Hostname: page-component-586b7cd67f-t7fkt Total loading time: 0 Render date: 2024-11-27T22:18:40.833Z Has data issue: false hasContentIssue false

Scattering by PEC half-plane and disk placed on parallel planes

Published online by Cambridge University Press:  19 April 2022

Mstislav E. Kaliberda*
Affiliation:
School of Radiophysics, Biomedical Electronics and Computer Systems, V.N. Karazin Kharkiv National University, Kharkiv, Ukraine
Leonid M. Lytvynenko
Affiliation:
Institute of Radio Astronomy of the National Academy of Sciences of Ukraine, Kharkiv, Ukraine
Sergey A. Pogarsky
Affiliation:
School of Radiophysics, Biomedical Electronics and Computer Systems, V.N. Karazin Kharkiv National University, Kharkiv, Ukraine
*
Author for correspondence: Mstislav E. Kaliberda, E-mail: [email protected]
Rights & Permissions [Opens in a new window]

Abstract

The scattering by the perfectly electric conducting (PEC) half-plane and PEC zero thickness disk placed on parallel planes is considered. The fields are represented in the spectral domain, i.e. in the domain of Fourier transform. The operator equations with respect to the Fourier amplitudes of the scattered field are obtained. The kernel functions of these equations contain poles. After regularization procedure, which is connected with the elimination of the poles, operator equations are converted to the system of singular integral equations. The convergence of the solution is based on the corresponding theorems. The scattered field consists of the plane wave, reflected by the infinite part of the half-plane, cylindrical waves, which appear as a result of scattering by the edge of the half-plane, and spherical waves, which appear as a result of scattering by the disk and multiple re-scattering by the disk-half-plane. The total near-field distribution and far-field patterns of cylindrical waves are presented.

Type
EM Field Theory
Copyright
Copyright © The Author(s), 2022. Published by Cambridge University Press in association with the European Microwave Association

Introduction

Circular disk and half-plane are canonical scattering objects. One can find classical solutions for scattering by the half-plane based on the method due to D. S. Jones, factorization of the kernel function of the dual integral equations and integral equations [Reference Jones1Reference Copson5]. In [Reference Khestanov6], scattering of an arbitrary two-dimensional (2D) wave beam is analyzed. In [Reference Bertoni, Green and Felsen7], inhomogeneous plane wave and in [Reference Green, Bertoni and Felsen8] the Gaussian beam incidence is considered. In [Reference Green, Bertoni and Felsen8], special attention is paid to the shadow region. In [Reference Rahmat-Samii and Mittra9], high-frequency asymptotic for the solution of scattering of an arbitrary 2D field is obtained. In [Reference Gorobets, Yeliseyeva and Antonenko10, Reference Yeliseyeva, Gorobets, Katrich and Nesterenko11], the solution for the half-plane is used to obtain the asymptotic expressions for the antenna modeling.

The analysis of scattering by zero-thickness perfectly electric conducting (PEC) disk in free space or layered media with the guaranteed-convergent methods has represented an interesting electromagnetic problem for decades. In [Reference Nomura and Katsura12, Reference Lytvynenko, Prosvirnin and Khizhnyak13], scattering by the circular disk or hole in the plane is considered with the method of moments. The Fourier amplitudes are expressed in terms of the series of hypergeometric polynomials, which are obtained as a result of integration of the Bessel functions. In [Reference Bouwkamp14, Reference Maixner and Andrejewski15], the power series expansion and spheroidal wave function is used. In [Reference Hongo and Naqvi16], the dual integral equations are obtained and solved with the use of the method of Kobayashi potentials.

In [Reference Losada, Boix and Horno17Reference Losada, Boix and Medina19], one-dimensional electric-field integral equation in the scalar Hankel transform domain for the zero-thickness PEC circular patch resonator in multilayered media and zero-thickness PEC disk buried in a lossy half-space are discretized by means of Galerkin method.

In [Reference Di Murro, Lucido, Panariello and Schettino20], scattering by an arbitrarily oriented zero-thickness PEC disk buried in a lossy half-space is formulated as electric-field integral equations in the vector Hankel transform domain and discretized with the use of Galerkin method. The matrix coefficients are converted to the rapidly converging integrals. In [Reference Lucido, Panariello and Schettino21], the authors perform analytical regularization and discretization within one procedure, namely Galerkin projection on the set of judicious expansion functions, which are the eigenfunctions of the singular (static) part. The method of analytical regularization which leads to the Fredholm integral equation of the second kind is successfully applied to the analysis of the scattering by the finite-thickness thin PEC disk, dielectric disk, and graphene disk in [Reference Balaban, Sauleau, Benson and Nosich22Reference Balaban, Shapoval and Nosich24]. The problem for the lens based on the disk inside the dielectric sphere excited by the dipole is reduced to the second-kind Fredholm matrix equation in [Reference Tikhenko, Radchenko, Dukhopelnykov and Nosich25].

Half-plane is an infinite object with an edge. From the mathematical point of view, it results in the appearance of poles in the kernel function of the integral equations. This requires the integration over contour in the complex plane. The edge can give us some interesting physical effects. For example, the PEC disk being not illuminated by the incident wave directly or being in the node of the standing wave can scatter the waves, which appear due to the edge of the half-plane.

In [Reference Kaliberda, Lytvynenko and Pogarsky26], we consider half-plane and disk placed on the same plane. In this paper, we consider plane wave scattering by PEC half-plane and disk in more general case, when they are placed on parallel planes. Here, an additional domain appears, a domain between the half-plane and the disk. From a mathematical point of view, this means that we need additional equations to describe the fields in this domain. From a methodological point of view, since the number of equations is increased as compared to [Reference Kaliberda, Lytvynenko and Pogarsky26], we need to introduce new operators which will allow us to write final equations in a concise form.

In this paper, we express scattered fields in the spectral domain in terms of the Fourier amplitudes (spectral functions), which are the Fourier transform of the currents density on the metal. The total scattered field can be represented as a sum of the fields of every isolated scatterer and the field which appears as a result of mutual coupling or re-scattering by the objects [Reference Schwarzschild27]. In case the Fourier amplitudes of the field scattered by the isolated half-plane and the disk are known, or, in other words, their scattering operators are known, one can write operator equations for the scattered field of the whole structure. Since the kernel functions of these equations can have singularities in the form of poles of the integrands, some additional mathematical manipulations are needed to convert them to the solvable integral equations. The convergence of the solution is based on the corresponding theorems. This approach is successfully applied to the gratings of the infinite PEC or graphene screens in [Reference Kaliberda, Litvinenko and Pogarsky28Reference Kaliberda, Litvinenko and Pogarsky30]. In [Reference Kaliberda, Litvinenko and Pogarsky31], scattered fields consist of the fields of either plane waves or cylindrical waves, or both. Here, we are going to use this approach to the structure where scattered field consists of plane, cylindrical, and spherical waves. The rigorous solution for such a geometry is obtained for the first time. Potentially, it can be used in ring resonators and antenna design [Reference Zhang, Yang, Fu and Zhang32, Reference Saidoglu and Nosich33], as well as to study the influence of the edge-effect.

Problem statement

Let us consider PEC half-plane y < 0, z = 0 and zero thickness PEC disk of radius r, x 2 + (y − Δ)2 < r, placed in the plane z = h, h > 0, where Δ is the shift of the disk along the y-axis. The plane wave with the Fourier amplitude q = (q x,  q y)* is incident from the “upper” half-space z > h and the plane wave with the Fourier amplitude p = (p x,  p y)* is incident from the “lower” half-space z < 0, where “*” means transpose. Since we assume h > 0, to simulate the case of the disk placed below the half-plane, we introduce second incident wave with the Fourier amplitude p.

In the considered problem, all components of the electromagnetic field can be expressed via the independent tangential electric components E x and E y. The incident field is

(1)$$\eqalign{\left(\matrix{E_x^i \hfill \cr E_y^i \hfill} \right) & = \left(\matrix{q_x \hfill \cr q_y \hfill} \right)\exp ( {-ik( Ax + By + \gamma ( A, \;B) z) } ) + \left(\matrix{\,p_x \hfill \cr p_y \hfill} \right) \cr & \times \exp( {ik( Ax + By + \gamma ( A, \;B) z) } ) , \;}$$

where k = 2π/λ is the wavenumber, $\gamma ( A, \;\,B) = \sqrt {1-A^2-B^2}$ with ${\mathop{\rm Re}\nolimits} \,\gamma \ge 0$, ${\mathop{\rm Im}\nolimits} \,\gamma \ge 0$, A = cosα, B = cosβ, are cosines of the incident angles γ 1, α, and β with respect to the z, x, and y axis. The time dependence exp(−iωt) is omitted.

In the spectral domain, i.e. in the domain of Fourier transform, we seek scattered field as Fourier integrals with unknown amplitudes $A_\Theta$, $B_\Theta$, $C_\Theta$, $D_\Theta$, Θ = x, y:

(2)$$\eqalign{& E_\Theta ^s ( x, \;y) = \left\{\matrix{\int\limits_{-\infty }^{ + \infty } {\int\limits_{-\infty }^{ + \infty } {A_\Theta ( \xi_x, \;\xi_y) \exp ( {ik( \xi_xx + \xi_yy + \gamma ( \xi_x, \;\xi_y) z) } ) d\xi_xd\xi_y} } , \;\,\,\,\hskip8ptz > h, \;\hfill \cr \int\limits_{-\infty }^{ + \infty } {\int\limits_{-\infty }^{ + \infty } {( {B_\Theta ( \xi_x, \;\xi_y) \exp ( {ik\gamma ( \xi_x, \;\xi_y) z} ) + C_\Theta ( \xi_x, \;\xi_y) } } } \hfill \times \exp ( {ik( \xi_y\Delta -\gamma ( \xi_x, \;\xi_y) ( z-h) ) } )\cr \quad\times \exp ( {ik( \xi_xx + \xi_yy) } ) d\xi_xd\xi_y, \;\,\,\,\hskip2pt0 < z < h, \;\hfill \cr \int\limits_{-\infty }^{ + \infty } {\int\limits_{-\infty }^{ + \infty } {D_\Theta ( \xi_x, \;\xi_y) \exp ( {ik( \xi_xx + \xi_yy-\gamma ( \xi_x, \;\xi_y) z) } ) d\xi_xd\xi_y} } , \;\,\,\,\hskip8ptz < 0, \;\hfill} \right.}$$

The structure geometry and directions of wave propagation are shown in Fig. 1. Total field is the sum of the incident and scattered fields.

Fig. 1. Structure geometry.

Let us introduce reflection and transmission operators of the isolated half-plane y < 0, z = 0, R 1, T 1, and disk x 2 + y 2 < r, which center coincides with the origin, R 2, T 2. Their action on arbitrary Fourier amplitude g is described by the integrals

(3)$$( R_jg) _\Theta ( \xi _x, \;\xi _y) = \sum\limits_{\Xi = x, \,y}^{} {\int\limits_{-\infty }^{ + \infty } {\int\limits_{-\infty }^{ + \infty } {R_{\,j, \Theta \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y) g_\Xi ( \zeta _x, \;\zeta _y) d\zeta _xd\zeta _y} } } , \;$$
(4)$$\eqalign{( T_jg) _\Theta ( \xi _x, \;\xi _y) & = \sum\limits_{\Xi = x, \,y}^{} {\int\limits_{-\infty }^{ + \infty } {\int\limits_{-\infty }^{ + \infty } {T_{\,j, \Theta \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y) g_\Xi ( \zeta _x, \;\zeta _y) d\zeta _xd\zeta _y} } } , \;\,\quad \cr\Theta & = x, \;y, \;\,\,j = 1, \;2.} $$

Kernel functions of the scattering operators $R_{j, \Theta \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y)$, $T_{j, \Theta \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y)$ are supposed to be known. The reflection operators of the half-plane can be found by the factorization of the kernel of dual integral equations [Reference Copson5]. The reflection operators of the disk can be found by the method of moments [Reference Nomura and Katsura12, Reference Lytvynenko, Prosvirnin and Khizhnyak13]. In [Reference Nomura and Katsura12, Reference Lytvynenko, Prosvirnin and Khizhnyak13], the problem is considered only for case the wave vector of the incident field is in the plane XOZ, the scattered field is represented in the cylindrical coordinate system. The case of arbitrary incidence can be obtained with the use of the affine transformation of rotation. In our analysis, we need scattered fields to be represented in the Cartesian coordinate system as a superposition of the plane waves which propagate under real and complex angles. For this purpose, we use representation of the Bessel function J m(x) in the form of superposition of plane waves: $J_m( x) = {{{( {-}i) }^m} \over {2\pi }}\int\limits_{\varphi -2\pi }^\varphi {\exp ( i( x\cos \psi -m\psi ) ) d\psi }$.

Operator equations

As we have mentioned in the Introduction, scattered field can be represented as a sum of the field scattered by the isolated half-plane and the disk, and the field re-scattered by them. If we denote the Fourier amplitude of the field of re-scattered waves, which propagate to the positive direction of the z-axis as B, and which propagate to the negative direction of the z-axis as C (2), then one can write the following operator equations:

(5)$$A = e^{-}s^{-}T_2e^ + s^ + B + e^{-}s^{-}R_2e^{-}s^{ +} q, \;$$
(6)$$\hskip-57ptB = R_1e^ + s^-C + T_1p, \;$$
(7)$$\hskip-38ptC = R_2e^ + s^ + B + T_2e^{-}s^{ +} q, \;$$
(8)$$\hskip-57ptD = T_1e^ + s^-C + R_1p, \;$$

where action of the operators s ± and e ± is reduced to multiplication by exp(±ikξ yΔ) and exp(±ikγ(ξ x,  ξ y)h). They describe the phase variations if the coordinate system is shifted in the positive or negative direction of the y- and z-axis.

Let us notice first that reflection and transmission operators are connected as follows: T j = I + R j, j = 1,  2, where I is unit operator. Also let us subtract the Fourier amplitude of the incident plane wave (which is proportional to the delta-function) from the Fourier amplitude of the scattered field. Introduce new functions C 1, B 1 as follows:

(9)$$B_1 = B-p, \;\quad \,C_1 = C-e^{-}s^{ +} q. $$

Then one can rewrite (5)–(8) as follows:

(10)$$A = B_1 + e^{-}s^{-}R_2e^ + s^ + B_1 + e^{-}s^{-}R_2s^ + ( e^ + p + e^-q) , \;$$
(11)$$B_1 = R_1e^ + s^-C_1 + R_1( p + q),$$
(12)$$C_1 = R_2e^ + s^ + B_1 + R_2s^ + ( e^ + p + e^-q),$$
(13)$$D = e^ + s^-C_1 + R_1e^ + s^-C_1 + R_1( p + q) + p.$$

If C 1 and B 1 are determined from (11), (12), then from (10), (13) A and D also can be determined. Therefore, our purpose is to reduce (11) and (12) to solvable integral equations.

Integral equations

Kernel functions of the reflection operator of the half-plane have poles at the point which correspond to the propagation constant of the reflected plane wave. Kernel functions of the reflection operators of the half-plane and disk have integrable inverse square root singularity at the points which correspond to the waves which propagate along the XOY plane (sliding waves).

Let us represent the reflection operator of the disk as product of the singular and regular terms, also we subtract that part, which contains poles and gives plane wave in the reflected field. Introduce new functions which do not have singularities:

(14)$$R_{2, \Theta , \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y) = R_{\Theta , \Xi }( \xi _x, \;\xi _y, \;\zeta _x, \;\zeta _y) \sqrt {1-\xi _x^2 -\xi _y^2 } , \;$$
(15)$$\eqalignno{B_{2, x}( \xi _x, \;\xi _y) & = \left({B_{1, x}( \xi_x, \;\xi_y) + \displaystyle{i \over {2\pi }}\displaystyle{{\sqrt {\sqrt {1-A^2} -B} } \over {\sqrt {\sqrt {1-A^2} -\xi_y} }}\displaystyle{{q_x + p_x} \over {\xi_y-\mathop B\limits_{below} }}} \right)\cr& \quad\times\sqrt {1-\xi _x^2 -\xi _y^2 } , \; }$$
(16)$$\eqalignno{B_{2, y}( \xi _x, \;\xi _y) & = \left({B_{1, y}( \xi_x, \;\xi_y) -\displaystyle{i \over {2\pi }}\displaystyle{A \over {\sqrt {1-A^2} }}} \right. \cr & \left. \times \ {\displaystyle{{q_x + p_x} \over {\sqrt {\sqrt {1-A^2} -B} \sqrt {\sqrt {1-A^2} -\xi_y} }}} \right. \cr & \left. { + \displaystyle{i \over {2\pi }}\displaystyle{{\sqrt {\sqrt {1-A^2} -\xi_y} } \over {\sqrt {\sqrt {1-A^2} -B} }}\displaystyle{{q_y + p_y} \over {\xi_y-\mathop B\limits_{below} }}} \right)\sqrt {1-\xi _x^2 -\xi _y^2 } , \;} $$
(17)$$C_{2, \Theta }( \xi _x\xi _y) = C_{1, \Theta }( \xi _x, \;\xi _y) \sqrt {1-\xi _x^2 -\xi _y^2 } . $$

Notation “below” (“above”) means that the poles should be bypassed from below (above). The Fourier amplitudes B 2 and C 2 describe only field of spherical waves.

After substitution of (14)–(17) as well as an explicit form of the reflection operator of the half-plane into (11), (12), one can obtain the integral equations. To write them in a more concise form first we introduce the following notations:

(18)$$( F_1g) ( \xi _x, \;\xi _y) = \displaystyle{i \over {2\pi }}\sqrt {\sqrt {1-\xi _x^2 } + \xi _y} \int\limits_{-\infty }^\infty {\displaystyle{{g( \xi _x, \;\zeta _y) } \over {\sqrt {\sqrt {1-\xi _x^2 } + \zeta _y} }}\displaystyle{{d\zeta _y} \over {\zeta _y-\mathop {\xi _y}\limits_{below} }}} , \;$$
(19)$$\eqalignno{( F_2g) ( \xi _x, \;\xi _y) & = \displaystyle{i \over {2\pi }}\sqrt {\sqrt {1-\xi _x^2 } + \xi _y} \int\limits_{-\infty }^\infty {\displaystyle{{g( \xi _x, \;\zeta _y) } \over {\sqrt {1-\xi _x^2 -\zeta _y^2 } }}\displaystyle{{\xi _x} \over {\sqrt {1-\xi _x^2 } }}}\cr & \quad\times \displaystyle{{d\zeta _y} \over {\sqrt {\sqrt {1-\xi _x^2 } -\zeta _y} }}, \; }$$
(20)$$\eqalignno{( F_3g) ( \xi _x, \;\xi _y) & = \displaystyle{i \over {2\pi }}\sqrt {1-\xi _x^2 -\xi _y^2 } \int\limits_{-\infty }^\infty {\displaystyle{{\sqrt {\sqrt {1-\xi _x^2 } -\xi _y} } \over {\sqrt {\sqrt {1-\xi _x^2 } -\zeta _y} }}} \displaystyle{{g( \xi _x, \;\zeta _y) } \over {\sqrt {1-\xi _x^2 -\zeta _y^2 } }}\cr& \quad\times \displaystyle{{d\zeta _y} \over {\zeta _y-\mathop {\xi _y}\limits_{below} }}, \; }$$
(21)$$F_4g = \int\limits_{-\infty }^\infty {\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta _x, \;\zeta _y) } \over {\sqrt {1-\zeta _x^2 -\zeta _y^2 } }}} d\zeta _xd\zeta _y} , \;$$
(22)$$F_5g = {-}\displaystyle{i \over {2\pi }}\sqrt {\sqrt {1-A^2} -B} \int\limits_{-\infty }^\infty {\displaystyle{{g( A, \;\zeta _y) } \over {\sqrt {\sqrt {1-A^2} -\zeta _y} }}} \displaystyle{{d\zeta _y} \over {\zeta _y-\mathop B\limits_{above} }}, \;$$
(23)$$F_6g = \displaystyle{i \over {2\pi }}\displaystyle{A \over {\sqrt {1-A^2} }}\displaystyle{1 \over {\sqrt {\sqrt {1-\alpha ^2} -B} }}\int\limits_{-\infty }^\infty {\displaystyle{{g( A, \;\zeta _y) d\zeta _y} \over {\sqrt {\sqrt {1-\alpha ^2} -\zeta _y} }}} , \;$$
(24)$$F_7g = {-}\displaystyle{i \over {2\pi }}\int\limits_{-\infty }^\infty {\displaystyle{{\sqrt {\sqrt {1-A^2} -\zeta _y} g( A, \;\zeta _y) } \over {\sqrt {\sqrt {1-A^2} -B} }}} \displaystyle{{d\zeta _y} \over {\zeta _y-\mathop B\limits_{above} }}, \;$$
(25)$$F_8g = g( A, \;B) . $$

Then integral equations are

(26)$$B_{2, x} = F_1e^ + s^-C_{2, x}, \;$$
(27)$$B_{2, y} = F_2e^ + s^-C_{2, x} + F_3e^ + s^-C_{2, y}, \;$$
(28)$$\eqalignno{C_{2, \Theta } = & F_4e^ + s^ + ( R_{2, \Theta , x}B_{2, x} + R_{2, \Theta , y}B_{2, y}) + ( q_x + p_x) F_5e^ + s^ + R_{2, \Theta , x} \cr & \quad + ( q_x + p_x) \cdot F_6e^ + s^ + R_{2, \Theta , y} + ( q_y + p_y) F_7e^ + s^ + R_{2, \Theta , y} \cr & \quad + F_8( R_{2, \Theta , x}s^ + ( e^ + p_x + e^-q_x) + R_{2, \Theta , y}s^ + ( e^ + p_y + e^-q_y) ) , \;\,\cr& \ \quad \Theta = x, \;y.} $$

Integrands in (18), (20), (22), (24) have non-integrable singularities on the real axis. To eliminate the singularities the regularization procedure is needed.

Regularization procedure

To calculate integrals (18), (20), (22), (24) first we transform the integration path so that it coincides with the real axis everywhere except the pole. The pole is bypassed from above or below. Then we add and subtract such a function from the integrand that their sum has no singularities. The integral from this function itself can be calculated analytically. Taking into account that [Reference Muskhelishvili34]

(29)$$\int\limits_{-\infty }^\infty {\displaystyle{1 \over {\zeta -\mathop \xi \limits_{below} }}d\zeta } = \pi i, \;$$
(30)$$\int\limits_{-\infty }^\infty {\displaystyle{1 \over {\zeta -\mathop \xi \limits_{above} }}d\zeta } = {-}\pi i, \;$$

obtain

(31)$$\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\mathop \xi \limits_{below} }}d\zeta } = \int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) -g( \xi ) } \over {\zeta -\xi }}d\zeta } + \pi ig( \xi ) , \;$$
(32)$$\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\mathop \xi \limits_{above} }}d\zeta } = \int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) -g( \xi ) } \over {\zeta -\xi }}d\zeta } -\pi ig( \xi ) . $$

Integrals on the right-hand side of (31), (32) are convergent. The integrands have no singularities. Thus we can understand them as Cauchy principal value integrals (notation PV). Taking into account that $PV\int_{-\infty }^\infty {d\xi /\xi } = 0$, finally obtain

(33)$$\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\mathop \xi \limits_{below} }}d\zeta } = PV\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\xi }}d\zeta } + \pi ig( \xi ) , \;$$
(34)$$\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\mathop \xi \limits_{above} }}d\zeta } = PV\int\limits_{-\infty }^\infty {\displaystyle{{g( \zeta ) } \over {\zeta -\xi }}d\zeta } -\pi ig( \xi ) . $$

Representation of (31), (32) in the form of Cauchy principal value integral (33), (34) is essential for us for discretization. In this case we can apply appropriate quadrature rule.

After regularization of (18), (20), (22), (24) as it is done in (33), (34), integral equations (26)–(28) can be discretized with the use of the quadrature rule. Equations (26)–(28) actually are the system of singular integral equations of the second kind on the infinite interval of integration.

Remark. In general, there is no need to explicitly express inverse square root singularity with the help of (14). However in this paper to solve integral equations (26)–(28) numerically we convert them to the system of algebraic equations with the help of quadrature rule. To build rapidly convergent discretization scheme, we should take into account singularities and thus to take proper quadratures.

For discretization of (26)–(28), we exchanged the infinite interval of integration by the bounded one (−aa). After that we divide segment [−aa] into N sub-segments and take single node point at the center of every sub-segment. Thus we use the compound midpoint rule for singular integrals.

After discretization, the linear matrix equation can be written as

(35)$$\hat{B}_2 = M_1\hat{C}_2, \;$$
(36)$$\hat{C}_2 = M_2\hat{B}_2 + q_xM_3 + p_xM_4, \;$$

where $\hat{B}_2$ and $\hat{C}_2$ are vectors which consist of unknown values of B 2,x, B 2,y, C 2,x, C 2,y at the nodes, M i, i = 1, …, 4, are matrices and vectors which correspond to the right-hand side of (26)–(28) after discretization.

To solve (35), (36) we use the iterative procedure

(37)$$\hat{C}_2^0 = q_xM_3 + p_xM_4, \;$$
(38)$$\hat{B}_2^j = M_1\hat{C}_2^j , \;$$
(39)$$\hat{C}_2^{\,j + 1} = M_2\hat{B}_2^j + q_xM_3 + p_xM_4, \;\quad j = 0, \;\,1, \;\ldots , \;L, \;$$

where superscript j means the number of iteration and L is the total number of iterations.

Numerical results

Let us study the convergence. Three parameters affect the error of the solution: number of nodes N, length of the truncated interval of integration a, and number of iterations L. We introduce error as follows:

(40)$$\varepsilon ( N) = \vert A^{sw}( N) -A^{sw}( 2N-1) \vert /\vert A^{sw}( 2N-1) \vert , \;$$
(41)$$\varepsilon ( a) = \vert A^{sw}( a) -A^{sw}( \Phi ) \vert /\vert A^{sw}( \Phi ) \vert , \;$$
(42)$$\delta ( L) = \vert A^{sw}( L) -A^{sw}( L + 1) \vert /\vert A^{sw}( L + 1) \vert , \;$$

where $A^{sw} = \sqrt {{( A_x^{sw} ( \xi _x = 0, \;\xi _y = 0) ) }^2 + {( A_y^{sw} ( \xi _x = 0, \;\xi _y = 0) ) }^2}$ is amplitude of the spherical wave in the orthogonal direction, Φ = 10 is sufficiently large constant value.

The convergence of the presented scheme is based on the corresponding theorems about approximation of singular and regular integrals by quadrature rule [Reference Lifanov35]. However, the actual rate of convergence should be studied. Figure 2 shows dependences of the error on the number of interpolation nodes N, length of the interval of integration a, and the number of iterations L. Starting from the certain value of parameter, the convergence is monotone. Equations (26)–(28) contain exponentially decaying term, which is described by the operators e ±. As a result, ɛ(a) decays exponentially (see Fig. 2(c)), if a → ∞. Here rate of convergence depends on kh. For larger values of kh, a faster convergence is observed.

Fig. 2. Error of the solution: (a) ɛ(N); (b) ɛ(a); and (c) δ(L).

Far field scattered by the structure can be represented as a sum of three summands:

(43)$$E^{sc} = E^{\,pw} + E^{err} + E^{sw}, \;$$

where E pw is the field of the plane wave reflected (or transmitted) by the infinite part of the half-plane. It does not decay, if  → ∞, where ρ is the distance. The second summand in (43) E err is expressed in terms of the error function. It describes the field of cylindrical waves except the plane y = 0, where it provides the continuity of the asymptotic representation of the far field. Finally E sw is the field of spherical waves. It decays as 1/(), if  → ∞. It describes the mutual coupling of the half-plane and the disk, since E pw and E err are exactly the same as in the case of the isolated half-plane.

The saddle-point method gives us the expression for the diffraction patterns of the spherical waves with amplitudes $A_\Theta ^{sw}$ (if z > 0), $D_\Theta ^{sw}$ (if z < 0)

(44)$$\eqalign{& \vert E_\Theta ^{sw} ( \rho \cos \phi \sin \theta , \;\rho \sin \phi \sin \theta ) \vert \cr & \quad \sim \left\{\matrix{\displaystyle{{2\pi } \over {k\rho }}A_\Theta^{sw} ( \cos \phi \sin \theta , \;\sin \phi \sin \theta ) , \;\,\,\,z > 0, \; \cr \displaystyle{{2\pi } \over {k\rho }}D_\Theta^{sw} ( \cos \phi \sin \theta , \;\sin \phi \sin \theta ) , \;\,\,\,z < 0, \;} \right.}$$

where Θ = x,  y, (ρ,  θ,  ϕ) are coordinates of the spherical coordinate system, θ is the polar angle, φ is the azimuthal angle, $A_\Theta ^{sw}$ and $D_\Theta ^{sw}$ are that parts of the Fourier amplitudes $A_\Theta ^{}$ and $D_\Theta ^{}$, which correspond to the spherical waves. They can be obtained from (10), (13) after regularization of integrals.

Figures 2–7 show far field of spherical waves. We study scattered fields for two values of the radius kr = π/2 (r = λ/4) and kr = π (r = λ/2), two values of the distance between the plane and the disk along the z-axis kh = π/2 and kh = π, and several values of the shift Δ along the y-axis. The considered values of the radius correspond to the resonant cases. Near them the maxima and minima of the total scattering cross section of the isolated disk are observed [Reference Nomura and Katsura12]. All diffraction patterns are normalized by the global maximum. In the XZ plane, φ = 00, the patterns are symmetric with respect to θ = 00, since the structure is symmetric with respect to the y-axis.

Fig. 3. Far-field patterns of spherical waves, non-zero electric-field components $A_x^{sw}$ and $A_y^{sw}$ (solid lines), $D_x^{sw}$ and $D_y^{sw}$ (dashed lines) for kΔ = 2π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kΔ = −2π (blue lines), φ = 900, kr = π, kh = π/2, normal incidence α = β = 900: (a) q x ≠ 0, q y = p x = p y = 0; (b) q y ≠ 0, q x = p x = p y = 0; (c) p x ≠ 0, q x = q y = p y = 0; and (d) p y ≠ 0, q x = q y = p x = 0.

Fig. 4. Far-field patterns of spherical waves for kΔ = 2π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kΔ = −2π (blue lines) φ = 00, kr = π, kh = π/2, normal incidence α = β = 900, q x ≠ 0, q y = p x = p y = 0: (a) $A_x^{sw}$ (solid lines), $A_y^{sw}$ (dashed lines) and (b) $D_x^{sw}$ (solid lines), $D_y^{sw}$ (dashed lines).

Fig. 5. Same study as in Fig. 3, but for kh = π.

Fig. 6. Far-field patterns of spherical waves $A_x^{sw}$ (solid lines), $D_x^{sw}$ (dashed lines) for kΔ = π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kr = π/2, kh = π/2, normal incidence α = β = 900, q x ≠ 0, q y = p x = p y = 0: (a) φ = 00 and (b) φ = 900 (here $A_y^{sw}$ = $D_y^{sw}$ = 0).

Fig. 7. Same study as in Fig. 6, but for kh = π.

In the case of the infinite PEC plane, value kh = π/2 corresponds to the maxima (hot-spot) and value kh = π corresponds to the minima (node) of the electric field of the standing wave formed by the superposition of the incident and reflected plane waves. In the case of infinite PEC plane, if we place PEC disk of zero thickness in the plane kh = π there will be no scattering. However, in our situation, in the case of the half-plane, non-zero field of cylindrical waves exists due to the presence of the edge. As a result, E sw is also non-zero. At the same time, because of the presence of the standing wave, if y < 0, the amplitude of spherical waves for kh = π/2 (see Figs 3(a) and 3(b)) exceed the amplitude of spherical waves for kh = π (see Figs 5(a) and 5(b)).

We study the scattered field for different shift Δ of the disk along the y-axis. For Δ > 0, the disk is mainly placed in the field of the incident plane wave with small contribution of the field of the edge of the half-plane. The far-field shows almost the same behavior for kh = π/2 and kh = π. Consider first the case q x ≠ 0 or q y ≠ 0 (incidence from “above”) and p x = 0, p y = 0. If one moves the disk toward the negative values of the y-axis, the far-field behavior significantly depends on the distance h. For kh = π/2, the disk is placed in the hot-spot of the standing wave. As a result, the amplitude of spherical wave growths toward some constant value when the influence of the cylindrical wave is neglected as compared to the standing wave. For kh = π, the disk is placed in the node of the standing wave. As a result, the amplitude of spherical wave decreases if the disk is moved far from the edge of the half-plane, but |E sw| > 0 due to excitation of cylindrical waves. In the case p x ≠ 0 or p y ≠ 0 (incidence from “below”) the value of h does not influence significantly, since the disk is not illuminated by the plane wave at all for Δ < −r.

Figures 8–10 show total field distribution in the vertical plane, x = 0, for different position of the disk. We consider the incidence from “above” (Figs 8 and 11) and from “below” (Figs 9 and 10). The patterns are normalized by the amplitude of the incident wave.

Fig. 8. Total field distribution |E x| in the plane x = 0 for kr = π, kh = π/2, q x ≠ 0, q y = p x = p y = 0, normal incidence: (a) kΔ = 2π; (b) kΔ = 0; and (c) kΔ = −π.

Fig. 9. Total field distribution |E x| for x = 0, kr = π, kh = π/2, p x ≠ 0, q x = q y = p y = 0, normal incidence: (a) kΔ = 2π; (b) kΔ = 0; and (c) kΔ = −π.

Fig. 10. Total field distribution |E x| for x = 0, kr = 3π, kh = π, p x ≠ 0, q x = q y = p y = 0, normal incidence.

Fig. 11. Total field distribution in the plane z = 2h for kr = π, kh = π/2, q x ≠ 0, q y = p x = p y = 0, normal incidence: (a) |E x| and (b) |E y|.

The reflected plane wave exists only in the domain y < 0. Except the rigorous theory, this is confirmed by the geometrical optics. The half-plane is the semi-infinite structure placed in the domain y < 0. Thus, in the domain y < 0 (in the case of orthogonal incidence) the plane wave is reflected, and in the domain y > 0 the plane wave is transmitted. The field of the reflected plane wave in the domain y < 0 as well as the hot-spots at kh = π/2 + πn and nodes at kh = πn, n = 0, 1, 2, … of the standing wave are clearly seen in Figs 8–10. Near the disk, the tangential components of the electric field vanish, E x = E y = 0. The minima of the tangential components of the electric field and spherical wave with hot-spots of the field near the disk are also seen in Figs 8–10.

Near the plane y = 0, the boundary between two domains appears: domain y > 0, where reflected plane wave does not exist, and domain y < 0, where reflected plane wave exists. The field scattered by the isolated half-plane at the boundary is described by E err (see (43)). Plane y = 0 acts as a shadow boundary or transition region. The transition region also appears in other infinite structures with the edge, for example, in the semi-infinite strip gratings [Reference Kaliberda, Litvinenko and Pogarsky31, Reference Hills and Karp36].

For Δ < −r, if q x = q y = 0 and p x = 1, the disk is not illuminated by the plane wave, since it is situated totally “above” the half-plane (the incidence from “below”). Here, the disk is placed in the field of cylindrical wave excited as a result of scattering by the edge of the half-plane. In Fig. 9(c), the field disturbance caused by the disk is slightly seen. Thus to illustrate better the field of the cylindrical wave scattered by the disk, in Fig. 10 we present pattern for lager value of the radius kr = 3π.

For full analysis, it is also necessary to show the field distribution in the horizontal plane. In Fig. 11 we present the near-field distribution in the plane z = 2h (“above” the structure) which corresponds to the minimum of the amplitude of the standing wave. The graphs are symmetric with respect to the line x = 0, since the structure is symmetric. The field of the spherical wave is noticeable in the domain y < 0 especially for E y. It is interesting to compare our results with results for an isolated disk (without half-plane). See, for example, [Reference Nomura and Katsura12]. In the case of the isolated disk in the plane perpendicular to $\vec{E}^i$ (x = 0), electric field has one maxima on the radius at the center of the disk.

Conclusion

In this paper, rigorous solution of the plane wave scattering by the circular PEC disk and PEC half-plane is obtained for the first time. The operator equations with respect to the Fourier amplitudes of the scattered field are reduced to the system of singular integral equations of the second kind. After discretization, the matrix equations are obtained, which are solved with the use of the iterative procedure.

The field scattered by the structure consist of plane wave, cylindrical waves, and spherical waves. The influence of the edge-effect of the half-plane on the disk is highlighted.

Conflict of interest

The authors declare none.

Mstislav E. Kaliberda received his B.S. and M.S. degrees in Applied Mathematics from the V.N. Karazin Kharkiv National University, Kharkiv, Ukraine in 2005 and 2006, respectively, and his Ph.D. degree in 2013 from the same university. Now, he is an Associate Professor in the School of Radio Physics. His current research interests are analytical and numerical techniques, integral equation, multi-element periodic structures, and graphene gratings.

Leonid M. Lytvynenko graduated from the V.N. Karazin Kharkiv National University, Kharkiv, Ukraine and received the combined B.S. and M.S. degree in Radiophysics and Electronics in 1959 and his Ph.D. degree in 1965. From 1966 to 1985 he was with the Institute of Radiophysics and Electronics of the National Academy of Sciences of Ukraine (IRE NASU) in Kharkiv, Ukraine. He is Professor in Radiophysics since 1977. In 1985, he founded the Institute of Radio Astronomy of NASU and served as its Director until 2017. His area of research is in the theory of waves scattering and propagation, antenna systems and engineering, microwave sources, and radio astronomy. He is vice-chairman of the Ukrainian National URSI Committee, member of the European Astronomy Society, and member of the International Astronomy Society. He is also the editor-in-chief of the journal “Radio Physics and Radio Astronomy.”

Sergey A. Pogarsky received his M.S. degree in Radiophysics and Electronics from the V.N. Karazin Kharkiv National University, Kharkiv, Ukraine in 1977, and his Ph.D. degree from the same university in 1984. Since 1977 he has been with the same university as researcher, and since 1984 as senior researcher and part-time senior lecturer at the Department of Physics of Ultra High Frequencies. Since 1999, he is Professor, and part-time Principal Scientist. His research interests include CAD techniques for microwave and millimeter wave components, antenna systems, and microwave transmission lines and circuits.

References

Jones, DS (1950) Note on diffraction by an edge. Quarterly Journal of Mechanics and Applied Mathematics 3, 420434.CrossRefGoogle Scholar
Jones, DS (1952) A simplifying technique in the solution of a class of diffraction problems. Quarterly Journal of Mathematics 3, 189196.CrossRefGoogle Scholar
Noble, D (1958) Methods based on the Wiener-Hopf Technique for the Solution of Partial Differential Equations. London: Pergamon Press.Google Scholar
Copson, ET (1946) On an integral equation arising in the theory of diffraction. Quarterly Journal of Mathematics os-17, 1934.CrossRefGoogle Scholar
Copson, ET (1950) Diffraction by a plane screen. Proceedings of the Royal Society of London 202, 277284.Google Scholar
Khestanov, RK (1968) Diffraction of a wave beam at a half-plane. Radiophysics and Quantum Electrons 11, 793799.CrossRefGoogle Scholar
Bertoni, HL, Green, A and Felsen, LB (1978) Shadowing an inhomogeneous plane wave by an edge. Journal of the Optical Society of America 68, 983989.CrossRefGoogle Scholar
Green, AC, Bertoni, HL and Felsen, LB (1979) Properties of the shadow cast by a half-screen when illuminated by a Gaussian beam. Journal of the Optical Society of America 69, 15031508.CrossRefGoogle Scholar
Rahmat-Samii, Y and Mittra, R (1978) Spectral analysis of high-frequency diffraction of an arbitrary incident field by a half plane – comparison with four asymptotic techniques. Radio Science 13, 3148.CrossRefGoogle Scholar
Gorobets, NN, Yeliseyeva, NP and Antonenko, YA (2012) Optimisation of radiation characteristics of wire-screened antennas. Telecommunications and Radio Engineering 71, 5969.CrossRefGoogle Scholar
Yeliseyeva, NP, Gorobets, AN, Katrich, VA and Nesterenko, MV (2017) Radiation fields of a system of two impedance crossed vibrators excited in-phase and placed over a rectangular screen. Progress in Electromagnetics Research B 77, 52503.CrossRefGoogle Scholar
Nomura, Y and Katsura, S (1955) Diffraction of electromagnetic waves by circular plate and circular hole. Journal of the Physical Society of Japan 10, 285304.CrossRefGoogle Scholar
Lytvynenko, LM, Prosvirnin, SL and Khizhnyak, AN (1988) Semiinversion of the operator with the using of method of moments in the scattering problems by the structures consisting of the thin disks. Preprint institute of radio astronomy. Academy of Sciences UKR SSR 19, 18 (in Russian).Google Scholar
Bouwkamp, CJ (1950) On the diffraction of electromagnetic waves by small circular disks and holes. Philips Research Reports 5, 401422.Google Scholar
Maixner, J and Andrejewski, W (1950) Strenge Theorie der Beugung ebener elektromagnetischer Wellen an der vollkommen leitenden Kreisscheibe und an der kreisförmigen Öffnung im vollkommen leitenden ebenen Schirm. Annalen der Physik 442, 157168.CrossRefGoogle Scholar
Hongo, K and Naqvi, QA (2007) Diffraction of electromagnetic wave by disk and circular hole in a perfectly conducting plane. PIER 68, 113150.CrossRefGoogle Scholar
Losada, V, Boix, RR and Horno, M (1999) Resonant modes of circular microstrip patches in multilayered substrates. IEEE Transactions on Microwave Theory and Techniques 47, 488498.CrossRefGoogle Scholar
Losada, V, Boix, RR and Horno, M (2000) Full-wave analysis of circular microstrip resonators in multilayered media containing uniaxial anisotropic dielectrics, magnetized ferrites, and chiral materials. IEEE Transactions on Microwave Theory and Techniques 48, 10571064.CrossRefGoogle Scholar
Losada, V, Boix, RR and Medina, F (2003) Fast and accurate algorithm for the short-pulse electromagnetic scattering from conducting circular plates buried inside a lossy dispersive half-space. IEEE Transactions on Geoscience and Remote Sensing 41, 988997.CrossRefGoogle Scholar
Di Murro, F, Lucido, M, Panariello, G and Schettino, F (2015) Guaranteed-convergence method of analysis of the scattering by an arbitrarily oriented zero-thickness PEC disk buried in a lossy half-space. IEEE Transactions on Antennas and Propagation 63, 36103620.CrossRefGoogle Scholar
Lucido, M, Panariello, G and Schettino, F (2017) Scattering by a zero-thickness PEC disk: a new analytically regularizing procedure based on Helmholtz decomposition and Galerkin method. Radio Science 52, 214.CrossRefGoogle Scholar
Balaban, MV, Sauleau, R, Benson, TM and Nosich, AI (2009) Dual integral equations technique in electromagnetic wave scattering by a thin disk. PIER B 16, 107126.CrossRefGoogle Scholar
Lucido, M, Balaban, MV and Nosich, AI (2021) Plane wave scattering from thin dielectric disk in free space: generalized boundary conditions, regularizing Galerkin technique and whispering gallery mode resonances. IET Microwaves, Antennas & Propagation 15, 11591170.CrossRefGoogle Scholar
Balaban, MV, Shapoval, OV and Nosich, AI (2013) THz wave scattering by a graphene strip and a disk in the free space: integral equation analysis and surface plasmon resonances. IOP Journal of Optics 15, 114007/9.Google Scholar
Tikhenko, ME, Radchenko, VV, Dukhopelnykov, SV and Nosich, AI (2021) Radiation characteristics of a double-layer spherical dielectric lens antenna with a conformal PEC disk fed by on-axis dipoles. IET Microwaves, Antennas & Propagation 15, 12491269.CrossRefGoogle Scholar
Kaliberda, M, Lytvynenko, L and Pogarsky, S (2022) Electromagnetic wave scattering by half-plane and disk placed in the same plane or circular hole in half-plane. Journal of Electromagnetic Waves and Applications. doi: 10.1080/09205071.2022.2032379.CrossRefGoogle Scholar
Schwarzschild, K (1901) Die beugung und polarisation des lichts durch einen. Spalt I. Mathematische Annalen 55, 177247.CrossRefGoogle Scholar
Kaliberda, ME, Litvinenko, LN and Pogarsky, SA (2010) Diffraction of H0m and E0m modes by a system of axially symmetric discontinuities in a coaxial circuit. Journal of Communications Technology and Electronics 55, 505511.CrossRefGoogle Scholar
Kaliberda, ME, Lytvynenko, LM, Pogarsky, SA and Roiuk, MP (2018) Diffraction of the H-polarized plane wave by a finite layered graphene strip grating. International Journal of Microwave and Wireless Technologies 11, 326333.CrossRefGoogle Scholar
Kaliberda, ME, Litvinenko, LN and Pogarsky, SA (2021) Operator method in the problem of the H-polarized wave diffraction by two semi-infinite gratings placed in the same plane. Radio Physics and Radio Astronomy 26, 350357.CrossRefGoogle Scholar
Kaliberda, M, Litvinenko, L and Pogarsky, S (2017) Method of singular integral equations in diffraction by semi-infinite grating: H-polarization case. Turkish Journal of Electrical Engineering Computer Sciences 25, 44964509.CrossRefGoogle Scholar
Zhang, L, Yang, J, Fu, X and Zhang, M (2013) Graphene disk as an ultra compact ring resonator based on edge propagating plasmons. Applied Physics Letters 103, 163114.CrossRefGoogle Scholar
Saidoglu, NY and Nosich, AI (2020) Method of analytical regularization in the analysis of axially symmetric excitation of imperfect circular disk antennas. Computers & Mathematics with Applications 79, 28722884.CrossRefGoogle Scholar
Muskhelishvili, NI (1972) Singular Integral Equations. Boundary Problems of Functions Theory and their Applications to Mathematical Physics. Groningen, The Netherlands: Wolters-Noordhoff (Revised translation from Russian).Google Scholar
Lifanov, IK (1996) Singular Integral Equations and Discrete Vortices. Utrecht, The Netherlands: VSP.CrossRefGoogle Scholar
Hills, NL and Karp, SN (1965) Semi-infinite diffraction gratings–I. Communications on Pure and Applied Mathematics 18, 203233.CrossRefGoogle Scholar
Figure 0

Fig. 1. Structure geometry.

Figure 1

Fig. 2. Error of the solution: (a) ɛ(N); (b) ɛ(a); and (c) δ(L).

Figure 2

Fig. 3. Far-field patterns of spherical waves, non-zero electric-field components $A_x^{sw}$ and $A_y^{sw}$ (solid lines), $D_x^{sw}$ and $D_y^{sw}$ (dashed lines) for kΔ = 2π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kΔ = −2π (blue lines), φ = 900, kr = π, kh = π/2, normal incidence α = β = 900: (a) qx ≠ 0, qy = px = py = 0; (b) qy ≠ 0, qx = px = py = 0; (c) px ≠ 0, qx = qy = py = 0; and (d) py ≠ 0, qx = qy = px = 0.

Figure 3

Fig. 4. Far-field patterns of spherical waves for kΔ = 2π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kΔ = −2π (blue lines) φ = 00, kr = π, kh = π/2, normal incidence α = β = 900, qx ≠ 0, qy = px = py = 0: (a) $A_x^{sw}$ (solid lines), $A_y^{sw}$ (dashed lines) and (b) $D_x^{sw}$ (solid lines), $D_y^{sw}$ (dashed lines).

Figure 4

Fig. 5. Same study as in Fig. 3, but for kh = π.

Figure 5

Fig. 6. Far-field patterns of spherical waves $A_x^{sw}$ (solid lines), $D_x^{sw}$ (dashed lines) for kΔ = π (black lines), kΔ = 0 (red lines), kΔ = −π (green lines), kr = π/2, kh = π/2, normal incidence α = β = 900, qx ≠ 0, qy = px = py = 0: (a) φ = 00 and (b) φ = 900 (here $A_y^{sw}$ = $D_y^{sw}$ = 0).

Figure 6

Fig. 7. Same study as in Fig. 6, but for kh = π.

Figure 7

Fig. 8. Total field distribution |Ex| in the plane x = 0 for kr = π, kh = π/2, qx ≠ 0, qy = px = py = 0, normal incidence: (a) kΔ = 2π; (b) kΔ = 0; and (c) kΔ = −π.

Figure 8

Fig. 9. Total field distribution |Ex| for x = 0, kr = π, kh = π/2, px ≠ 0, qx = qy = py = 0, normal incidence: (a) kΔ = 2π; (b) kΔ = 0; and (c) kΔ = −π.

Figure 9

Fig. 10. Total field distribution |Ex| for x = 0, kr = 3π, kh = π, px ≠ 0, qx = qy = py = 0, normal incidence.

Figure 10

Fig. 11. Total field distribution in the plane z = 2h for kr = π, kh = π/2, qx ≠ 0, qy = px = py = 0, normal incidence: (a) |Ex| and (b) |Ey|.