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 (−a; a). After that we divide segment [−a; a] 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 kρ → ∞, 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/(kρ), if kρ → ∞. 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.