# Numerical Investigation of the System-Matrix Method for Higher-Order Probe Correction in Spherical Near-Field Antenna Measurements

Authors: Thorkild B. Hansen
Journal: International Journal of Antennas and Propagation
 (2012)

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## Abstract

The system-matrix method for higher-order probe correction in spherical near-field scanning is
based on a renormalized least-squares approach in which the normal matrix closely resembles the
identity matrix when most of the energy of the probe pattern resides in the first-order modes. This
method will be “stressed-tested” in the present paper by employing probes for which up to 49%
of the pattern energy resides in the higher-order modes. The condition number of the resulting
normal matrix will be computed, and its “distance” from the identity matrix displayed. It is also
shown how the condition number of the normal matrix can be further reduced.


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## Body

## 1. Introduction

The standard theories for spherical near-field scanning of electromagnetic fields [1–5] hold for first-order probes that have e±iϕ azimuthal pattern dependence only. For general higher-order two-port probes, which have unequal port patterns that contain modes eiμϕ with μ≠±1, one cannot use these standard theories. (The term “higher-order mode,’’ refers to all modes with |μ|≠1, including the mode μ=0. Through χ-scanning, the standard method [3] can deal with higher-order probes in special situations. However, this approach does not work in the situation of highest practical importance where the data consists of the output of a two-port higher-order probe.) Therefore, first-order probes have been preferred in spherical near-field scanning over the past 30 years.Unfortunately, first-order probes are inherently narrow-banded, and thus a large number of different probes (each covering a narrow frequency band) are needed to measure the AUT over a broadband of frequencies. In practice, this means that wide-band characterizations become very time consuming because the spherical scan must be repeated many times. In addition, it takes a considerable amount of time to calibrate and change probes because precise alignment procedures are required.Broadband probes that overcome all these problems do indeed exist, but their patterns contain higher-order modes. Typically, most of the probe-pattern energy is still in the first-order modes, but the higher-order modes are nevertheless strong enough to prevent a first-order correction scheme from being accurate. Therefore, the problem of developing probe-corrected theories for spherical near-field scanning that hold for higher-order probes has received considerable attention recently; see [6–8] and references therein.In the present paper we shall evaluate the system-matrix method presented in [8], which uses a renormalized least-squares approach to obtain a probe-corrected theory for general higher-order two-port probes in spherical scanning. The ports need not have identical patterns, and the theory holds for both a ϕ-scan (0≤θ≤π, 0≤ϕ≤2π) or a θ-scan (0≤θ≤2π, 0≤ϕ≤π), and the scan points are obtained by rectangular θ-ϕ sampling. The spherical expansion coefficients of the antenna under test (AUT) are determined by solving a linear system of equations involving a square normal matrix. This solution can be achieved in two alternative ways: (i) an iterative method that employs the conjugate gradient method and (ii) a direct method where the normal matrix is inverted explicitly. Both versions require O(N3) operations with very little overhead. Here, N is the truncation number in the spherical expansion of the AUT field; see Section 2. Through a validation in [8] with experimental data, it was demonstrated that 29280 spherical expansion coefficients of an AUT can be computed in 8 seconds on a PC running Matlab.We will “stress-test’’ the method by using probes for which up to 49% of the pattern energy resides in the higher-order modes. We compute the condition number and other statistics of the resulting normal matrix. Since the AUT spherical expansion coefficients can be obtained more rapidly when the normal matrix is close to the identity matrix, we shall investigate ways to “move’’ the normal matrix closer to the identity matrix.The paper is organized as follows. In Section2 we show how the AUT far-field pattern can be expressed in terms of the transverse spherical vector-wave functions and spherical expansion coefficients. Section 3 describes the renormalized least-squares solution from [8] that will be examined in this paper. In Section 4 we introduce the higher-order test probe that will be used in the numerical examples. Section 5 presents numerical results that include the evaluation of the condition number of the normal matrix for various probes and matrix truncations. In addition, we compute spherical expansion coefficients of a simulated AUT using different truncations of the normal matrix to demonstrate that the higher-order method is exact to machine precision. Moreover, we show that the method is very stable in the presence of noise, as would be expected since the normal matrix is extremely well conditioned. Section 6 presents conclusions. Throughout, we assume time-harmonic fields that have e-iωt time dependence with ω>0.


## 2. Vector-Wave Expansion of the Electric Field of the AUT

In this section we express the AUT far-field pattern in terms of spherical expansion coefficients and transverse spherical vector-wave functions. The standard spherical coordinates(r,θ,ϕ) with unit vectors given by(1)r̂=x̂cos⁡ϕsin⁡θ+ŷsin⁡ϕsin⁡θ+ẑcos⁡θ,θ̂=x̂cos⁡θcos⁡ϕ+ŷcos⁡θsin⁡ϕ-ẑsin⁡θ,ϕ̂=-x̂sin⁡ϕ+ŷcos⁡ϕ
will be used throughout. Here, the unit vectors for the rectangular coordinates (x,y,z) are x̂, ŷ, and ẑ. The AUT is shown in Figure 1 inside the scan sphere with radius R. Moreover, the AUT minimum-sphere radius Rmin is defined such that the maximum (supremum) value of the coordinate r for all points on the AUT equals Rmin.Figure 1
A probe with its reference point on the scan sphere of radiusR and its normal pointing towards the origin measures the field of the AUT.The electric and magnetic AUT far fields can be expressed in terms of the far-field patternF(θ,ϕ) as [9, page 110](2)E(r)~F(θ,ϕ)eikrr,H(r)~ϵ0μ0r̂×F(θ,ϕ)eikrr,
where μ0 and ϵ0 are the free-space permeability and permittivity, respectively. Also, k=ωμ0ϵ0 is the wavenumber. The far-field pattern determined from the electric field as(3)F(θ,ϕ)=lim⁡r→∞re-ikrE(rr̂)
can be expressed in terms of the transverse vector-wave functions Mnm and Nnm as(4)F(θ,ϕ)=1k∑n=1N∑m=-nni-n-1×[AnmMnm(θ,ϕ)+iBnmNnm(θ,ϕ)],
where Anm and Bnm are the spherical expansion coefficients of the AUT, satisfying Anm=0 and Bnm=0 when |m|>n. The truncation number N is determined from the radius of the minimum sphere as(5)N=kRmin⁡+γ(kRmin⁡)1/3,
where the constant γ determines the number of digits of accuracy achieved [10, Section  3.4.2]. The transverse vector-wave functions can be expressed in terms of the spherical harmonic Ynm(θ,ϕ) [11, page 99] as [11, pages 742–746](6)Mnm(θ,ϕ)=θ̂imYnm(θ,ϕ)n(n+1)sin⁡θ-ϕ̂(∂/∂θ)Ynm(θ,ϕ)n(n+1)
and Nnm(θ,ϕ)=r̂×Mnm(θ,ϕ). The formula (4) makes it possible to compute the AUT far-field pattern in any direction from the spherical expansion coefficients Anm and Bnm. The goal of this paper is to evaluate the method presented in [8] for computing Anm and Bnm from the output of a higher-order probe on the scan sphere.


## 3. Renormalized Least-Squares Formulation for Higher-Order Probes

In this section we briefly outline the method derived in detail in [8]. By applying Fourier series expansions for the d-functions in Jensen’s transmission formulas [1–3], one finds that the output of an arbitrary probe on the scan sphere can be expressed as the Fourier series(7)V(j)(θ,ϕ)=∑q=-NN∑m=-NN[∑n=1NAnmAmqn(j)+∑n=1NBnmBmqn(j)]×eimϕeiqθ+ϵ(θ,ϕ),
where ϵ(θ,ϕ) accounts for positioning errors, reflections from chamber walls, inaccuracies in the probe model, and so forth. Here, the index j, which can take the values 1 or 2, represents the two ports of the higher-order probe. Equation (7) holds only when multiple interactions between the probe and AUT are negligible and defines a function that is 2π-periodic with respect to both θ and ϕ.The probe Fourier coefficient𝒜mqn(j) is the Fourier coefficient for the output of Port no. j when An′m′=δnn′δmm′ and Bn′m′=0. Similarly, the probe Fourier coefficient ℬmqn(j) is the Fourier coefficient for the output of Port no. j when Bn′m′=δnn′δmm′ and An′m′=0. We note that 𝒜mqn(j)=0 and ℬmqn(j)=0 when either |q|>n or |m|>n. Here, δmm′=1 if m=m′ and zero otherwise.It was shown in [8] how the probe Fourier coefficients 𝒜mqn(j) and ℬmqn(j) can be computed from the far-field pattern of an arbitrary probe. In the present paper we employ a higher-order probe made from Hertzian dipoles (see Section 4), so the probe output is determined directly from the field on the scan sphere. Hence, we do not need to go through the full formulation developed in [8]. To compute 𝒜mqn(j) and ℬmqn(j), we let VAnm(j)(θ,ϕ) denote the higher-order probe output due to a source with An′m′=δnn′δmm′ and Bn′m′=0. Similarly, VBnm(j)(θ,ϕ) is the higher-order probe output due to a source with An′m′=0 and Bn′m′=δnn′δmm′. The Fourier expansion (7) implies that VAnm(j)(θ,ϕ) and VBnm(j)(θ,ϕ) can be computed at ϕ=0 through(8)VAnm(j)(θ,0)=∑q=-nnAmqn(j)eiqθ,VBnm(j)(θ,0)=∑q=-nnBmqn(j)eiqθ.
We extend the θ variable to the entire range 0≤θ≤2π by noting that the spherical unit vector satisfies r̂(θ,ϕ)=r̂(2π-θ,ϕ+π). The standard sampling theorem for bandlimited periodic functions then gives the following exact expressions for the probe Fourier coefficients(9)Amqn(j)=12n+2∑s=02n+1VAnm(j)(πs(n+1),0)e-iπqs/(n+1),Bmqn(j)=12n+2∑s=02n+1VBnm(j)(πs(n+1),0)e-iπqs/(n+1),
where q=-n,…,0,…,n.Having completed the description of the Fourier formula (7), we next convert it to matrix form. Let the unknown AUT expansion coefficients Anm and Bnm be given by the column vector T with length O(2N2). Hence, the two-dimensional arrays Anm and Bnm are collapsed into one-dimensional arrays and combined in a column vector. Similarly, we let the sampled higher-order probe output V(j)((t-1)Δθ,(p-1)Δϕ) be given by the column vector W of length O(4N2), where t and p are integers. The sphere is discretized through θt=(t-1)Δθ and ϕp=(p-1)Δϕ, where Δθ and Δϕ are chosen as usual to be less than or equal to 2π/(2N+1).The formula (7) defines the probe matrix P¯, so that the probe output is(10)W=P¯T
which is the nonsquare system-matrix equation with more equations than unknowns for determining T for a given W. The probe matrix P¯ has the form(11)P¯=F¯Q¯,
where matrix multiplications with F¯ can be performed using a 2D FFT algorithm and Q¯ performs the summation over n in the square brackets of (7).We developed in [8] the renormalized least-squares solution to (10) given by(12)(p¯-1)HQ¯HF¯Hτ¯W=M¯[p¯T],
where the square matrix M¯ is(13)M¯=(p¯-1)HQ¯HF¯Hτ¯F¯Q¯p¯-1.
Here τ¯ is a diagonal matrix containing the surface element ΔϕΔθ|sin[(p-1)Δθ]| and p¯ is the first-order correction factor, which is a diagonal matrix that represents a first-order correction. The renormalization achieved with p¯ results in M¯ being almost equal to the identity matrix when most of the probe-pattern energy is in the first-order modes.In this paper we use the Hertzian-dipole first-order correction factor with elements𝒰hn(1)(kR) and 𝒰gn(1)(kR), where 𝒰 is the constant determined from the probe Fourier coefficients as(14)U=-8π31g1(kR)∑q=-11B0q1(1)eiqπ/2,
where hn(1)(z) is the spherical Hankel function [11, page 740] and(15)gn(1)(z)=1z∂∂z[zhn(1)(z)].
As discussed in [8], one can compute an optimal first-order correction factor, which may result in more well-conditioned normal matrices than the Hertzian-dipole correction factor used in this paper.The choice of first-order correction factorp¯ does not change the outcome of the computation of the AUT expansion coefficients. It merely affects the matrix M¯ and of course the left side of (12). A good correction factor results in M¯ being close to the identity matrix. Equation (12) can be solved with respect to p¯T using a linear iterative solver such as the conjugate gradient method, regardless of how closely M¯ resembles the identity matrix. However, when M¯≈I¯, we can obtain a closed-form solution by using the Neumann series. The computation scheme presented here has computational complexity N3 [8], and the matrix M¯ is never computed explicitly.


## 4. Higher-Order Test Probe

We shall use an offset Hertzian dipole as the test probe for evaluating the computation scheme. The probe has two ports that each equal the tangential components of the electric field on the scan sphere as shown in Figure2.Figure 2
The higher-order test probe with its reference point at(θ0,ϕ0) on the scan sphere of radius R. The output of Port no. 1 is V(1)(θ0,ϕ0)=Eθ(R,θ0+ψ,ϕ0), and the output of Port no. 2 is V(2)(θ0,ϕ0) given by (19).The higher-order test probe is specified by the offset angleψ. Specifically, when the reference point of the probe is at (θ0,ϕ0), the output of Port no. 1 is the θ component of the electric field at r1(θ0,ϕ0)=Rr̂1=Rr̂(θ0+ψ,ϕ0):(16)V(1)(θ0,ϕ0)=θ̂(θ0+ψ,ϕ0)⋅E(r1(θ0,ϕ0))=Eθ(R,θ0+ψ,ϕ0).The output of Port no. 2 is obtained by rotating the Hertzian dipole of Port no. 1 90 degrees with respect to the unit vectorr̂(θ0,ϕ0). To determine the location of the dipole for Port no. 2, we introduce two lengths Δ and L so that (R+Δ)r̂1=Rr̂0+Lθ̂0, where r̂0 and θ̂0 are the unit vectors corresponding to (θ0,ϕ0). Since r̂1·r̂0=cosψ, we have (R+Δ)cosψ=R and (R+Δ)2=R2+L2, so L=Rtanψ. We can now determine the location r2 of the dipole for Port no. 2 by noting that (R+Δ)r̂2=Rr̂0+Lϕ̂0 which gives(17)r2(θ0,ϕ0)=Rr̂2=R(r̂0cos⁡ψ+ϕ̂0sin⁡ψ),
where ϕ̂0=ϕ̂(θ0,ϕ0). The direction α̂2 of the dipole for Port no. 2 is tangential to the sphere at r2 and lies in the plane containing the origin, r̂2, and r̂0:(18)α̂2(θ0,ϕ0)=1sin⁡ψ(r̂2cos⁡ψ-r̂0)=ϕ̂0cos⁡ψ-r̂0sin⁡ψ
so that the output of Port no. 2 is(19)V(2)(θ0,ϕ0)=α̂2(θ0,ϕ0)⋅E(r2(θ0,ϕ0)).
When ψ=0, the test probe reduces to a first-order probe with outputs equal to the tangential components of the electric field at (θ0,ϕ0). From [8, equation (1)] it is seen that(20)VAnm(1)(θ,0)=θ̂(θ+ψ,0)⋅Mnm(θ+ψ,0)hn(1)(kR),VBnm(1)(θ,0)=θ̂(θ+ψ,0)⋅Nnm(θ+ψ,0)gn(kR),VAnm(2)(θ,0)=α̂2(θ,0)⋅Mnm(r̂2(θ,0))hn(1)(kR),VBnm(2)(θ,0)=α̂2(θ,0)⋅Nnm(r̂2(θ,0))gn(kR)
so that the probe Fourier coefficients 𝒜mqn(j) and ℬmqn(j) can be determined from (9).We shall perform the evaluation of the higher-order computation method using a scan sphere of radius6λ with a minimum radius of the AUT of Rmin=4λ (λ is the wavelength). We employ test probes with ψ equal to 0∘, 0.5∘, 1∘, and 2∘. Figure 3 shows the power spectrum of these probes. The value at |μ|=K is obtained by summing the power of all modes with μ=±K. The plots are normalized so that the power in the μ=±1 modes is 0 dB.The power in the modes of test probes withψ equal to 0∘, 0.5∘, 1∘, and 2∘. The power for each value of |μ|=K is obtained by summing the power of all modes with μ=±K. The plots are normalized so that the power in the μ=±1 modes is 0 dB.
(a)(b)(c)(d)Table1 shows the power content of first-order modes as a function of ψ. The commercially available higher-order probe that was used in the experiential validation in [8] had 97% of its power in the first-order modes. Nevertheless, the remaining 3% of the power residing in the higher-order modes made first-order probe correction completely inadequate. For one of the field components, the AUT far-field pattern error was nearly 10 dB near the main direction; see [8, Figure 5], hence, the need for higher-order methods even when almost all the energy is in the first-order modes.Table 1
Probe-mode power spectrum.
ψ=0ψ=0.5∘ψ=1∘ψ=2∘Power in modes|μ|=1100%96%84%51%Power in modes|μ|≠10%4%16%49%


## 5. Evaluation of the Normal Matrix

With anR=6λ scan sphere and an AUT minimum radius of Rmin=4λ, we compute in this section the normal matrix M¯ corresponding to each of the four probes with ψ equal to 0∘, 0.5∘, 1∘, and 2∘ shown in Figure 3. With γ=7, the truncation formula (5) gives N=46, and we sample the sphere with 48 equally spaced samples in θ and 96 equally spaced samples in ϕ. In actual processing of near-field scanning data, one should never compute M¯ explicitly; see the discussion in [8]. Indeed, the computation and storage of M¯ with N>75 is impractical both in terms of computation time and storage requirement on a typical PC. However, we compute M¯ explicitly in this section to evaluate its condition number and to investigate how closely it resembles the identity matrix.ForN=46 the matrix M¯ has size 4416 × 4416. We shall also consider “truncated’’ versions of M,¯ where only terms with n≤Ntr are included. A truncated M¯ corresponds to computing the spherical expansion coefficients Anm and Bnm of the AUT only up to n=Ntr≤N based on data sampled at the original rate. In other words, when working with a truncated M¯, we neglect AUT coefficients with n>Ntr while keeping the sampling rate of the higher-order probe output on the scan sphere unchanged. Table 2 shows the size of the truncated normal matrices that will be considered here.Table 2
Size of truncatedM¯ matrices.
NtrSize (M¯)464416 × 4416444048 × 4048423696 × 3696403360 × 3360383040 × 3040Table3 shows the condition numbers for the original M¯ matrix and its truncated versions when ψ=0, ψ=0.5∘, ψ=1∘, and ψ=2∘ probes are employed. Here, the Hertzian-dipole correction factor p¯ is included in the computation of M¯. We see that M¯ is well conditioned in all cases. Moreover, the condition number grows as expected with ψ (the condition number is lowest for the first-order probe). We also see that the condition number decreases with truncation (the matrix truncated at n=38 has a lowest condition number for constant ψ). This also implies that the M¯ matrix of a given size gets more well conditioned as the sampling rate on the scan sphere is increased. The optimal first-order correction factor discussed in [8] may result in even more well-conditioned normal matrices.Table 3
Condition number ofM¯ obtained with Hertzian p¯.
Ntrψ=0ψ=0.5∘ψ=1∘ψ=2∘4614.626.431.356.0443.04.87.417.5422.23.45.312.8401.92.84.310.0381.62.53.78.2Table4 shows the corresponding condition numbers obtained by setting p¯=I¯ in the computation of M¯. In other words, no first-order correction factor is applied. In this case the matrix M¯ can be extremely ill conditioned. For example, when ψ=2∘ and Ntr=N=46 the condition number is 1e5. Comparing Tables 3 and 4 clearly demonstrates the benefits of using a proper first-order correction factor represented by the diagonal matrix p¯ containing 𝒰hn(1)(kR) and 𝒰gn(1)(kR), where 𝒰 is given by (14). Also, since p¯ is a diagonal matrix, its associated computational cost is negligible.Table 4
Condition number ofM¯ obtained with p¯ = I¯.
Ntrψ=0ψ=0.5∘ψ=1∘ψ=2∘463e46e48e41e5441e32e32e34e34219521825541240465056853819202130Table5 shows the largest and smallest diagonal values in M¯ (the diagonal elements are positive) for the different probes and different truncation limits under consideration with M¯ computed using a Hertzian p¯. Also shown are the maximum magnitudes of off-diagonal elements for each matrix. The corresponding values for p¯=I¯ are shown in Table 6. We see that it is the proper Hertzian correction factor which insures that M¯ is close to the identity matrix. In agreement with the condition numbers in Table 3, the matrix M¯ is closest to the identity matrix for the first-order probe. Also, truncating M¯ moves it closer to I¯.Table 5
Properties ofM¯ obtained with Hertzian p¯. D is the maximum value occurring in the diagonal (all diagonal elements are positive), d is the minimum value occurring in the diagonal, and O is the maximum magnitude occurring away from the diagonal.
Ntrψ=0ψ=0.5∘ψ=1∘ψ=2∘DdODdODdODdO461.590.420.181.580.420.181.560.430.171.570.410.17441.100.900.0741.090.900.0711.070.910.0661.090.910.092421.050.940.0461.040.950.0451.030.950.0451.040.960.091401.030.960.0341.020.960.031.010.970.0451.030.970.090381.020.970.0271.020.970.0261.010.970.0441.020.970.089Table 6
Properties ofM¯ obtained with p¯ = I¯. D is the maximum value occurring in the diagonal (all diagonal elements are positive), d is the minimum value occurring in the diagonal, and O is the maximum magnitude occurring away from the diagonal.
Ntrψ=0ψ=0.5∘ψ=1∘ψ=2∘DdODdODdODdO464.32e-40.154.32e-40.154.22e-40.144.02e-40.11440.282e-47e-30.282e-47e-30.282e-46e-30.272e-46e-3424e-22e-48e-44e-22e-48e-44e-22e-47e-44e-22e-47e-4409e-32e-42e-49e-32e-42e-49e-32e-42e-49e-32e-42e-4384e-32e-48e-54e-32e-48e-54e-32e-47e-54e-32e-41e-4We finally consider a particular AUT consisting of 500z-directed Hertzian dipoles randomly distributed in a box with dimensions -2.8λ<x<2.8λ, -0.03λ<y<0.03λ, and -2.8λ<z<2.8λ, as shown in Figure 4. (M¯ is of course independent of the AUT; M¯ depends only on the probe, the sampling rate on the scan sphere, and on the highest value of n for which the AUT spherical expansion coefficients are computed.) We computed the exact spherical expansion coefficients Anmexact and Bnmexact of this AUT from its tangential electric field on the scan sphere using a standard first-order method.Figure 4
The AUT consisting of 500z-directed Hertzian dipoles randomly distributed in a box with dimensions -2.8λ<x<2.8λ, -0.03λ<y<0.03λ, and -2.8λ<z<2.8λ, so that Rmin=4λ.We also computed these AUT expansion coefficients from the output of theψ=2∘ higher-order probe using the method described in this paper with Ntr=46 and Ntr=38. These expansion coefficients are denoted Anm(Ntr) and Bnm(Ntr). Relative dB errors are computed as(21)EAnm(Ntr⁡)=20log⁡10⁡(|Anmexact-Anm(Ntr⁡)|max⁡(|Anmexact|)),EBnm(Ntr⁡)=20log⁡10(|Bnmexact-Bnm(Ntr⁡)|max⁡(|Bnmexact|)).
Figure 5 shows the relative dB errors of the AUT spherical expansion coefficients computed without truncating M¯. The error level is at −300 dB corresponding to machine precision (1e-15). Hence, we have numerically validated the higher-order probe-correction scheme. Figure 6 shows the relative dB errors computed with Ntr=38. Here we are neglecting all spherical expansion coefficients with n>38. We see that the error now is at the −130 dB level, which is still very good by anechoic chamber standards (the error level in a good anechoic chamber is −60 dB).Error plots of the spherical expansion coefficients computed from the higher-order probe output withψ=2∘ without truncating the M¯ matrix. (a) is ℰAnm(46) and (b) is ℰBnm(46).
(a)(b)Error plots of the spherical expansion coefficients computed from the higher-order probe output withψ=2∘ by truncating the M¯ matrix. (a) is ℰAnm(38) and (b) plot is ℰBnm(38).
(a)(b)We next illustrate the benefit of dealing with well-conditioned matrices when the near-field data is noisy. Assume that the truncatedM¯ matrix (Ntr=38) is employed in the presence of Gaussian probe-output noise at the -60dB level. In other words, the exact probe output W is contaminated by noise as follows:(22)W(noisy)=W+A10-60/20[G1+iG2]/2,
where G1 and G2 are independent Gaussian random vectors with mean and standard deviation equal to zero and one, respectively. The amplitude factor A is the square root of the standard deviation of the exact probe-output power. The noisy data W(noisy) is inserted into (12) truncated at Ntr=38 to get the corresponding set of noisy AUT expansion coefficients. Figure 7 shows that the error level of these AUT expansion coefficients is at -58dB. Hence, as a consequence of the well-conditioned M¯ matrix, the error of the computed AUT expansion coefficients is roughly at the same level as the noise present in the probe-output data.Error plots of the spherical expansion coefficients computed from the higher-order probe output withψ=2∘ by truncating the M¯ matrix in the presence of Gaussian probe-output noise at the -60dB level. (a) is ℰAnm(38) and (b) plot is ℰBnm(38).
(a)(b)


## 6. Conclusions

We evaluated the system-matrix method for higher-order probe correction in spherical scanning using probes with varying higher-order mode pattern energy. The first-order correction factor employed by the method greatly reduces the condition number of the resulting normal matrix, even when half of the probe-pattern energy resides in higher-order modes. Indeed, for the probe with half its energy in the higher-order modes, the first-order correction factor reduced the condition number of a4416×4416 normal matrix from 1e5 to 56.We also found that even better condition numbers are achieved by truncating the normal matrix; this is equivalent to increasing the sampling rate on the scan sphere for fixed AUT mode truncation number. Increasing the sampling rate by 10% can significantly reduce the condition number and move the normal matrix closer to the identity matrix. This is important for making the Neumann series solution efficient.For probes (like the one used in the experimental validation in [8]) with a few percent of the pattern energy in higher-order modes, the first-order correction factor resulted in a 3696×3696 normal matrix with a condition number of 3.4. The diagonal elements of this normal matrix were in the range from 0.95 to 1.04, and the maximum magnitude of the off-diagonal elements was 0.045. Without the first-order correction factor, the diagonal elements of this normal matrix were in the range from 2e-2 to 4e-2, and the maximum magnitude of the off-diagonal elements was 8e-4. Due to the well-conditioned normal matrices, the method is well behaved in the presence of noise.



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*Source: 493705-2012-03-07.xml*