Analysis of Wave Propagation with Different Magnetic Configurations in Helicon Plasmas

Abstract

A two-dimensional plasma–wave interaction model, which is based on the cold collisional plasma dielectric tensor, is applied to investigate the wave propagation and power depositions under different magnetic configurations in helicon plasmas. The varied magnetic configurations are formed by changing the radius of the magnetic coil. When the magnetic coil was positioned closer to the plasma, the magnetic field within the plasma became stronger and more curved. Consequently, the simulation results show that the wave propagation and power deposition in plasmas follow the curved magnetic field lines. In the axial direction, the periodic distribution of wave fields and power deposition are clearly observed and keep consistency in helicon plasmas due to the eigenmodes of helicon waves. Furthermore, a concave dark area where the wave cannot propagate is observed in the closest magnetic coil case and leads to limited power deposition.

1. Introduction

Electric propulsion has become one of the most widely used technologies in space propulsion due to its advantages of long lifetime, high reliability and low cost [1,2,3]. A prominent type of electric propulsion is the helicon plasma thruster, which represents a novel electrodeless system [4,5,6,7,8,9,10,11]. This propulsion system consists of a helicon plasma source and a magnetic nozzle. The helicon plasma source is primarily responsible for the ionization of the propellant gas, while the magnetic nozzle facilitates plasma acceleration, resulting in the generation of thrust [12,13].

The helicon source of thrusters utilizes RF antennas to emit electromagnetic waves in a background magnetic field for the purpose of ionizing neutral gas [14,15,16]. Due to its distinctive physical mechanism, it can achieve remarkably high ionization efficiency [17]. This property was first discovered in the experiments by Boswell in 1980s [18] and was a key factor in its suitability as a plasma source for electric propulsion. Moreover, it also has broad application prospects in the fields of material processing, plasma etching and fusion-relevant processes [17,19]. Therefore, extensive studies for the helicon source have been carried out by numerous researchers. The wave propagation, the mechanism of power deposition and plasma transport in helicon sources have been extensively investigated [17,20,21]. It is found that there are two branches of waves existing in helicon plasmas [14,22,23]. One is the helicon mode, which is a fast wave with long wavelength. And the other one is the Trivelpiece–Gould (TG) mode, which is a slow wave with small wavelength compared with the helicon mode. These two coupling modes propagating in plasmas are one of reason for the high ionization rate of the helicon source and the mode conversion between them could be the main mechanism of power deposition [17,20]. Furthermore, the experimental results show that the helicon plasma source can operate in three distinct modes: capacitive (E mode), inductive (H mode) and helicon-wave mode (W mode) [24]. The mode transition can be observed with increasing power or magnetic field, and a density jump occurs from one mode to another. In general situation, the W mode can produce higher plasma density than others. And in recent study, it was found that there is a special discharge mode called ‘blue core’ in the helicon-wave mode that can further enhance the plasma density and the plasma can present a very bright core of blue lights [25].

The influence of background magnetic fields plays a vital role in determining the performance of helicon sources [26]. Traditionally, theoretical and numerical studies have predominantly assumed the applied magnetic fields to be homogeneous, aiming to simplify their inherent complexity. Arnush and Chen [27] developed a plasma–wave interaction model based on the uniform magnetic field to investigate the property of wave propagation in different parameter regimes. Cho also established a 1D self-consistent model of helicon plasmas to calculate the coupling of the plasma–wave interaction and plasma transports [28]. Nevertheless, it is crucial to recognize that magnetic fields in helicon discharges are inherently non-uniform, and this non-uniformity would lead a substantial influence on both wave propagation and plasma transport. Therefore, Kinder and Kushner [29,30] developed a two-dimensional Hybrid Plasma Equiqment Model (HPEM) to study the power absorption and plasma transport in helicon source with considering the non-uniform magnetic field. Similarly, the other self-consistent model, which can deal with 2D non-uniform properties, was introduced by Bose et al. [31]. It is concluded that the propagation of waves is enhanced in the downstream by increasing the electromagnet coil current ratio (CCR) and this is accompanied by a increase in power absorption in the downstream. In order to simulate the physical processes in a linear helicon device, Naulin [32] established a 3D global fluid model, which considered the inhomogeneous magnetic field. The phenomenon of turbulent fluctuations are observed in numerical results and the results agree well with the experiments. Magarotto et al. [33,34] presented a numerical tool named 3D-VIRTUS, which consists of an Electro-Magnetic Module and a Fluid Module to simulate the helicon plasma sources with inhomogeneous plasma density and magnetic field. This code has been validated against other well-established numerical approaches and experimental measurements. A two-dimensional fully kinetic particle-in-cell model coupling with the electromagnetic wave module was introduced by Emoto [35] to investigate the thrust generation of a magnetic nozzle in a helicon plasma thruster. It is found that the diamagnetic effect plays a significant role in the thruster generation. In addition, a hybrid PIC/fluid transport model combined with a frequency-domain electromagnetic field model was introduced by Jiménez [36] to analyze the helicon discharge with a cusped magnetic configuration in helicon thrusters. It is concluded that the cusp plays a central role in determining the plasma losses to the walls.

Thus, the non-uniformity of magnetic fields is a crucial problem of helicon discharges. In this paper, the wave propagation and power deposition with different magnetic configurations in helicon plasmas are investigated by a 2D plasma–wave interaction model. The wave pattern and the distribution of power density are discussed to analyze the characteristics of wave propagation in different distributions of magnetic fields.

The structure of the rest of the paper is as follows. The model description is introduced in Section 2. Section 3 gives the main results and discussion. Finally, Section 4 is the conclusion of this work.

2. Model Description

Figure 1 sketches the typical helicon source system inside a conducting vacuum chamber of length L and radius $r_w$. The cylindrical coordinate is considered in this model. The helicon source of radius $r_p$, located in the center of chamber, is made of a cylindrically dielectric tube where the plasma is generated and heated. The thickness of the dielectric tube is not taken into account. The plasma in the tube is confined by the background magnetic field ${\mathit{B}}_a(r,z)$, which is produced by the external magnetic coil. Here, a single magnetic coil is considered to produce the magnetic field and the magnetic configuration is varied by changing the radius of the magnetic coil $R_c$. Thus, the distribution of magnetic fields is given as [37]

$${\mathit{B}}_a(r,z)=B_a(r,z)({\mathbf{1}}_{r}sin\alpha +{\mathbf{1}}_{z}cos\alpha )$$

(1)

where $\alpha$ is the local angle between the magnetic field and the axis. In the helicon source, the plasma density is nonuniform and considered to be as a function of $n(r,z)$. The antenna with the radius $r_a$ wrapped around the plasma source emits the electromagnetic radiation of frequency $\omega$. The EM wave propagates in the plasma and the angle between the wavenumber $\mathit{k}$ and the magnetic field ${\mathit{B}}_a$ is defined as $\beta$.

Therefore, Maxwell equations, which govern the plasma wave response, are given in the frequency domain

$$\begin{array}{cc}\hfill & \nabla \times \mathit{E}=i\omega \mathit{B}\hfill \end{array}$$

(2)

$$\begin{array}{cc}\hfill & \nabla \times \mathit{B}={\mu }_0(-i\omega \mathit{D}+{\mathit{j}}_a)\hfill \end{array}$$

(3)

where $\mathit{E}$ and $\mathit{B}$ represent the induced electromagnetic field. ${\mathit{j}}_a$ is the external current density, which is determined by the geometry of specific antenna types. $\mathit{D}$ is the electric displacement field and the expression is written as [19]

$$\mathit{D}={ϵ}_0\overline{\overline{\kappa }}(r,z)·\mathit{E}$$

(4)

Here, ${ϵ}_0$ is the permittivity in the vacuum and $\overline{\overline{\kappa }}(r,z)$ is a general dielectric tensor in the medium. Considering the applied magnetic field, the general dielectric tensor takes the form [37,38]

$$\stackrel{=}{\kappa }=\left[\begin{array}{ccc}cos\alpha & 0& sin\alpha \\ 0& 1& 0\\ -sin\alpha & 0& cos\alpha \end{array}\right]·\left[\begin{array}{ccc}{\kappa }_1& i{\kappa }_2& 0\\ -i{\kappa }_2& {\kappa }_1& 0\\ 0& 0& {\kappa }_3\end{array}\right]·\left[\begin{array}{ccc}cos\alpha & 0& -sin\alpha \\ 0& 1& 0\\ sin\alpha & 0& cos\alpha \end{array}\right]$$

(5)

where ${\kappa }_j$ ($j=1,2,3$) is the component of the dielectric tensor and can be written as [39]

$$\begin{array}{cc}\hfill & {\kappa }_1=1-\sum _k\frac{{\omega }_{pk}^2\left(\omega +i{\nu }_k\right)}{\omega \left[{\left(\omega +i{\nu }_k\right)}^2-{\omega }_{ck}^2\right]},\hfill \end{array}$$

(6)

$$\begin{array}{cc}\hfill & {\kappa }_2=-\sum _k\frac{s_k{\omega }_{ck}{\omega }_{pk}^2}{\omega \left[{\left(\omega +i{\nu }_k\right)}^2-{\omega }_{ck}^2\right]},\hfill \end{array}$$

(7)

$$\begin{array}{cc}\hfill & {\kappa }_3=1-\sum _k\frac{{\omega }_{pk}^2}{\omega \left(\omega +i{\nu }_k\right)}\hfill \end{array}$$

(8)

where ${\omega }_{ck}$ and ${\omega }_{pk}$ are the cyclotron and plasma angular frequencies for ions and electrons ($k=i,e$). ${\nu }_k$ is the particle collision frequency and $s_k$ is the sign of the electric charge. It is noted that we consider the helicon plasma is cold and low temperature. Thus, the thermal effect of particles like Landau damping is not taken into account.

Then, all variables are assumed to vary as $exp\left(im\theta -i\omega t\right)$, the general Maxwell equations can be expanded for each azimuthal m mode [37]

$$\begin{array}{cc}\hfill & \frac{im}{r}{E}_z-\frac{\partial }{\partial z}{E}_{\theta }-i\omega B_r=0,\hfill \end{array}$$

(9)

$$\begin{array}{cc}\hfill & \frac{\partial }{\partial z}{E}_r-\frac{\partial }{\partial r}{E}_z-i\omega B_{\theta }=0,\hfill \end{array}$$

(10)

$$\begin{array}{cc}\hfill & \frac{1}{r}\frac{\partial }{\partial r}\left(r{E}_{\theta }\right)-\frac{im}{r}{E}_r-i\omega B_z=0,\hfill \end{array}$$

(11)

$$\begin{array}{cc}\hfill & \frac{im}{r}{B}_z-\frac{\partial }{\partial z}{B}_{\theta }+i\omega {\mu }_0{D}_r={\mu }_0{j}_r,\hfill \end{array}$$

(12)

$$\begin{array}{cc}\hfill & \frac{\partial }{\partial z}{B}_r-\frac{\partial }{\partial r}{B}_z+i\omega {\mu }_0{D}_{\theta }={\mu }_0{j}_{\theta },\hfill \end{array}$$

(13)

$$\begin{array}{cc}\hfill & \frac{1}{r}\frac{\partial }{\partial r}\left(r{B}_{\theta }\right)-\frac{im}{r}{B}_r+i\omega {\mu }_0{D}_z={\mu }_0{j}_z\hfill \end{array}$$

(14)

Considering the helicon source is enclosed in a metallic vacuum chamber, the boundary condition in this model is mainly determined by the ideally conducting walls and the smooth condition in the symmetric axis. Therefore, the boundary conditions are written as [40,41]

$$\begin{array}{cc}\hfill & E_r=E_{\theta }=B_z=0,\mathrm{at}\left(r,z\right)=\left(r,0\right),\left(r,L\right)\hfill \end{array}$$

(15)

$$\begin{array}{cc}\hfill & E_{\theta }=E_z=B_r=0,\mathrm{at}\left(r,z\right)=\left(r_w,z\right).\hfill \end{array}$$

(16)

and at the symmetric axis $r=0$

$$\begin{array}{cc}\hfill & E_z=r{E}_{\theta }=0,\mathrm{when}m\ne 0\hfill \end{array}$$

(17)

$$\begin{array}{cc}\hfill & r{E}_{\theta }=B_{\theta }=0,\mathrm{when}m=0\hfill \end{array}$$

(18)

Therefore, this equation system can be solved by applying the finite difference method and Yee’s scheme coupling the boundary conditions to obtain all components of EM fields. The Yee’s scheme is a well-known staggered grids method to discretize the calculation domain for the electromagnetic wave propagation problems [42]. The different components of EM fields are positioned in different grids. The advantages of this method are convenient to deal with boundary conditions and reduce the calculation time. This algorithm has been well described in Refs. [37,40,41].

Once all EM fields have been determined, the power deposition in plasmas can be calculated. The time-averaged power density in plasmas for each m mode is [26,37]

$$\begin{array}{c}\hfill p_{abs}=\frac{1}{2}\mathrm{Re}\left({\mathit{E}}^{*}·{\mathit{j}}_p\right)\end{array}$$

(19)

Here, ${\mathit{j}}_p$ is the current density of plasmas. The asterisk represents the complex conjugate. It is assumed that the antenna is a perfect conductor and no power is loss in it. All RF energy is deposited in the plasma. Therefore, the total power absorbed by plasmas is

$$\begin{array}{c}\hfill P_{tot}=\frac{1}{2}{\int }_{V_p}\mathrm{Re}\left({\mathit{E}}^{*}·{\mathit{j}}_p\right)dV\end{array}$$

(20)

where $V_p$ is the volume of plasmas. The antenna impedance Z can be calculated by [27]

$$\begin{array}{c}\hfill Z=-\frac{{\int }_{V_a}\left({\mathit{j}}_a^{*}·\mathit{E}\right)dV}{|I_a{|}^2}\end{array}$$

(21)

where $V_a$ represents the volume of antenna. $I_a$ is the amplitude of the antenna current. Thus, the antenna resistance and reactance are $\mathrm{Re}\left(Z\right)$ and $\mathrm{Im}\left(Z\right)$, respectively.

3. Results and Discussion

In this section, the numerical results of different magnetic configurations in helicon plasmas are discussed. The numerical simulations are carried out by the two-dimensional plasma–wave interaction model, and the geometric setup of the helicon source is depicted in Figure 1. The source system which has a radius of 1 cm, is immersed in a cylindrical vacuum chamber with the length 10 cm and the radius 2 cm. A typical antenna type named ‘Nagoya III’ is applied to emit RF electromagnetic waves with a frequency of $13.56$ MHz for ionizing and heating the plasma. It is assumed that the antenna wire is an ideal thin conductor. The radial component of the current density $j_{za}$ can be neglected. Thus, the expression of current density for the Nagoya III antenna is written as [37,40]

$$\begin{array}{cc}\hfill j_{za}& =\left\{\begin{array}{cc}& \frac{I_a}{\pi r_a}G\left(r\right)H(z-z_1)H(z_2-z),m\mathrm{is}\mathrm{odd}\hfill \\ & 0,\mathrm{otherwise}\hfill \end{array}\right.\end{array}$$

(22)

$$\begin{array}{cc}{j}_{\theta a}& =i\frac{r_a}{m}\frac{\partial j_{za}}{\partial z}\end{array}$$

(23)

Here, $z_1$ and $z_2$ are the position of the axial ends of the antenna. H is the Heaviside step function and $G\left(r\right)$ is given as a Gaussian function profile in order to deal with the singularity at the antenna border [37]. The azimuthal component of current density $j_{\theta a}$ is calculated by satisfying the divergence free of the antenna current. For Nagoya III antenna, the main contribution of azimuthal modes m has been proved to be $m=+1$ mode [37,40,41]. It can be higher than $97\%$. Therefore, only $m=+1$ mode is taken into account in the simulation.

In this work, we focus on the wave propagation in different magnetic configurations. Thus, in order to reduce the complexity due to the process of the plasma transport, the fluid process of plasmas is not taken into account. The plasma parameters is given as an input data. It is assumed that the plasma density in helicon source is axially uniform and satisfies a Gaussian distribution in radial direction [37,43]. The reference density $n^{*}$ is set at the position of center. The particle collision in plasmas is considered to be dominated by the electron–ion collision and the electron collision frequency is ${\nu }_e={\nu }_{ei}$. It can be written as

$$\begin{array}{c}\hfill {\nu }_{ei}=n{T}_{e}ln\mathsf{\Lambda }\times 2.9\times {10}^{-12}\end{array}$$

(24)

where n is the plasma density and $T_e$ is the electron temperature. $\mathsf{\Lambda }$ is the parameter depending on the electron density and temperature.

In this model, the magnetic coil is used to produce the background magnetic field to confine the plasmas. The magnetic configurations is implemented by varying the radius of magnetic coil. We set that a single magnetic coil is axially located at the center of the plasma source and the current on the magnetic coil is unchanged. The resulting magnetic configuration can be determined by the radius of magnetic coil and calculated by Ampere’s law [44,45]. All parameters of the source system in simulations are given in

Table 1. Numerical parameters used in the simulations.

Symbol	Parameter	Value
L	Chamber and source length	10 cm
$r_w$	Chamber radius	2 cm
$r_p$	Plasma source radius	1 cm
$r_a$	Antenna loop radius	$1.2$ cm
$L_a$	Antenna axial length	$2.5$ cm
$z_a$	Antenna central position	$2.5$ cm
$d_t$	Antenna wire thickness	$0.1$ cm
$I_a$	Antenna current	1 A
$f_{RF}$	Frequency of RF emission	$13.56$ MHz
$B_a^{*}$	Reference magnetic field	150 G
$n^{*}$	Reference plasma density	$3.8\times {10}^{18}$ ${\mathrm{m}}^{-3}$

.

In addition, the finite different method with Yee’ s scheme is applied on a uniform Cartesian grid in $(r,z)$ to discretize Equations (9)–(14) into a matrix problem, which is then solved numerically for $\mathit{E}$ and $\mathit{B}$ on the grid nodes with a direct serial solver. Each of staggered regular grid used here has $N_z\times N_r=3000\times 1000$ nodes, which for the chamber geometry gives a cell size with $\Delta z\approx 33.3$ $\mathsf{\mu }$m, $\Delta r=20$ $\mathsf{\mu }$m. Therefore, the calculation time for this setting is about two hours per case in this work.

Figure 2 shows the spatial distribution of magnetic field produced by a single magnetic coil in this source structure when the radius of coil $R_c$ is 3 cm. The yellow light point is the position of the current loop of magnetic coil. The magnetic field streamlines are represented by the black solid line and the red solid line gives the bound between the vacuum and plasmas. It is known, based on Ampere’s law, that the produced magnetic field near the coil is stronger. Therefore, the magnitude and curvature of magnetic fields in plasmas become larger when the radius of the coil $R_c$ decreases, which means that the magnetic coil is much closer to the plasmas. Based on these simulation setting, the uniform magnetic field and different magnetic configuration by varying the radius of magnetic coil are presented and discussed.

3.1. The Uniform Magnetic Configuration

The uniform magnetic field applying in the plasma source, which are given as a nominal simulation case to compare with other magnetic configuration cases, are investigated in this part. The 2D distribution contour of magnetic field in plasmas are described in Figure 3. Because of the uniformity, the magnitude of magnetic field is a constant and equal to 150 G. Moreover, the magnetic lines are completely axial. It is noticed that the uniform magnetic configuration is equivalent to the case that the radius of magnetic coil is located at infinity.

Figure 4 shows the absolute values of electromagnetic fields $E_r$ and $B_r$ induced by the antenna when the applied magnetic field is homogeneous. The results reveal that the magnitude of EM fields in vacuum space is trivial except for the location of the RF antenna. However, the EM fields are significantly enhanced in the plasma region and exhibits a periodic distribution in axial direction. This results mention that the main RF energy emitting by the antenna deposits in the plasma region and can be proved by the results of power density in Figure 5. And, the periodic phenomenon is due to the dominant parallel eigenmode of helicon waves in axial direction. According to the dispersion relation of non-uniform helicon plasmas, we have the relation [40,46]

$$\begin{array}{c}\hfill \omega \approx \frac{{\omega }_{ce}{k}_{\Vert }^2{c}^2}{{\omega }_{pe}^2}\end{array}$$

(25)

where c is the speed of light. $k_{\Vert }=2\pi /\lambda$ is the parallel wavenumber, with the axial wavelength $\lambda$. Therefore, the square of axial wavelength is proportional to the strength of the applied magnetic field. In addition, the small wavelength mode (TG mode) coupling to the helicon mode can be observed in the variation of $\left|E_r\right|$ in radial direction. The TG mode mainly concentrates propagating near the boundary of plasmas, whereas the long-wavelength helicon mode propagates in the bulk region of plasmas. In addition, the influence of reflection of boundaries are also observed in Figure 4.

The absorbed power density in plasmas for the uniform magnetic field case is given in Figure 5. The axially periodic distribution for the “hot regions” where the local maximum power density occurs is also observed and it is consistent with the results of wave fields in Figure 4. This further proves that the main parallel eigenmode dominates the wave propagation and power deposition in helicon plasmas. Moreover, the ‘hot regions’ mainly concentrate in the center of plasmas and the power density decreases significantly in the radial direction due to the reduction of plasma density and collision frequency.

3.2. The Non-Uniform Magnetic Configuration

Different configurations of magnetic fields applied in helicon plasmas can significantly affect the wave propagation and power depositions. In this part, four magnetic field distributions, which are formed by varying the position of magnetic coil, are investigated. The spatial wave patterns and power density in plasmas are described and discussed.

Figure 6 shows the 2D contour map of magnetic fields when different radii of magnetic coil are changing. When the radius of magnetic coil is sufficiently large, as $R_c=15$ cm, it produces an almost uniform magnetic field distribution, with the magnetic field lines in the plasma source being nearly parallel to the axis. As $R_c$ decreases, the magnetic coil is closer to the plasma source. The strength of magnetic field is higher in the center and gradually goes down on both sides. The magnetic field lines also become more curved in the center and divergent to both ends.

When the radial of magnetic coil is $R_c=3$ cm, the local maximum magnetic field strength in the center is higher than 1000 G. The wave propagation in space are given in Figure 7. It is shown that the wave propagation is suppressed in a concave region of plasmas where it is near the location of magnetic coil and leads to a dark area in the contour map. This is because the RF wave cannot propagate into plasmas due to a very strong magnetic field in this region. Additionally, it can be clearly seen that the wave propagation follows the magnetic field lines. The curved distributions of wave fields keep consistency with the trends of magnetic field lines. With increasing $R_c$, the curvature of magnetic field lines gradually become small and the wave still propagates in plasmas along the magnetic lines, which shows in Figure 7b–d. The TG mode can be clearly observed near the boundary when the radius of magnetic coil is large. The periodic structure along the axial direction still exists and the wavelength becomes small with increasing the radius of magnetic coil. This is because the strength of magnetic fields reduces when the magnetic coil is far away from the plasma. Moreover, the distribution of wave fields in the results suggests that the reflection of wave occurs in the plasma due to the conducting ends and plasma boundary and it is enhanced by the curved magnetic fields.

Consequently, the power absorbed density $p_{abs}$ shown in Figure 8 also exhibits the trends that follow the magnetic field lines. Moreover, in the high magnetic field region at the axial center in the case of $R_c=3$ cm, a concave “cold zone” can be observed due to the suppression of wave propagation in this region. As $R_c$ increases, the curvature and strength of the magnetic field decrease, making the axial periodic structure more evident. It further confirms that wave propagation and power deposition in plasmas follow the variation of magnetic field lines. When $R_c=0.15$ cm, the magnetic field distribution tends to be uniform. Hence, the resulting EM filed distribution and power density is similar with the uniform case, except the region where the curvature of magnetic lines is enhanced near the plasma boundary.

Table 2. The antenna impedance of different magnetic configurations.

${\mathit{R}}_{\mathit{c}}$ (cm)	Antenna Impedance Z
	$\mathit{Re}\left(\mathit{Z}\right)$($\mathsf{\Omega }$)	$\mathit{Im}\left(\mathit{Z}\right)$($\mathsf{\Omega }$)
3	$0.0466$	$2.1753$
5	$0.0215$	$2.1795$
8	$0.0376$	$2.2046$
15	$0.1007$	$2.1938$
Uniform	$0.1069$	$1.9399$

gives the antenna impedance for different magnetic configurations. The uniform magnetic field case has the maximum antenna resistance and suggests that it leads to the optimal plasma–wave coupling in these configurations. The plasma resistance of the case $R_c=15$ cm is close to the uniform case. This further confirms the results of Figure 8. And, the resistance is small when the magnetic coil is quite near the plasma. For the antenna reactance, it is observed that the magnetic configurations influences the reactance slightly.

4. Conclusions

The wave propagation and power deposition with different magnetic configurations in helicon plasmas have been investigated. The two-dimensional plasma–wave interaction model, which is based on the finite difference method and Yee’s scheme, has been introduced. The magnetic configurations are varied by changing the radial position of the magnetic coil. As suggested by Ampere’ s law, it is shown that the magnetic field in plasmas is stronger and more curved when the magnetic coil is closer to the plasmas.

Therefore, the wave propagation and power absorption in different magnetic configurations including the uniform case have been simulated. It is concluded that the axially periodic distribution of wave pattern due to the eigenmodes of helicon waves is clearly observed and the “hot regions”, which are the local maximum of power density, keeps consistency with the distribution of electromagnetic waves. When the radius of the magnetic coil becomes small, the wave propagation and power density would be curved alone with the magnetic field lines and the axially periodic phenomenon still exits. The reflection of wave due to the conducting ends can also be seen and it is enhanced by the curved magnetic lines. When the magnetic coil is much closer to the plasmas, with the radius $R_c=3$ cm, a saddle type of magnetic configuration, which has much stronger strength of magnetic fields in the center of plasmas, are formed. Thus, a concave dark area in plasmas where the wave cannot propagates and hardly be deposited is shown. This leads to very small plasma resistance and is not beneficial for plasma–antenna coupling.