Radiative transfer of elastic waves in two-dimensional isotropic scattering media: Semi-analytical approach for isotropic source radiation

We formulate the radiative transfer of P- and S-wave energy from an isotropically radiating source in a two-dimensional infinite isotropic scattering medium. For a stable numerical calculation of seismogram envelopes, we take a semi-analytical approach: Energy densities of P and S waves are divided into three parts of the direct-wave terms, the single-scattering terms, and the multiple-scattering terms, and the first two terms and the last term are evaluated analytically and numerically, respectively. Concerning the single-scattering terms, the P- to-S and S-to-P single conversion scattering terms are expressed analytically with a complete elliptic integral of the first kind. The multiple-scattering terms are represented by a double integral with respect to frequency and wavenumber, and can be numerically evaluated by a discrete wavenumber summation and a Fast Fourier Transform. The results based on the numerical implementation are confirmed with an independent numerical calculation using the Monte Carlo method. Our formulation is also applied to consider the equilibration between P and S waves at larger lapse times. The equilibrated S-to-P energy ratio is reproduced and the equilibration time is first derived for two-dimensional cases. Our formulation will be a reference for the understanding of more complex cases.

section_content: Seismogram envelopes have been used to estimate the strength of scattering and absorption in the Earth. Synthesizing realistic seismogram envelopes is needed to model observed envelopes and to invert for the strength of scattering and absorption in the Earth. Radiative transfer theory, which was originally developed in astrophysics (e. g. Chandrasekhar, 1960), is widely used in seismology, because it offers clear physical meanings and mathematical tractability. Various kinds of settings have been modeled using radiative transfer theory in seismology. For more detailed developments, readers can refer to Sato and Fehler (1998). Modeling started from the single scattering of scalar waves for an isotropic source and isotropic scattering in three-dimensional media (e. g. Aki and Chouet, 1975; Sato, 1977a), and in two-dimensional media (e. g. Kopnichev, 1975). Later, multiple scattering was included in the modeling for the three-dimensional case by Wu (1985) and Zeng et al. (1991), and for the two-dimensional case by Shan and Gao (1988). Vector waves (or P waves and S waves) were first considered for the single-scattering case by Sato (1977b) and for the multiple scattering case by Zeng (1993) and Sato (1994), all of which treated threedimensional cases. However, concerning two-dimensional Copyright c The Society of Geomagnetism and Earth, Planetary and Space Sciences (SGEPSS); The Seismological Society of Japan; The Volcanological Society of Japan; The Geodetic Society of Japan; The Japanese Society for Planetary Sciences; TERRAPUB. doi:10. 5047/eps. 2011. 03. 006 cases, we have only found a paper by Trégourès and van Tiggelen (2002) which derived a radiative transfer equation in a thin-plate bounded by two free surfaces. A canonical problem for a two-dimensional full space has not been found. 

The partitioning of P waves and S waves is an important subject. The S-to-P energy ratio is known to be equilibrated after multiple conversion scatterings between P waves and S waves. The equilibrated ratio was elegantly derived for three-dimensional full spaces by Weaver (1982), and, later, for two-dimensional full spaces by Sánchez-Sesma and Campillo (2006). To consider the transition process into the equilibrium, radiative transfer theory for vector waves is necessary; see Zeng (1993), Sato (1994) and Ryzhik et al. (1996). Snieder (2002) proposed a simpler ball-counting method. The S-to-P energy ratio can be used to judge whether a wavefield is in a diffuse state (multiple scattering regime) or not. Shapiro et al. (2000) conducted the first seismic observation in this context and concluded that seismic coda is in a diffuse state. Sánchez-Sesma and Campillo (2006) clarified that the S-to-P energy ratio is also important to retrieve strict Green's tensors from crosscorrelations of noise records using seismic interferometry, which is a rapidly-growing field in seismology, acoustics, exploration geophysics, etc. (e. g. Curtis et al., 2006). 

In this study, we formulate the radiative transfer of elastic waves in a two-dimensional full space for the first time. Simple assumptions on the isotropy of source radiation and scattering enable us to derive semi-analytical expressions: the direct-wave terms and the single-scattering terms are analytically evaluated, and the multiple-scattering terms having an order higher than or equal to two are numerically calculated. The numerical implementation of our formulation is tested and confirmed by comparisons with the purely numerical approach of a Monte Carlo simulation. Finally, we discuss the energy partitioning of a P wave and an S wave in two-dimensional media as an application of our formulation.
section_name: Introduction

section_name: Formulation

section_content: We assume that P-wave energy W P and S-wave energy W S are impulsively radiated from an isotropic source located at the origin in a two-dimensional isotropic scattering medium (Fig. 1 ). Strictly speaking, assumptions of isotropic source radiation and an isotropic scattering pattern are too simple. But they greatly help to understand the mathematical background and to provide a reference for more realistic (or complex) cases. On the way to receivers, energy is scattered and converted from P-to-S and S-to-P. Energy densities for P waves and S waves at location x and time t, which are denoted as E P (x, t) and E S (x, t), satisfy the following integral equation (e. g. Sato, 1994) :

where α 0, β 0 are, respectively, the P-wave and S-wave velocity, and g P P 0, g P S 0, g S P 0, g SS 0 are total scattering coefficients for P-to-P, P-to-S, S-to-P, S-to-S scattering. G P (x, t) is a propagator for P-wave energy which is characterized by the geometrical spreading factor of a reciprocal of r = |x| and propagation with P-wave velocity (e. g. Shang and Gao, 1988; Sato, 1993) as:

(3)

Similarly, G S (x, t) is a propagator for S-wave energy as:

where b is an intrinsic absorption coefficient which is assumed to be equal for both P and S waves here. Operating a Fourier transform with respect to space and a Laplace transform with respect to time on Eqs. ( 3 ) and ( 4 ), we can get the following two relations:

where ˆmeans Laplace transform, ˜means Fourier transform, and k = |k|. The Fourier-Laplace transform of Eqs. (1) and (2) leads to the following two equations:

These are the formal solutions in the wavenumber and frequency domain. However, the direct inverse Fourier-Laplace transform of Eqs. ( 7 ) and ( 8 ) asks for careful numerical treatments, as pointed out by Zeng (1993). So we take the different approach proposed by Sato (1994). We divide the total energy density into a direct wave part, a single-scattering part, and a multiple-scattering part having an order of higher than or equal to 2 as shown in Eq. ( 9 ) for P waves:

ˆẼ P (k, s) = ˆẼ P,0 (k, s) + ˆẼ P,1 (k, s) + ˆẼ P,M (k, s). (9)

The direct P wave ˆẼ P,0 (k, s) is radiated from the source as a P wave and reaches the receiver without any scattering:

The single scattering term ˆẼ P,1 (k, s) is composed of two parts:

ˆẼ P,1 (k, s) = W P ˆG P α 0 g P P 0 ˆG P + W S ˆG S β 0 g S P 0 ˆG P. (11)

On the right-hand side, the first term is a P wave which is radiated from the source as a P wave, scattered once into a P wave, and reaches the receiver. The second term is a P wave which is radiated from the source as an S wave, scattered once into a P wave, and reaches the receiver. 

The last term ˆẼ P,M (k, s) is the summation of energy which is radiated from the source as a P wave or an S wave and scattered more than twice and reaches the receiver as a P wave:

+α 0 g P S 0 β 0 g S P 0 (1 + α 0 g P P 0 ˆG P ) ˆG P ˆG S +W S ˆG S β 0 g S P 0 ˆG P α 0 g P P

+β 0 g SS 0 ˆG S + α 0 g P S 0 β 0 g S P 0 ˆG P ˆG S. 

(

The corresponding expressions for S waves are as follows:

ˆẼ S (k, s) = ˆẼ S,0 (k, s) + ˆẼ S,1 (k, s) + ˆẼ S,M (k, s),( 13 )

(1 -α 0 g P P 0 ˆG P ) +α 0 g P S 0 β 0 g S P 0 (1 + β 0 g SS 0 ˆG S ) ˆG P ˆG S +W P ˆG P α 0 g P S 0 ˆG S β 0 g SS 0 ˆG S (1 -α 0 g P P 0 ˆG P ) +α 0 g P P 0 ˆG P + α 0 g P S 0 β 0 g S P 0 ˆG P ˆG S (16)

We assume the same attenuation for both P and S waves as:

This is a requirement for the analytical derivation of the single-scattering terms as shown in the next subsection and Appendix. The observed ratio of the attenuation of a P wave to that of an S wave for frequencies higher than 1 Hz mostly ranges between 0. 7 and 2 in the lithosphere as shown in figure 5. 3 of Sato and Fehler (1998). Therefore, Eq. ( 17 ) might be the first-order approximation. However, when this assumption does not hold in a strict sense, we need to make an inverse Fourier-Laplace transform of Eqs. ( 7 ) and ( 8 ) directly.
section_name: Basic equations

section_content: In principle, it is possible to estimate the single-scattering terms both by integration in the space-time domain and the inverse Fourier-Laplace transform in the wavenumberfrequency domain. We can obtain P-to-P and S-to-S single scatterings by both methods (e. g. Sato, 1993). However, concerning P-to-S and S-to-P single conversion scatterings, we have so far only succeeded in deriving the analytical expressions by integration in the space-time domain using elliptical coordinates (e. g. page 46 in Sato and Fehler, 1998; page 1195 in Morse and Feshbach, 1953). Here, we briefly summarize the results. The detailed derivation is shown in Appendix. 

Four terms of P-to-P, P-to-S, S-to-P, S-to-S singlescattering energy densities are denoted as E P P,1 (x, t), E P S,1 (x, t), E S P,1 (x, t), E SS,1 (x, t) respectively. The Pto-P single-scattering term is expressed as:

This single-scattering term is equal to the scalar wave case with P-wave velocity (e. g. Sato, 1993). The S-to-S singlescattering term can be derived similarly as:

Conversion scattering terms of P-to-S and S-to-P are more complex:

where

and

and K (x) is the complete elliptic integral of the first kind (e. g. page 590 in Abramowitz and Stegun, 1970). It is noted that this function also appears in the single scattering of scalar waves on a spherical surface (Maeda et al., 2003). 

We find that the S-to-P single-scattering term has the same space-time dependence as the P-to-S singlescattering term:

(23)
section_name: Analytical representation of the single-scattering terms

section_content: Evaluating the direct-wave terms and the singlescattering terms in the space-time domain, the total energy density of P waves is expressed as follows:

The third term in the right-hand side corresponds to the multiple-scattering P wave having an order higher than or equal to 2. This term depends only on k. The Bessel function of the first kind J 0 (kr) originates from a twodimensional Fourier transform. The term can be evaluated numerically using a discrete wavenumber summation (e. g. Bouchon, 1981; Zeng, 1993), equivalent to the trapezoidal rule, with respect to wavenumber, and the Fast Fourier Transform (FFT) with respect to frequency. A similar expression for S waves is as follows:

(25)
section_name: Total energy density of P waves and S waves

section_content: In order to check the self-consistency of the formulation, we consider the energy conservation of a P wave and an S wave. Substituting k = 0 into Eq. ( 7 ) leads to:

The inverse Laplace transform of this equation leads to:

Similarly,

α 0 g P S 0 + β 0 g S P 0 + W S β 0 g S P 0 -W P α 0 g P S 0 α 0 g P S 0 + β 0 g S P 0 e -(α 0 g P S 0 +β 0 g S P 0 )t e -bt. 

(29)

We find that

When b = 0, the sum of the P-wave and S-wave energy is conserved, which means that our formulation is selfconsistent.
section_name: Self-consistency of the formulation

section_name: Numerical Calculation

section_content: We evaluate the direct-wave and the single-scattering terms analytically, and the multiple-scattering terms with the discrete wavenumber summation and FFT. For numerical implementations, we introduce the following normalized (non-dimensional) quantities:

where g P 0 ≡ g P P 0 + g P S 0. We need to discretize the spacetime domain. In the following, we divide the normalized space range 0 ≤ ρ ≤ 40. 96 with a step of 0. 04 and divide the normalized time range 0 ≤ τ ≤ 20. 48 with a step of 0. 01. In evaluating the single-scattering terms, we use a subroutine for the function K (x) in Press et al. (1992). In the discrete wavenumber summation, we should set the range where the effect of fictitious sources does not appear, as:

ρ max = 40. 96 in this case. We assume that the damping of the medium is 0. However, we introduce an artificial damping b = 0. 5 × g P 0 α 0 in the wavenumber-frequency domain for preventing numerical instabilities. The artificial damping is compensated by multiplication of e bt in the time domain. We assume a Poisson solid of α 0 = 6. 0 (km/s) and β 0 = 3. 46 (km/s). Concerning scattering parameters, we assume g P P 0 = g P S 0 = 0. 05 (km -1 ). Then, g S P 0 = 0. 029 (km -1 ) and g SS 0 = 0. 144 (km -1 ) are determined due to the constraints of Eqs. ( 17 ) and (A. 10). The values might be larger for the usual Earth's crust, but are comparable in a volcanic region (e. g. Yamamoto and Sato, 2010). We use such larger scattering coefficients because we are interested in multiple conversion scatterings and their influence on the partitioning of P-wave and S-wave energy as discussed in the next section. For these parameters, the range of calculation in real space and time is 0 ≤ r ≤ 409. 6 [km], 0 ≤ t ≤ 34. 13 [s].
section_name: Numerical implementation of the formulation

section_content: It is necessary to check the numerical implementation of our formulation. For the calculation of seismogram envelopes, a Monte Carlo simulation (e. g. Gusev and Abubakirov, 1987; Hoshiba, 1991) is versatile enough to be applicable to any type of random media and source radiation at the cost of computation time. In this study, we use a two-dimensional version of Yoshimoto (2000), which is equivalent to Przybilla et al. (2006). For the calculation, we emanate 1,000,000 particles from the source. On the way to receivers, scatterings can take place probabilistically according to the assumed medium parameters. The time step is assumed to be 0. 0167 s from dt = dτ/(g P 0 α 0 ). We count the number of particles arriving at a receiver and at a time. We can trace each particle from the source to the receiver by keeping track of the number of scatterings. So we can extract the single-scattering terms and the multiple-scattering terms separately even with the Monte Carlo method. The resultant envelopes are also normalized according to Eq. ( 31 ) for comparison with the envelopes based on our formulation.
section_name: Monte Carlo simulation to confirm the numerical implementation

section_content: In Fig. 2, we show the energy densities of four singlescattering terms of P-to-P, P-to-S, S-to-P, S-to-S scattering at a receiver with a normalized distance ρ of 0. 2. The horizontal axis is the normalized time τ and the vertical is the normalized energy density ε P, ε S as defined in Eq. ( 31 ). The panel shows the contribution of the four terms. Solid curves are obtained by our implementation. Gray curves are calculated based on the Monte Carlo simulation. Both traces show good coincidence with each other. Because W S = 1. 5γ 5 W P = 23. 38W P assuming a Poisson solid of γ = √ 3, S-to-S and S-to-P single-scattering terms are larger than the other two terms. We also note that S-to-P and P-to-S single-scattering terms are similar as proved in Eq. ( 23 ). The P-to-P and S-to-S scattering terms have a square-root singularity at the onset times of P waves and S waves, respectively. The P-to-S and S-to-P scattering terms have a logarithmic singularity at the onset of an S wave. Both kinds of singularities are integrable. The Monte Carlo results show larger fluctuations at larger lapse times especially for a P wave due to the smaller number of Pwave particles. In Fig. 3, we show the contribution of single scattering (dotted curves) and multiple scattering (broken curves) in the total energy density (gray solid curves) at two receivers with the normalized distances of 1 and 2. The top panel shows an S wave and the bottom panel shows a P wave. The single-scattering term is dominant around the onset times of a P wave and an S wave. On the other hand, the multiple-scattering term grows soon after the P-wave onset. A small fluctuation in S-wave energy at lapse times between P-wave onset and S-wave onset is found. This is due to numerical instabilities which we cannot so far remove. However, we think that the fluctuation is not serious because its amplitude is less than 1% of the maximum amplitude of the S-wave energy. 

In Fig. 4, we show temporal changes of P-wave and S-wave energy density at two receivers with normalized distances of 1 and 2. All of the direct-wave, the singlescattering and the multiple-scattering terms are included. Solid curves are from our implementation. Gray curves are calculated by the Monte Carlo method. Both traces show fairly good matches. This provides confirmation that we can correctly calculate P-wave and S-wave energy density by our proposed method.
section_name: Results

section_content: We have succeeded in formulating the elastic radiative transfer for a two-dimensional random full space for the first time. This is a canonical problem. It is not easy to find Norm. Time practical applications. However, our formulation is useful from the viewpoint of the physics of wave propagation in random media. Our formulation makes it possible to understand directly the effect of dimensionality on the radiative transfer of elastic waves by comparison with formulations for three-dimensional cases. Another benefit of our formulation concerns the validity of seismic interferometry as discussed in this section. 

Recently, the partitioning of P-wave and S-wave energy draws attention to the applicability of seismic interferometry, as shown by Sánchez-Sesma and Campillo (2006). This is also of importance in investigating which is predominant between single scattering and multiple scattering in seismic coda (e. g. Shapiro et al., 2000). Intensive studies have been carried out so far in three-dimensional scattering media (e. g. Margerin et al., 2000). Our formulation enables us to quantitatively investigate the partitioning problem in two-dimensional scattering media, which has scarcely been considered. 

In order to solve the problem, we can start from Eqs. ( 27 ) and (29). By taking the limit of t → ∞ after dividing Eq. ( 29 ) by Eq. ( 27 ), we obtain the S-to-P energy ratio in equilibrium:

The relation (A. 10) is used in the second equality. Equation ( 33 ) is consistent with a result in Sánchez-Sesma and Campillo (2006). For the Poisson solid, the S-to-P energy ratio will converge to 3 irrespective of the initial S-to-P energy ratio at the source. This is thanks to multiple conversion scatterings between a P wave and an S wave. And (A. 10) shows that seismic waves tend to become S waves easily through conversion scatterings. 

The time necessary to attain a state of equilibrium is sometimes called the equilibration time. We can derive the Norm. Time The gray line shows the equilibrated value of 3 which is expected for a two-dimensional Poisson medium at large lapse times. The initial value of the S-to-P energy ratio is assumed to be 23. 38 and 0. 043 for the left and the right panels, respectively. 

equilibration time from the time constant of the exponential terms on the right-hand side of Eqs. ( 27 ) and ( 29 ) for b = 0:

Equation ( 34 ) is found to be the same as the threedimensional cases shown by Sato (1994). In the twodimensional cases, the relation (A. 10) holds between the P-to-S and the S-to-P conversion scattering coefficients. So the equilibration time can be expressed as:

These expressions are obtained for the two-dimensional case for the first time. Contrasting with Eq. (A. 10) for two-dimensional cases, the following relation holds for the three-dimensional cases (e. g. Margerin et al., 2000) :

So, in comparison with the two-dimensional case, the equilibration time in the three-dimensional case can be expressed as:

The equilibration time is smaller in the two-dimensional case than the three-dimensional case for the same P-to-S total scattering coefficient g P S 0. However, this becomes the opposite for the same S-to-P total scattering coefficient g S P 0. Therefore, the relation depends on the scattering coefficients. 

Temporal changes in P-wave and S-wave energy in all the space are shown in the middle and the bottom panels of Fig. 5. The top panel shows the S-to-P energy ratio. The gray line shows the equilibrated value of 3 which is expected for a two-dimensional Poisson medium at large lapse times as in Eq. ( 33 ). The initial value of the S-to-P energy ratio is 23. 38 in the left panels. The ratio decreases with time and converges to the expected value of 3. This is due to the multiple conversion scatterings between a P wave and an S wave. The equilibration time of Eq. ( 35 ) is calculated to be 1. 5 in the normalized time. In the right panels, we consider a case with a different initial value of the S-to-P energy ratio of 0. 043 (= 1/23. 38). For this case, the S-to-P energy ratio gradually increases with time and converges to the value of 3. From these tests, we confirm that the equilibrated value of 3 is irrespective of the initial value at the source and is the result of multiple conversion scatterings between a P wave and an S wave. 

In Fig. 6, the bottom panel shows the S-to-P energy ratio at three receivers with normalized distances of 0. 2, 1 and 2. The top panel shows the S-to-P energy ratio in all the space (or global equilibration) for comparison. Different from the global equilibration, it takes a longer time to reach the equilibrium at each point in the space (or local equilibration). At least, more than 10 in normalized time seems necessary for local equilibration. This is explained by the spatial distribution of energy: S waves are dominant close to the source, and P waves are rich close to an expanding propagation front. The local value of the S-to-P energy ratio remains larger than 3 near the source for a longer time due to S waves slowly diffusing outward, though the ratio in the entire space (global value) becomes 3 quickly.
section_name: Discussions

section_content: We have formulated the radiative transfer of P-wave and S-wave energy from an isotropic source in a twodimensional isotropic scattering media. For a stable numerical calculation of seismogram envelopes, we divide energy densities of P waves and S waves into three parts: the direct-wave terms, the single-scattering terms, and the multiple-scattering terms having an order of higher than or equal to 2. The direct-wave terms and the single-scattering terms can be evaluated analytically. Analytical expressions for the single scatterings are obtained in the spacetime domain using elliptic coordinates. Especially, the single conversion scatterings of P-to-S and S-to-P have been discovered to be represented by a complete elliptic integral of the first kind. Multiple scattering terms can be expressed by double integration with respect to frequency and wavenumber. Discrete wavenumber summation with respect to wavenumber, and FFT with respect to frequency, is adopted. The results based on the numerical implementation of our formulation have been validated by an independent numerical calculation using the Monte Carlo method. Using our formulation, we investigated the equilibration between P-wave and S-wave energy in a two-dimensional random full space. The equilibrated value of the S-to-P energy ratio has been reproduced and the equilibration time has been derived, for the first time, for two-dimensional media. Though our formulation is made for a canonical problem imposing simple assumptions of an isotropic source radiation and an isotropic scattering pattern, it enables us to see the effect of dimensionality on the radiative transfer of elastic waves. It is also helpful in understanding the mathematical background of radiative transfer theory. 

where the ranges of coordinates are 1 ≤ v ≤ ∞, -1 ≤ w ≤ 1, and the constant v corresponds to an ellipse and the constant w corresponds to a hyperbola. The source is located at the origin z 1 = 0 and z 2 = 0 or v = 1, and w = -1, and the receiver is located at z 1 = 0 and z 2 = r corresponding to v = 1 and w = 1. The source-scatterer distance is r a ≡ z 2 1 + z 2 2 = r 2 (v + w), and the scattererreceiver distance is r b ≡ z 2 1 + (z 2r ) 2 = r 2 (v -w). Assuming a geometrical symmetry with respect to z 1 = 0, we can derive the P-to-P single-scattering term as:

Thus, Eq. ( 18 ) is derived. The S-to-S single-scattering term can be derived similarly as:

Conversion scattering terms need more careful treatment. 

The P-to-S single-scattering term is expressed as:

Here, the assumption of Eq. ( 17 ) is necessary to take exp(-ηt) out of the integral. We introduce the following quantity

which satisfies the equation 2α 0 t r (γ +1) -γ -1 γ +1 w 2 -1 = 0. γ is defined in Eq. ( 22 ). 

For the evaluation of the integral in (A. 5), we need to divide the range of time into two parts. First is the time range where a P wave arrives but an S wave does not arrive. 

(1) 1 ≤ α 0 t r < γ

For the range, the following inequality holds: -1 ≤ w ≤ w -≤ 1 < w +. According to page 290 in Gradshteyn and Ryzhik (1994), the integral (A. 5) can be estimated using the incomplete elliptic integral of the first kind F(x, y) and the complete elliptic integral of the first kind K (x) as E P S,1 (x, t) = W P g P S 0 γ e -ηt π 2 r (γ -1)

= W P g P S 0 2γ e -ηt π 2 r (γ -1)

× F sin -1 (w + -w -) (w+1) (w -+1) (w + -w), (w + -1) (w -+1) 2(w + -w -)

w--1 = W P g P S 0 γ e -ηt π 2 r

(A. 7)

(2)

For the second range, the following inequality holds: -1 ≤ w ≤ 1 ≤ w -< w +. Similarly, according to page 290 in Gradshteyn and Ryzhik (1994), the integral can be estimated: E P S,1 (x, t) = W P g P S 0 γ e -ηt π 2 r (γ -1)
section_name: Conclusions

section_content: W P g P S 0 2γ e -ηt π 2 r (γ -1)

r -1 √ (w + -1) (w -+ 1) × F sin -1 (w + -1) (w+1)

2(w + -w), 2(w + -w -) (w + -1) (w -+1)

(A. 8) Summarizing the two cases, we obtain Eq. ( 20 ). 

Finally, the S-to-P single scattering term is considered. W S g S P 0 β 0 W P g P S 0 α 0 E P S,1 (x, t) = W S W P γ 2 E P S,1 (x, t). (A. 9)

In the derivation, the following relation is used:. 10) This relation holds for any type of two-dimensional scattering medium due to the reciprocity (e. g. Aki, 1992).
section_name: =

section_content: Acknowledgments. Constructive comments from the editor Dr. Tatsuhiko Hara and an anonymous reviewer are greatly acknowledged. We are very grateful to the other reviewer, Dr. Jun Kawahara, for pointing out many typing errors left in the original manuscript. We used Generic Mapping Tools (Wessel and Smith, 1998). This study was supported by Grant-in-Aid for Scientific Research (C) ( 20540413 ) and for Young Scientists (B) (20740248) from the Japan Society for the Promotion of Science (JSPS) and the Ministry of Education, Culture, Sports, Science and Technology (MEXT). We also thank JSPS and Deutsche Forschungsgemeinschaft (DFG) for support under the Japan- Germany Research Cooperative Program.

section_name: Appendix A. Derivation of the Single-Scattering Terms

section_content: We derive the single-scattering terms using the elliptical coordinate (e. g. page 46 in Sato and Fehler, 1998 ; page 1195 in Morse and Feshbach, 1953). The location of a scatterer z = (z 1, z 2 ) T is:
section_name: Appendix A. Derivation of the Single-Scattering Terms