NV0ω02ω2iωγ=±ωμ0c0αANV0ω02ω2iωγ.
(28c)

Equations (28) are valid for the case that the metal chiral structure stands in free space. If it’s merged into a background material with εb and μb, Eqs. (28) should be modified as follows:

ε=εb+Ωεω02ω02ω2iωγ,
(29a)
μ=μb+Ωμω2ω02ω2iωγ,
(29b)
κ=Ωκω0ωω02ω2iωγ,
(29c)

where εb is usually larger than one; μb is usually very close to one. Ωε, Ωμ, and Ωκ are the coefficients of the resonance terms in ε, μ, and κ, i.e. Ωε=αlNV0ε0ω02 , Ωμ=βANV0 , and Ωκ=βlc0NV0ω0=μ0c0αANV0ω0 , where c 0 is the speed of light in vacuum. They describe the strength of the resonance. The expressions of the frequency dependence of ε and μ given by Eqs. (29a) and (29b) are the same as those in traditional metamaterials [37

37. J. B. Pendry, A. J. Holden, D. J. Robbins, and W. J. Stewart, “Magnetism from conductors and enhanced nonlinear phenomena,” IEEE Trans. Microw. Theory Tech.47, 2075 (1999).

]. The linear ω dependence of κ is the same as Condon model for the homogeneous chiral molecular media [38

38. E. U. Condon, “Theories of optical rotatory power,” Rev. Mod. Phys. 9, 432–457 (1937). [CrossRef]

]. This is a general feature of natural optically active materials [39

39. L.D. Landau, E. M. Lifshitz, and L. P. Pitaevskii, Electrodynamics of Continuous Media (2nd ed., Pergamon Press, Oxford, 1984), §104, p.362–367.

].

Because α=lL and β=μ0AL , we then can obtain the following relation:

Ωκ2=ΩεΩμ,
(30)

which seems to limit the possibility of obtaining large Ωκ in these designs composited by the passive materials only.

Acknowledgements

Work at Ames Laboratory was supported by the Department of Energy (Basic Energy Sciences) under contract No. DE-AC02-07CH11358. This work was partially supported by the European Community FET project PHOME (contract No. 213390). The author Rongkuo Zhao specially acknowledges the China Scholarship Council (CSC) for financial support.

References and links

1.

J. B. Pendry, “A chiral route to negative refraction,” Science 306, 1353–1355 (2004). [CrossRef] [PubMed]

2.

S. Tretyakov, I. Nefedov, A. Sihvola, S. Maslovski, and C. Simovski, “Waves and energy in chiral nihility,” J. Electromagn. Waves Appl. 17, 695–706 (2003). [CrossRef]

3.

C. Monzon and D. W. Forester, “Negative refraction and focusing of circularly polarized waves in optically active media,” Phys. Rev. Lett. 95, 123904 (2005). [CrossRef] [PubMed]

4.

S. Tretyakov, A. Sihvola, and L. Jylha, “Backward-wave regime and negative refraction in chiral composites,” Photonics Nanostruct. Fundam. Appl. 3, 107 (2005). [CrossRef]

5.

V. Yannopapas, “Negative index of refraction in artificial chiral materials,” J. Phys. Condens. Matter 18, 6883–6890 (2006). [CrossRef]

6.

V. M. Agranovich, Y. N. Gartstein, and A. A. Zakhidov, “Negative refraction in gyrotropic media,” Phys. Rev. B 73 , 045114 (2006). [CrossRef]

7.

C. Zhang and T. J. Cui, “Negative reflections of electromagnetic waves in a strong chiral medium,” Appl. Phys. Lett. 91, 194101 (2007). [CrossRef]

8.

J. K. Gansel, M. Thiel, M. S. Rill, M. Decker, K. Bade, V. Saile, G. V. Freymann, S. Linden, and M. Wegener, “Gold helix photonic metamaterial as broadband circular polarizer,” Science 325, 1513–1515 (2009). [CrossRef] [PubMed]

9.

E. Plum, J. Zhou, J. Dong, V. A. Fedotov, Th. Koschny, C. M. Soukoulis, and N. I. Zheludev, “Metamaterial with negative index due to chirality,” Phys. Rev. B 79, 035407 (2009). [CrossRef]

10.

J. Zhou, J. Dong, B. Wang, Th. Koschny, M. Kafesaki, and C. M. Soukoulis, “Negative refractive index due to chirality,” Phys. Rev. B 79, 121104 (2009). [CrossRef]

11.

J. Dong, J. Zhou, Th. Koschny, and C. M. Soukoulis, “Bi-layer cross chiral structure with strong optical activity and negative refractive index,” Opt. Express 17, 14172–14179 (2009). [CrossRef] [PubMed]

12.

E. Plum, V. A. Fedotov, and N. I. Zheludev, “Optical activity in extrinsically chiral metamaterial,” Appl. Phys. Lett. 93, 191911 (2008). [CrossRef]

13.

E. Plum, X.-X. Liu, V. A. Fedotov, Y. Chen, D. P. Tsai, and N. I. Zheludev, “Metamaterials: optical activity without chirality,” Phys. Rev. Lett. 102, 113902 (2009). [CrossRef] [PubMed]

14.

L. Jelinek, R. Marquěs, F. Mesa, and J. D. Baena, “Periodic arrangements of chiral scatterers providing negative refractive index bi-isotropic media,” Phys. Rev. B 77, 205110 (2008). [CrossRef]

15.

B. Wang, J. Zhou, Th. Koschny, and C. M. Soukoulis, “Nonplanar chiral metamaterials with negative index,” Appl. Phys. Lett. 94, 151112 (2009). [CrossRef]

16.

V. Yannopapas, “Circular dichroism in planar nonchiral plasmonic metamaterials,” Opt. Lett. 34, 632–634 (2009). [CrossRef] [PubMed]

17.

S. Zhang, Y. S. Park, J. Li, X. Lu, W. Zhang, and X. Zhang, “Negative refractive index in chiral metamaterials,” Phys. Rev. Lett. 102, 023901 (2009). [CrossRef] [PubMed]

18.

E. Plum, V. A. Fedotov, A. S. Schwanecke, Y. Chen, and N. I. Zheludev, “Giant optical gyrotropy due to electromagnetic coupling,” Appl. Phys. Lett. 90, 223113 (2007). [CrossRef]

19.

M. Kuwata-Gonokami, N. Saito, Y. Ino, M. Kauranen, K. Jefimovs, T. Vallius, J. Turunen, and Y. Svirko, “Giant optical activity in quasi-two-dimensional planar nanostructures,” Phys. Rev. Lett. 95, 227401 (2005). [CrossRef] [PubMed]

20.

M. Decker, R. Zhao, C.M. Soukoulis, S. Linden, and M. Wegener, “Twisted split-ring-resonator photonic metamaterial with huge optical activity,” Opt. Lett. 35, 1593–1595 (2010). [CrossRef] [PubMed]

21.

M. Decker, M. Ruther, C. E. Kriegler, J. Zhou, C. M. Soukoulis, S. Linden, and M. Wegener, “Strong optical activity from twisted-cross photonic metamaterials,” Opt. Lett. 34, 2501–1503 (2009). [CrossRef] [PubMed]

22.

M. Decker, M. W. Klein, M. Wegener, and S. Linden, “Circular dichroism of planar chiral magnetic metamaterials,” Opt. Lett. 32, 856–858 (2007). [CrossRef] [PubMed]

23.

D. R. Smith, S. Schultz, P. Markoš, and C. M. Soukoulis, “Determination of effective permittivity and permeability of metamaterials from reflection and transmission coefficients,” Phys. Rev. B 65, 195104 (2002). [CrossRef]

24.

X. Chen, T. M. Grzegorczyk, B. I. Wu, J. Pacheco, and J. A. Kong, “Robust method to retrieve the constitutive effective parameters of metamaterials,” Phys. Rev. E 70, 016608 (2004). [CrossRef]

25.

Th. Koschny, M. Kafesaki, E. N. Economou, and C. M. Soukoulis, “Effective medium theory of left-handed materials,” Phys. Rev. Lett. 93, 107402 (2004). [CrossRef] [PubMed]

26.

Th. Koschny, P. Markoš, E. N. Economou, D. R. Smith, D. C. Vier, and C. M. Soukoulis, “Impact of inherent periodic structure on effective medium description of left-handed and related metamaterials,” Phys. Rev. B 71, 245105 (2005). [CrossRef]

27.

D. R. Smith, D. C. Vier, Th. Koschny, and C. M. Soukoulis, “Electromagnetic parameter retrieval from inhomogeneous metamaterials,” Phys. Rev. E 71, 036617 (2005). [CrossRef]

28.

Z. Li, K. Aydin, and E. Ozbay, “Determination of the effective constitutive parameters of bianisotropic metamaterials from reflection and transmission coefficients,” Phys. Rev. E 79, 026610 (2009). [CrossRef]

29.

B. Wang, J. Zhou, Th. Koschny, M. Kafesaki, and C. M. Soukoulis, “Chiral metamaterials: simulations and experiments,” J. Opt. A: Pure Appl. Opt. 11, 114003 (2009). [CrossRef]

30.

D. H. Kwon, D. H. Werner, A. V. Kildishev, and V. M. Shalaev, “Material parameter retrieval procedure for general bi-isotropic metamaterials and its application to optical chiral negative-index metamaterial design,” Opt. Express 16, 11822–11829 (2008). [CrossRef] [PubMed]

31.

I. V. Lindell et al., Electromagnetic Waves in Chiral and Bi-Isotropic Media (Artech House, Boston · London, 1994).

32.

A. Serdyukov et al., Electromagnetics of Bi-anisotropic Materials: Theory and Applications (Gordon and Breach Science Publishers, Amsterdam, 2001).

33.

Some people (see, for instance, A. Lakhtakia et al., “Reflection of plane waves at planar achiral-chiral interfaces: independence of the reflected polarization state from the incident polarization state,” J. Opt. Soc. Am. A7, 1654 (1990).) use the Drude-Born-Fedorov relations: D = ε(B + β∇ × E), B = μ(H + β∇ × H), where β characterizes the strength of the chirality. They can be brought to the same form. The transformations between the parameters of the two systems are given in Ref. 26. [CrossRef]

34.

CST MICROWAVE STUDIO (CST MWS) is a specialist tool for the 3D EM simulation of high frequency components, http://www.cst.com/Content/Products/MWS/Overview.aspx.

35.

P. Markoš and C. M. Soukoulis, Wave Propagation: From Electrons to Photonic crystals and Left-Handed Materials (Princeton University Press, Princeton, 2008).

36.

R. Zhao, J. Zhou, Th. Koschny, E. N. Economou, and C. M. Soukoulis, “Repulsive Casimir force in chiral metamaterials,” Phys. Rev. Lett. 103, 103602 (2009). [CrossRef] [PubMed]

37.

J. B. Pendry, A. J. Holden, D. J. Robbins, and W. J. Stewart, “Magnetism from conductors and enhanced nonlinear phenomena,” IEEE Trans. Microw. Theory Tech.47, 2075 (1999).

38.

E. U. Condon, “Theories of optical rotatory power,” Rev. Mod. Phys. 9, 432–457 (1937). [CrossRef]

39.

L.D. Landau, E. M. Lifshitz, and L. P. Pitaevskii, Electrodynamics of Continuous Media (2nd ed., Pergamon Press, Oxford, 1984), §104, p.362–367.

OCIS Codes
(160.4760) Materials : Optical properties
(160.1585) Materials : Chiral media
(160.3918) Materials : Metamaterials

ToC Category:
Metamaterials

History
Original Manuscript: April 5, 2010
Revised Manuscript: May 27, 2010
Manuscript Accepted: June 4, 2010
Published: June 23, 2010

Citation
Rongkuo Zhao, Thomas Koschny, and Costas M. Soukoulis, "Chiral metamaterials: retrieval of the effective parameters with and without substrate," Opt. Express 18, 14553-14567 (2010)
http://www.opticsinfobase.org/oe/abstract.cfm?URI=oe-18-14-14553


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References

  1. J. B. Pendry, “A chiral route to negative refraction,” Science 306, 1353–1355 (2004). [CrossRef] [PubMed]
  2. S. Tretyakov, I. Nefedov, A. Sihvola, S. Maslovski, and C. Simovski, “Waves and energy in chiral nihility,” J. Electromagn. Waves Appl. 17, 695–706 (2003). [CrossRef]
  3. C. Monzon, and D. W. Forester, “Negative refraction and focusing of circularly polarized waves in optically active media,” Phys. Rev. Lett. 95, 123904 (2005). [CrossRef] [PubMed]
  4. S. Tretyakov, A. Sihvola, and L. Jylha, “Backward-wave regime and negative refraction in chiral composites,” Photonics Nanostruct. Fundam. Appl. 3, 107 (2005). [CrossRef]
  5. V. Yannopapas, “Negative index of refraction in artificial chiral materials,” J. Phys. Condens. Matter 18, 6883–6890 (2006). [CrossRef]
  6. V. M. Agranovich, Y. N. Gartstein, and A. A. Zakhidov, “Negative refraction in gyrotropic media,” Phys. Rev. B 73, 045114 (2006). [CrossRef]
  7. C. Zhang, and T. J. Cui, “Negative reflections of electromagnetic waves in a strong chiral medium,” Appl. Phys. Lett. 91, 194101 (2007). [CrossRef]
  8. J. K. Gansel, M. Thiel, M. S. Rill, M. Decker, K. Bade, V. Saile, G. V. Freymann, S. Linden, and M. Wegener, “Gold helix photonic metamaterial as broadband circular polarizer,” Science 325, 1513–1515 (2009). [CrossRef] [PubMed]
  9. E. Plum, J. Zhou, J. Dong, V. A. Fedotov, Th. Koschny, C. M. Soukoulis, and N. I. Zheludev, “Metamaterial with negative index due to chirality,” Phys. Rev. B 79, 035407 (2009). [CrossRef]
  10. J. Zhou, J. Dong, B. Wang, Th. Koschny, M. Kafesaki, and C. M. Soukoulis, “Negative refractive index due to chirality,” Phys. Rev. B 79, 121104 (2009). [CrossRef]
  11. J. Dong, J. Zhou, Th. Koschny, and C. M. Soukoulis, “Bi-layer cross chiral structure with strong optical activity and negative refractive index,” Opt. Express 17, 14172–14179 (2009). [CrossRef] [PubMed]
  12. E. Plum, V. A. Fedotov, and N. I. Zheludev, “Optical activity in extrinsically chiral metamaterial,” Appl. Phys. Lett. 93, 191911 (2008). [CrossRef]
  13. E. Plum, X.-X. Liu, V. A. Fedotov, Y. Chen, D. P. Tsai, and N. I. Zheludev, “Metamaterials: optical activity without chirality,” Phys. Rev. Lett. 102, 113902 (2009). [CrossRef] [PubMed]
  14. L. Jelinek, R. Marquěs, F. Mesa, and J. D. Baena, “Periodic arrangements of chiral scatterers providing negative refractive index bi-isotropic media,” Phys. Rev. B 77, 205110 (2008). [CrossRef]
  15. B. Wang, J. Zhou, Th. Koschny, and C. M. Soukoulis, “Nonplanar chiral metamaterials with negative index,” Appl. Phys. Lett. 94, 151112 (2009). [CrossRef]
  16. V. Yannopapas, “Circular dichroism in planar nonchiral plasmonic metamaterials,” Opt. Lett. 34, 632–634 (2009). [CrossRef] [PubMed]
  17. S. Zhang, Y. S. Park, J. Li, X. Lu, W. Zhang, and X. Zhang, “Negative refractive index in chiral metamaterials,” Phys. Rev. Lett. 102, 023901 (2009). [CrossRef] [PubMed]
  18. E. Plum, V. A. Fedotov, A. S. Schwanecke, Y. Chen, and N. I. Zheludev, “Giant optical gyrotropy due to electromagnetic coupling,” Appl. Phys. Lett. 90, 223113 (2007). [CrossRef]
  19. M. Kuwata-Gonokami, N. Saito, Y. Ino, M. Kauranen, K. Jefimovs, T. Vallius, J. Turunen, and Y. Svirko, “Giant optical activity in quasi-two-dimensional planar nanostructures,” Phys. Rev. Lett. 95, 227401 (2005). [CrossRef] [PubMed]
  20. M. Decker, R. Zhao, C. M. Soukoulis, S. Linden, and M. Wegener, “Twisted split-ring-resonator photonic metamaterial with huge optical activity,” Opt. Lett. 35, 1593–1595 (2010). [CrossRef] [PubMed]
  21. M. Decker, M. Ruther, C. E. Kriegler, J. Zhou, C. M. Soukoulis, S. Linden, and M. Wegener, “Strong optical activity from twisted-cross photonic metamaterials,” Opt. Lett. 34, 1501–1503 (2009). [CrossRef] [PubMed]
  22. M. Decker, M. W. Klein, M. Wegener, and S. Linden, “Circular dichroism of planar chiral magnetic metamaterials,” Opt. Lett. 32, 856–858 (2007). [CrossRef] [PubMed]
  23. D. R. Smith, S. Schultz, P. Markoš, and C. M. Soukoulis, “Determination of effective permittivity and permeability of metamaterials from reflection and transmission coefficients,” Phys. Rev. B 65, 195104 (2002). [CrossRef]
  24. X. Chen, T. M. Grzegorczyk, B. I. Wu, J. Pacheco, and J. A. Kong, “Robust method to retrieve the constitutive effective parameters of metamaterials,” Phys. Rev. E Stat. Nonlin. Soft Matter Phys. 70, 016608 (2004). [CrossRef]
  25. Th. Koschny, M. Kafesaki, E. N. Economou, and C. M. Soukoulis, “Effective medium theory of left-handed materials,” Phys. Rev. Lett. 93, 107402 (2004). [CrossRef] [PubMed]
  26. Th. Koschny, P. Markoš, E. N. Economou, D. R. Smith, D. C. Vier, and C. M. Soukoulis, “Impact of inherent periodic structure on effective medium description of left-handed and related metamaterials,” Phys. Rev. B 71, 245105 (2005). [CrossRef]
  27. D. R. Smith, D. C. Vier, Th. Koschny, and C. M. Soukoulis, “Electromagnetic parameter retrieval from inhomogeneous metamaterials,” Phys. Rev. E Stat. Nonlin. Soft Matter Phys. 71, 036617 (2005). [CrossRef]
  28. Z. Li, K. Aydin, and E. Ozbay, “Determination of the effective constitutive parameters of bianisotropic metamaterials from reflection and transmission coefficients,” Phys. Rev. E Stat. Nonlin. Soft Matter Phys. 79, 026610 (2009). [CrossRef]
  29. B. Wang, J. Zhou, Th. Koschny, M. Kafesaki, and C. M. Soukoulis, “Chiral metamaterials: simulations and experiments,” J. Opt. A, Pure Appl. Opt. 11, 114003 (2009). [CrossRef]
  30. D. H. Kwon, D. H. Werner, A. V. Kildishev, and V. M. Shalaev, “Material parameter retrieval procedure for general bi-isotropic metamaterials and its application to optical chiral negative-index metamaterial design,” Opt. Express 16, 11822–11829 (2008). [CrossRef] [PubMed]
  31. I. V. Lindell,  et al., Electromagnetic Waves in Chiral and Bi-Isotropic Media (Artech House, Boston · London, 1994).
  32. A. Serdyukov,  et al., Electromagnetics of Bi-anisotropic Materials: Theory and Applications (Gordon and Breach Science Publishers, Amsterdam, 2001).
  33. Some people [see, for instance, A. Lakhtakia et al., “Reflection of plane waves at planar achiral-chiral interfaces: independence of the reflected polarization state from the incident polarization state,” J. Opt. Soc. Am. A 7, 1654 (1990).] use the Drude-Born-Fedorov relations: D = ε (B + β∇ ×E), B = μ(H + β∇ ×H), where β characterizes the strength of the chirality. They can be brought to the same form. The transformations between the parameters of the two systems are given in Ref. 26. [CrossRef]
  34. CST MICROWAVE STUDIO (CST MWS) is a specialist tool for the 3D EM simulation of high frequency components, http://www.cst.com/Content/Products/MWS/Overview.aspx.
  35. P. Markoš, and C. M. Soukoulis, Wave Propagation: From Electrons to Photonic crystals and Left-Handed Materials (Princeton University Press, Princeton, 2008).
  36. R. Zhao, J. Zhou, Th. Koschny, E. N. Economou, and C. M. Soukoulis, “Repulsive Casimir force in chiral metamaterials,” Phys. Rev. Lett. 103, 103602 (2009). [CrossRef] [PubMed]
  37. J. B. Pendry, A. J. Holden, and D. J. Robbins, “andW. J. Stewart,“ Magnetism from conductors and enhanced nonlinear phenomena,” IEEE Trans. Microw. Theory Tech. 47, 2075 (1999).
  38. E. U. Condon, “Theories of optical rotatory power,” Rev. Mod. Phys. 9, 432–457 (1937). [CrossRef]
  39. L. D. Landau, E. M. Lifshitz, and L. P. Pitaevskii, Electrodynamics of Continuous Media (2nd ed., Pergamon Press, Oxford, 1984), §104, p.362–367.

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