Wave Propagation 2010 Part 15 pdf

(a) Composite A (Sendust 25 vol%, Al 25 vol%) (b) Composite B (Sendust 12.5 vol%, Al 37.5 vol%) (c) Composite C (Sendust 10 vol%, Al 40 vol%) Fig. 13. Frequency dependences of return loss for composites made of both sendust and aluminum particles dispersed in polystyrene resin. The frequency range is from 1 to 10 GHz. (a) Composite B (Sendust 12.5 vol%, Al 37.5 vol%) (b) Composite C (Sendust 10 vol%, Al 40 vol%) Fig. 14. Frequency dependences of return loss for composites made of both sendust and aluminum particles dispersed in polystyrene resin. The frequency range is from 15 to 40 GHz. less than −20 dB at frequencies above 15 GHz and the normalized −20 dB bandwidth of these two composites was broader than that for the composite made of only sendust. In addition, the sample thicknesses where the return loss is less than −20 dB were very thin. In particular, composite C had high values of normalized −20 dB bandwidth in spite of the high frequency range and the frequency where the return loss is less than −20 dB can be selected by changing the sample thickness in the range from 0.5 to 0.7 mm. It is concluded from these results that the absorption characteristics of the composite made of sendust in the high frequency range could be improved by adding aluminum particles. Moreover, aluminum is low cost, abundant chemical element, and light wight. For example, the mass densities of composites A, B and C were approximately 2.4, 2.1, and 2.0 g / cm 3 , respectively, while the mass density of the composite made of 53 vol%-sendust is approximately 3.5 g / cm 3 . Therefore, a light-weight absorber can be fabricated by incorporating both sendust and aluminum. 4. Conclusion Frequency dependences of μ r * , ε r * , and absorption characteristics for the composite made of sendust were investigated in the frequency range from 100 MHz to 40 GHz. By the comparison with the composite made of various magnetic material, the mechanism of the frequency dependences of μ r ’ and μ r ” was found to be the magnetic resonance in the low frequency range and the magnetic moment in the high frequency range. The values of μ r ’ for the composite made of sendust were less than unity and the values of μ r ” was not zero like the composite made of ferrite particles dispersed in polystyrene resin. Thus, the composite made of sendust had a return loss of less than −20 dB at frequencies above 10 GHz in addition to the absorption at frequencies of several GHz. From these result, it is concluded that a practical absorber suitable for frequencies above 10 GHz is possible using a composite made of sendust. The values of μ r ’ and μ r ” for the composite made of both sendust and aluminum particles dispersed in polystyrene resin could be controlled by changing the volume mixture ratio of sendust and aluminum. Thus, the absorption characteristics at frequencies above 10 GHz for the composite made of only sendust could be improved by using the composite made of both sendust and aluminum by selecting a suitable volume mixture ratio of sendust and aluminum, and a flexible design of an absorber was proposed. 5. Acknowledgement This research was supported by the Japan Society for the Promotion of Science (JSPS) and Grant-in-Aid for JSPS Fellows. 6. References a Kasagi, T., Tsutaoka, T., & Hatakeyama, K. (1999). Particle size effect on the complex permeability for permalloy composite materials. IEEE Trans. Magn., Vol. 35, No. 5, pp. 3424-3426, 0018-9464 b Kasagi, T., Tsutaoka, T., & Hatakeyama, K. (2006). Negative Permeability Spectra in Permalloy Granular Composite Materials. Appl. Phys. Lett., Vol. 88, 17502, 0003-6951 Lim, K. M., Lee, K. A., Kim, M. C., & Park, C. G. (2005). Complex permeability and electromagnetic wave absorption properties of amorphous alloy-epoxy composites. J. Non-Cryst. Solids., Vol. 351, pp. 75-83, 0022-3093 Nishikata, A. (2002). New Radiowave Absorbers Using Magnetic Loss Caused by Metal Particles’ Internal Eddy Current. Proceedings of EMC EUROPE 2002 International Symposium on Electromagnetic Compatibility, pp. 697-702, Sorrento Italy, September 2002 Song, J. M., Kim, D. I., Choi, J. H., & Jeung, J. H., (2005). EM Wave Absorbers Prepared with Sendust. APMC2005 Proceedings, 0-7803-9433, Suzhou China, December 2005 Wada, Y., Asano, N., Sakai, K., & Yoshikado, S. (2008). Preparation and Evaluation of Composite Electromagnetic Wave Absorbers Made of Fine Aluminum Particles Dispersed in Polystyrene Medium. PIERS Online, Vol. 4, pp. 838-845, 1931-7360 1. Introduction Interest continues to grow in controlling the propagation of electromagnetic waves by utilizing periodically or randomly arranged artificial structures made of metal, dielectric, and other materials. When the size o f the constituent structures and the separation between the neighboring structures are much smaller than the wavelength of the electromagnetic waves, the structure arrays behave as a continuous medium for the electromagnetic waves. That is, macroscopic medium parameters such as effective permittivity and permeability can be defined for t he array. The artificial continuous medium is called a “metamaterial.” In the frequency region below the microwave frequency, the use of metallic structures as artificial media has been studied since the late 1940’s (Collin, 1990). At first, only control of the permittivity was studied and not that of the permeability. However, Pendry et al. (1999) proposed methods for fabricating artificial magnetic media, namely, magnetic metamaterials, which were built from nonmagnetic conductors. It was shown that not only can relative permeability be changed from unity but it also can have a negative value. Although the relative permeabilities of naturally occurring media are almost unity in such high frequency regions as microwave, terahertz, and optical regions, the restriction that the relative permeability is almost unity can be removed using the metamaterial. Moreover, the magnetic metamaterial enabled us to fabricate media with simultaneous negative p ermittivity and permeability, or negative refractive index media that were predicted by Veselago (1968). In fact, Shelby et al. (2001) made the first experimental verification of a n egative refractive index metamaterial in the microwave region. This increased re searcher interest in metamaterials. It was not possible to independently control the wavenumber and the wave impedance in a medium until magnetic metamaterials were developed. The wavenumber is related to the propagation and r efraction of electromagnetic waves, and the wave impedance is connected with the r eflection. Phenomena about electromagnetic waves are described by these two quantities. In dielectric media, both of the wavenumber and wave impedance change with a change of the permittivity, and we cannot set these parameters independently. However, the wavenumber and wave impedance can be changed independently in metamaterials because we can control the permeability as well as the permittivity with metamaterials. By utilizing the flexibility of the wavenumber and wave impedance in metamaterials, such novel phenomena as a perfect lens (superlens) (Pendry, 2000; Lagarkov & Kissel, 2004), a hyperlens (Jacob et al., 2006; Liu et al., 2007), and an invisibility cloak (Pendry et al., 2006; Leonhardt, 2006; Schurig et al., 2006) have been proposed and verified experimentally. No-Reflection Phenomena for Chiral Media Yasuhiro Tamayama, Toshihiro Nakanishi, Kazuhiko Sugiyama, and Masao Kitano Department of Electronic Science and Engineering, Kyoto University Japan 20 2 Electromagnetic Wave s In this chapter, we focus on Brewster’s no-reflection effect in metamaterials. The Brewster condition is one of the laws of reflection and refraction of electromagnetic waves at a boundary between two distinct media (Saleh & Teich, 2007). For a particular angle of incidence, known as the Brewster angle, the reflected wave vanishes. The Brewster effect is applied in optical instruments, for example, to generate completely polarized waves from unpolarized waves only with a glass plate and to suppress the insertion losses of intracavity elements. The Brewster effect arises for transverse-magnetic (TM) waves [transverse-electric (TE) waves] at an interface between two distinct dielectric (magnetic) media. Hence, this phenomenon can o nly be observed for TM waves and not for TE waves in naturally occurring media that do not respond to high-frequency magnetic fields. However, since we can fabricate magnetic media in high frequency regions with a metamaterial technique (Pendry et al., 1999; Holloway et al ., 2003; Zhang et al., 2005), the Brewster condition for TE waves can be satisfied (Doyle, 1980; Futterman, 1995; Fu et al., 2005). In fact, the TE Brewster effect has been experimentally observed in the microwave region (Tamayama et al., 2006) and also in the optical region ( Watanabe et al., 2008). In addition to permittivity and permeability, chirality parameter and non-reciprocity parameter can be controlled using metamaterials. It is also possible to control the anisotropy in electromagnetic r esponses. Therefore, investigating the no-reflection condition for generalized media is important. Brewster’s condition has been studied for anisotropic media (Grzegorczyk e t al., 2005; Tanaka et al., 2006; Shen et al., 2006; Shu et al., 2007), chiral media (bi-isotropic media) (Bassiri et al., 1988; Lindell et al., 1994), and bi-anisotropic media (Lakhtakia, 1992). However, thus far, the explicit relations among the medium parameters for achieving non-reflectivity in chiral and bi-anisotropic media have not been determined. The purpose of t his chapter is to d erive the explicit relation among the permittivity, permeability, and chirality parameter of the chiral medium that satisfy the no-reflection condition for a planar interface between a vacuum and the chi ral medium. The no-reflection condition is derived from the vanishing eigenvalue condition of the reflection Jones matrix. The analysis can be largely simplified by decomposing the reflection Jones matrix into the unit and Pauli matrices (Tamayama et al., 2008). We find that in general chiral media, the no-reflection condition is satisfied by elliptically polarized incident waves for at most one particular angle of incidence. This is merely a natural extension of the usual Brewster effect for achiral (nonchiral) media. When the wave impedance and the absolute value of the wavenumber i n the chiral medium equal those in a vacuum for one of the circularly polarized (CP) waves, the corresponding CP wave is transmitted to the medium without reflection for all angles of incidence. The no-reflection effect for chiral nihility media resembles that for achiral media. We provide a fini te-difference time-domain (FDTD) analysis ( Taflove & Hagness, 2005) of the no-reflection effect for CP waves. We analyze the scatterings of electromagnetic waves by a cylinder and a triangular prism made of a chiral medium whose medium parameters satisfy the no-reflection condition for one of the CP waves. The simulation demonstrates that the corresponding CP wave is not scattered and the other CP wave is largely scattered. We show that a circular polarizing beam splitter can be achieved by utilizing the no-reflection effect. 2. Propagation of electromagnetic waves in chiral media We calculate the wavenumber and wave impedance i n chiral media. The constitutive equations for chiral media have several types of expressions. The Post and Tellegen representations are mainly used as the constitutive e quations. The Post representation is 416 Wave Propagation No-Reflection Phenomena for Chiral Media 3 written as D D D = ε P E E E −iξ P B B B, H H H = μ −1 P B B B −iξ P E E E,(1) and the Tellegen representation is written a s D D D = ε T E E E −iκ T H H H, B B B = μ T H H H + iκ T E E E,(2) where ε P, T is the permittivity, μ P, T is the permeability, and ξ p and κ T are the chirality parameters. The subscript P (T) stands f or the Post (Tellegen) representation. These representations are equivalent and interchangeable with the following transformation (Lakhtakia, 1992): ε T = ε P + μ P ξ 2 P , μ T = μ P , κ T = μ P ξ P .(3) In thi s chapter, we consistently use the Post representation and omit the subscript P for simplicity. Maxwell’s equation for a monochromatic plane electromagnetic w ave is given by k k k × E E E = ωB B B, k k k × H H H = −ωD D D,(4) where k k k is the wavenumber vector and ω is the angular frequency. Substituting Eq. (1) into Eq. (4) and assuming k k k = ke e e z (e e e z is the unit v ector in the z-direction), we obtain k ⎡ ⎢ ⎢ ⎣ 1 O 1 1 O 1 ⎤ ⎥ ⎥ ⎦ ⎡ ⎢ ⎢ ⎣ E x E y H x H y ⎤ ⎥ ⎥ ⎦ = ω ⎡ ⎢ ⎢ ⎣ 0iμξ 0 μ −iμξ 0 −μ 0 0 −(ε + μξ 2 ) 0iμξ ε + μξ 2 0 −iμξ 0 ⎤ ⎥ ⎥ ⎦ ⎡ ⎢ ⎢ ⎣ E x E y H x H y ⎤ ⎥ ⎥ ⎦ .(5) From the condition for a non-trivial solution of Eq. (5), we have k = ±ω(  εμ + μ 2 ξ 2 + μξ), ±ω(  εμ + μ 2 ξ 2 −μξ).(6) After substitution of the derived wavenumber into Eq. (5), the relation among the wavenumber and the electromagnetic fields is obtained and summarized in Tabl e 1. Here we define the wave impedance Z c of the chiral medium as Z c =  μ ε + μξ 2 .(7) The eigenpolarizations in chiral media are found to be CP waves because E y /E x = ±iis satisfied. Equations (6) and (7) contain double-valued square root functions. Thus, the wavenumber and wave impedance cannot be calculated without ambiguity. To choose the correct branch, we diagonalize Eq. (5). By using the transformation matrix U = 1 2 ⎡ ⎢ ⎢ ⎣ 11 1 1 −ii i −i iZ −1 c iZ −1 c −iZ −1 c −iZ −1 c Z −1 c −Z −1 c Z −1 c −Z −1 c ⎤ ⎥ ⎥ ⎦ , U −1 = 1 2 ⎡ ⎢ ⎢ ⎣ 1i −iZ c Z c 1 −i −iZ c −Z c 1 −iiZ c Z c 1i iZ c −Z c ⎤ ⎥ ⎥ ⎦ ,(8) 417 No-Reflection Phenomena for Chiral Media 4 Electromagnetic Wave s k k + −k + k − −k − E x 1 1 1 1 E y −i i i −i H x iZ −1 c iZ −1 c −iZ −1 c −iZ −1 c H y Z −1 c −Z −1 c Z −1 c −Z −1 c Table 1. Relation am ong wavenumber and electromagnetic fields in chiral media. Ratio of each electromagnetic field component to E x is written for each eigenmode. Here k ± = ω(  εμ + μ 2 ξ 2 ±μξ)=ω[Z c (ε + μξ 2 ) ± μξ] and Z c =  μ/(ε + μξ 2 ) [Re(Z c ) > 0] . Eq. (5) is diagonalized as follows: k ⎡ ⎢ ⎢ ⎣ E x + iE y −iZ c H x + Z c H y E x −iE y −iZ c H x − Z c H y E x −iE y + iZ c H x + Z c H y E x + iE y + iZ c H x − Z c H y ⎤ ⎥ ⎥ ⎦ = ⎡ ⎢ ⎢ ⎣ k + O −k + k − O −k − ⎤ ⎥ ⎥ ⎦ ⎡ ⎢ ⎢ ⎣ E x + iE y −iZ c H x + Z c H y E x −iE y −iZ c H x − Z c H y E x −iE y + iZ c H x + Z c H y E x + iE y + iZ c H x − Z c H y ⎤ ⎥ ⎥ ⎦ ,(9) where we use the r elation Z c (ε + μξ 2 )=μZ −1 c [ Z 2 c = μ/(ε + μξ 2 )]andset k ± = ω[Z c (ε + μξ 2 ) ± μξ]. (10) If Z c is determined, k ± can be calculated unambiguously. The real part of the wave impedance Re (Z c ) is related to the time-averaged Poynting vector, which governs the power flow of electromagnetic waves. When a branch of Z c is chosen so that Re(Z c ) > 0 is satisfied, the power flows of eigenmodes represented by the first and third (second and fourth) rows of Eq. (9) are directed to the positive (negative) z-direction. Thus, k + and k − (−k + and −k − ) are the wavenumbers for the eigenmodes whose power flows are directed to the positive (negative) z-direction. Even if we choose a branch of Z c that satisfies Re (Z c ) < 0, we can obtain the same result by regarding −Z c as the wave impedance. T herefore, there is no loss of generality in supposing that the real part of Z c is positive. The wavenumber and wave impedance can be calculated from Eqs. (7) and (10) and the condition Re (Z c ) > 0without ambiguity. We define the eigenmodes represented by the first and second (third and fourth) rows of Eq. ( 9) as left circularly polarized (LCP) [right circularly polarized (RCP)] waves. 3. R eflectivity and transmissivity for chiral media We derive the reflectivity and transmissivity at the boundary between a vacuum and an isotropic chiral m edium (Bassiri et al., 1988). As shown in Fig. 1, suppose that a monochromatic plane electromagnetic wave is incident from the vacuum (permittivity ε 0 , permeability μ 0 ) on the chiral m edium at an incident angle of θ. The electromagnetic fields of the incident (i), reflected (r), and transmitted (t) waves are written as follows: E E E i = E E E 1 exp[ik 0 (x cosθ −ysinθ)], (11) H H H i = H H H 1 exp[ik 0 (x cosθ −ysinθ)], (12) E E E r = E E E 2 exp[ik 0 (−x cosθ − ysinθ)], (13) H H H r = H H H 2 exp[ik 0 (−x cosθ −ysinθ)], (14) E E E t = E E E 3 exp[ik + (x cos θ + −ysinθ + )] + E E E 4 exp[ik − (x cos θ − −ysinθ − )], (15) H H H t = H H H 3 exp[ik + (x cos θ + −ysinθ + )] + H H H 4 exp[ik − (x cosθ − −ysinθ − )], (16) 418 Wave Propagation No-Reflection Phenomena for Chiral Media 5 y x E i E i k 0 θ θ θ + θ - E r E r k 0 E t + E t - k + k - ε 0 , μ 0 ε, μ, ξ Fig. 1. Geometry of coordinate system. Incident, reflected, and transmitted waves are denotedbysubscriptsi,r,andt.Regionx < 0 represents vacuum, and region x ≥0 represents the chiral medium. where E E E 1 = E i⊥ e e e z + E i (cos θe e e y + sinθe e e x ), (17) H H H 1 = Z −1 0 [E i e e e z − E i⊥ (cos θe e e y + sinθe e e x )], (18) E E E 2 = E r⊥ e e e z + E r (−cos θe e e y + sinθe e e x ), (19) H H H 2 = Z −1 0 [E r e e e z + E r⊥ (cos θe e e y −sinθe e e x )], (20) E E E 3 = E t+ [i(cos θ + e e e y + sinθ + e e e x )+e e e z ], (21) H H H 3 = E t+ Z −1 c [−(cosθ + e e e y + sinθ + e e e x )+ie e e z ], (22) E E E 4 = E t− [−i(cosθ − e e e y + sinθ − e e e x )+e e e z ], (23) H H H 4 = E t− Z −1 c [−(cosθ − e e e y + sinθ − e e e x ) −ie e e z ]. (24) In the above equations, k 0 = ω √ ε 0 μ 0 is the wavenumber in the vacuum, Z 0 =  μ 0 /ε 0 is the wave impedance of the vacuum, and e e e x , e e e y ,ande e e z are respectively the unit vectors in the x-, y-, and z-directions. Due to the translational invariance of the interface, Snell’s equations k 0 sinθ = k + sinθ + = k − sinθ − , (25) 419 No-Reflection Phenomena for Chiral Media 6 Electromagnetic Wave s are satisfied. From the continuity of the tangential components of the electromagnetic fields across the boundary, we obtain E i⊥ + E r⊥ = E t+ + E t− , (26) E i cosθ −E r cosθ = iE t+ cosθ + −iE t− cos θ − , (27) Z −1 0 (E i + E r )=iZ −1 c (E t+ − E t− ), (28) Z −1 0 (−E i⊥ cosθ + E r⊥ cosθ)=−Z −1 c (E t+ cos θ + + E t− cosθ − ). (29) The reflection and transmission matrices are derived from E qs. (26)-(29) and w ritten as  E r⊥ E r  =  R 11 R 12 R 21 R 22  E i⊥ E i  ,  E t+ E t−  =  T ++ T +− T −+ T −−  E i+ E i−  , (30) where R 11 = ( Z 2 c − Z 2 0 )cosθ(cos θ + + cosθ − )+2Z 0 Z c (cos 2 θ −cosθ + cosθ − ) Δ , (31) R 12 = i2Z 0 Z c cosθ(cos θ + −cosθ − ) Δ , ( 32) R 21 = − i2Z 0 Z c cosθ(cos θ + −cosθ − ) Δ , (33) R 22 = −( Z 2 c −Z 2 0 )cosθ(cos θ + + cosθ − )+2Z 0 Z c (cos 2 θ −cosθ + cosθ − ) Δ , (34) T ++ = 2Z c (Z c + Z 0 )cosθ(cos θ + cos θ − ) Δ , (35) T +− = − 2Z c (Z c − Z 0 )cosθ(cos θ −cosθ − ) Δ , (36) T −+ = − 2Z c (Z c − Z 0 )cosθ(cos θ −cosθ + ) Δ , (37) T −− = 2Z c (Z c + Z 0 )cosθ(cos θ + cos θ + ) Δ , (38) Δ =(Z 2 c + Z 2 0 )cosθ(cos θ + + cosθ − )+2Z 0 Z c (cos 2 θ + cosθ + cos θ − ), (39) E i± = E i⊥ ∓iE i 2 . (40) 4. N o-reflection conditions for chiral media We find from Eqs. (30)-(34) that the relation between the electric field of the incident wave and that of the reflected wave is written as (Tamayama et al., 2008)  E r⊥ E r  = 1 Δ M R  E i⊥ E i  , M R = c u I + c 2 σ 2 + c 3 σ 3 , (41) c u = 2Z 0 Z c (cos 2 θ −cosθ + cos θ − ), (42) c 2 = −2Z 0 Z c cosθ(cos θ + −cosθ − ), (43) c 3 =(Z 2 c − Z 2 0 )cosθ(cos θ + + cosθ − ), (44) 420 Wave Propagation [...]... TE waves in the case of achiral media (ξ = 0), it arises for EP waves in the case of chiral media (ξ = 0) whose wave impedances do not equal the vacuum wave impedance These no-reflection conditions are satisfied for a particular incident angle When the wave impedance and the absolute value of the wavenumber in the chiral medium equal those in the vacuum for one of the CP waves, the corresponding CP wave. .. CP wave is not converted into the other CP wave on the reflection and refraction because the wave impedance matching condition Zc = Z0 is satisfied in this case Thus, we may separately analyze the propagations of LCP and RCP waves Figure 5 shows the propagations of electromagnetic waves when the diameter of the cylindrical chiral medium is smaller and larger than the beam width of the electromagnetic waves... magnetization are found to be P = ε 0 f (ω − ω0 ) E → 0 and M = f (ω − ω0 ) H → 0 for LCP waves and P = ε 0 [ f (ω − ω0 ) − H 2] E → −2ε 0 E and M = [ f (ω − ω0 ) − 2] H → −2H for RCP waves when ω → ω0 This implies that the medium behaves as a vacuum for LCP waves and as an anti-vacuum for RCP waves 12 426 Electromagnetic Waves Wave Propagation 0.5 20 0 10 Vacuum 0 (b) Chiral medium 0 10 20 x/λ 30 40 y/λ 30 y/λ... One sees that LCP waves propagate with no scattering, and RCP waves are largely scattered Next, we analyze the propagation of electromagnetic waves when they are incident on a triangular prism made of the chiral medium For k − = 0.6k0 , Snell’s equation for RCP waves is expressed as sin θ = 0.6 sin θ− ; hence, the critical angle for RCP waves is θc = arcsin (0.6) 37◦ Therefore, LCP waves are completely... 63.5◦ (left panels) Propagations of LCP waves and (right panels) of RCP waves 14 428 Electromagnetic Waves Wave Propagation are rearranged as follows: ∂Ez± = iω (μ ± μξZc ) Hx ± , ∂y ∂Ez± − = iω (μ ± μξZc ) Hy± , ∂x ∂Hy± ∂Hx ± μξ − = −iω (ε + μξ 2 ) ± Ez ± , ∂x ∂y Zc (55) (56) (57) where the relation H = ±(i /Zc ) E is used and the positive (negative) sign corresponds to LCP (RCP) waves Section 4.3... reflection, while RCP waves are totally reflected with the incident angle greater than 37◦ This implies that we can divide the incident waves into LCP and RCP waves That is, the prism can be utilized as a circular polarizing beam splitter The left (right) panels of Fig 6 show the propagations of LCP (RCP) waves Simulations are performed for three incident angles: 26.5◦ , 45◦ , and 63.5◦ The LCP wave is transmitted... polarized waves The no-reflection effect is observed at a particular incident angle that satisfies cu = ± c3 The condition cu = c3 (cu = − c3 ) yields a no-reflection angle, called the Brewster angle, for TM (TE) waves in isotropic achiral media 8 422 Electromagnetic Waves Wave Propagation From cu = ± c3 , the no-reflection angles θTM and θTE for TM and TE waves are derived as follows: ε2 − ε r μ r μ2 − ε r... Polarization No-reflection angle Medium parameters, Incident angle ξ =0 Wave impedance TE ∃θ TM ∃θ yes cu = − c3 cu = c3 Zc = Z0 ξ =0 Wave impedance Medium parameters, Incident angle Polarization No-reflection angle No-Reflection Phenomena Chiral Media No-Reflection Phenomena forfor Chiral Media 15 429 16 430 Electromagnetic Waves Wave Propagation For future studies, we must prepare metamaterials whose ε... (2005) 18 432 Electromagnetic Waves Wave Propagation Near-infrared double negative metamaterials, Opt Express 13(13): 4922–4930 Zhang, S., Park, Y.-S., Li, J., Lu, X., Zhang, W & Zhang, X (2009) Negative Refractive Index in Chiral Metamaterials, Phys Rev Lett 102(2): 023901 Part 6 Nonlinear Phenomena and Electromagnetic Wave Generation 21 Manipulating the Electromagnetic Wave with a Magnetic Field Shiyang... and nonuniform EMFs They can also offer us the manipulability on the flow of EM wave with the tunability by an EMF The research content of the present chapter consists of four parts In the fist part, we examine the mechanism governing the photonic band gaps (PBGs) of a two dimensional (2D) MPC, 2 436 Electromagnetic Waves Wave Propagation based on the simulations on the photonic band diagrams and the transmission . developed. The wavenumber is related to the propagation and r efraction of electromagnetic waves, and the wave impedance is connected with the r eflection. Phenomena about electromagnetic waves are. waves. First, we analyze the scattering of electromagnetic waves by a cylinder made of the chiral medium. To adopt the two-dimensional FDTD method, Maxwell’s equations for CP waves 426 Wave Propagation No-Reflection. the electromagnetic waves. One sees that LCP waves propagate with no scattering, and RCP waves are largely scattered. Next, we analyze the propagation of electromagnetic waves when they are incident