Field-line resonance structures in Mercury’s multi-ion magnetosphere

We employ the fluid wave simulation model which has been developed by Kim and Lee (2003). Similar to previous wave simulations (Kim et al., 2008), the background magnetic field B₀ and the electron density N_e are assumed to be constants with N_e = 3 cm⁻³, and B₀ = 86 nT at Mercury. The ambient magnetic field, B₀, lies in the z direction and the inhomogeneity is introduced in the x direction. Since the Mercury’s magnetopause is located near 1.4 R _m (Anderson et al., 2011), we assumed a shorter radial distance of 1 R _m than the magnetopause location in x direction, where R _m is the Mercury’s radius. To save computing time, electron mass is assumed to be m_e = m _H /100. We limit ourselves to harmonic variations in the y and z and all waves are proportional to exp(ik _y y+ik _z z), where k _y and k _z are the given y and z direction wavenumbers. For simplicity, k _y is assumed to be 0 and k _z = 2π/L _z , where L _z = 1 R _m , which is similar to the field line length of L _z = 0.93 at L = 1.5 in dipole coordinate. The simulation is driven by imposing an impulse in E _y at X =0 during the interval 0 ≤ τ ≤ 2, where X = x/L _x , τ = t/t_ci, and t_ci = 2π/ω_ci. The simulation is run from τ = 0–60 and the boundaries become perfect reflectors after the impulsive stimulus ends (τ = 2), thus the total energy in the box model will remain constant in time after this interval.

Because H⁺ and He⁺ are major ions at Mercury (Zurbuchen et al., 2008, 2011) and waves near the He²⁺ gy-rofrequency are observed (Boardsen et al., 2009a, b), we adopt an electron-H⁺-He²⁺-He⁺ plasma and the electron density is also assumed to be sum of the ion densities. For simplicity, the He²⁺ density ratio to electron density (ηHe2 = N_He2/N_e) is assumed to be 0.025, however, in order to see the multi-ion effects easily, we assume decreasing He⁺ density ratio in space. Figure 1(a) shows the ion density ratio to electron density (η_ion = N_ion/N_e) profile. We assumed the H⁺ density ratio (ηH) increases from 0 at X = 0 to 0.95 at X = 1 while He⁺ density (ηHe) decreases from 0.95 to 0. Using this profile, we calculate the normalized critical frequencies to ω_ci (Ω = ω/ω_ci), such as cutoffs Ω_L(R) (where ) and ion-ion hybrid (and Alfvén) resonances (Ω_ii and Ω _A ) frequencies. These frequencies are plotted in Fig. 1(b) and shaded regions represent frequency stop-bands where waves are evanescent. Different from the two-ion case predicted by Kim et al. (2008), the IIH resonance modes in between the proton and heaviest ion gyrofrequencies split into the two branches of Ω_ii−1 (where ) and Ω_{ii −2} (where ). Here, Ω_{ii −1} decreases from 1 to 0.527 and Ω_{ii −2} decreases from 0.486 to 0.312. When the impulsive input is excited at X =0, most waves in these resonance frequency ranges encounter the resonance location without cutoffs. In this case, the maximum absorption can increase up to 100% (Lee et al., 2008; Kim et al., 2011). However, below most waves except between the local cutoff of Ω_R = 0.124 and resonance frequency of Ω = 0.143 at X = 0 cannot propagate toward the resonances. Therefore, if the wave power is not enough large to penetrate the wave stop gap, the mode conversion at the Alfvén resonance does not occur.

We store time histories of the electromagnetic fields at each grid point in X during the simulation running time of 0 < τ < 60 and obtain the wave power spectra through the fast Fourier transform. Figure 2 shows the wave spectra of (a) B _x (radial component), which is and (b) B _y (azimuthal component).

In this figure, harmonics of the global cavity modes appear in both components near Ω = 0.14 which is in between Ω _L < Ω < Ω _A , and Ω = 0.32, 0.38, and 0.51 which are larger than the local Ω _R . In contrast with the global cavity wave modes, the continuous spectrum appears only in azimuthal component of B _y . For , there are two continuous bands whose frequencies decrease with increasing X. These continuous spectrum are impulsively excited by the broadband compressional source at X = 0 and corresponds to the IIH resonant conditions of Ω_ii−1 and Ω_ii−2. For , power enhancement of B _y only occurs at Ω = 0.14 near X = 0. This mode is associated with Alfvén resonance. Different to Ω_ii−1 and Ω_ii−2, most waves in the frequency range of Ω _A at X = 0 cannot propagate into the simulation domain as shown in Fig. 1(b) but some wave energy can directly reach Ω _A near X = 0.

Figure 2 also shows that each resonant wave mode branches have different power at different locations. Resonant waves at Ω_ii−1 have strong power in wide range 0 ≤ X ≤ 0.95, while waves at Ω_ii−2 are strong for 0.6 ≤ X ≤ 0.85 but weak for 0 ≤ X < 0.6. Moreover, the Alfvén resonance mode (Ω _A ) occurs only near X ≈ 0. Therefore, single or multiple frequencies of mode-converted wave can be detected at certain locations. For instance, two mode-converted waves can be detected at X = 0.06 (Ω_high = Ω_ii−1 ≈ 0.93 and Ω_low = Ω _A ≈ 0.16) and X = 0.7 (Ω_high = Ω_ii−1 ≈ 0.57 and Ω_low = Ω_ii−2 ≈ 0.44) while a single frequency of mode-converted wave (Ω_high = Ω_ii−1 ≈ 0.8) can be observed at X = 0.2 (these frequencies are marked as open circles in Fig. 2(b)). In order to examine the coupling properties, we plot the time histories of B _x and B _y in Fig. 3, which are obtained using the inverse Fourier transforms. In this figure, the first and second panels are wave time histories of higher (Ω_high) and lower frequencies (Ω_low) of magnetic azimuthal component (B _y ) at (a) X = 0.06, (b) 0.2, and (c) 0.7, respectively. We also plot the wave time histories of the azimuthal (B _y ) and radial (B _x ) components in the third and fourth panels of Fig. 3 that show superposition of two resonant waves of Ω_high and Ω_low. However, because only one resonant wave mode is dominant at X = 0.2, the second panel is remained as blank.

Similar to the previous multi-ion simulation study by Kim et al. (2008), wave azimuthal components with single frequency grow in time as shown in the first and second panels of Fig. 3. When mode-converted waves contain two different frequencies, waves can show modulation of the amplitude in time. For X = 0.06, because frequency ratio of two resonant waves Ω_high/ Ω_low is 6.27 and the amplitude of Ω_low is greater than Ω_high, wave amplitude beating is not significantly appeared in the third panel. Different to case of X = 0.06, for X = 0.7 in Fig. 3(c), Ω_high/Ω_low = 1.31 and the wave amplitudes are similar for both frequencies, therefore, the amplitude beating in time is clearly shown in the third panel of Fig. 3(c). In this case, when two wave amplitudes are assumed to be the same and constant in time, the beat period T_beat can be approximated to be 1/(ΔΩ) ≈ 7.7, which is consistent with the simulation results. In contrast to the increase of the azimuthal component (B _y ), the radial component (B _x ) damps for two mode-converted waves (fourth panels in Figs. 3(a) and (c)) and for a single mode (Fig. 3(b)). When there are two mode-converted waves appeared at the same location in Fig. 3(a) and (c), B _x also show wave amplitude beating with damping in time.

In this paper, we perform a wave simulation in three-ion plasmas to consider multiple heavy ion effects at Mercury. The simulation results show that several resonant waves between the ion gyrofrequencies can occur at certain locations and show wave amplitude beating in time histories.

Mercury’s magnetosphere contains heavier (e.g., O⁺, K⁺, Na⁺) and lighter ions (e.g., He⁺, He²⁺) and MESSENGER spacecraft have recently detected ULF wave events near and (Boardsen et al., 2009a, b, 2012). The observed magnetic component of transverse waves tends to be strongly linearly polarized and oriented approximately perpendicular to the estimated field gradient (which is plasma inhomogeneity). This is consistent with wave simulation results: In Figs. 2 and 3, the B _y component which is perpendicular to the plasma inhomogeneity is dominant at the mode-converted waves. Previous two-ion simulations demonstrated the IIH resonance occurs in H⁺-Na⁺ plasmas but did not include He⁺ or He²⁺ ions. In this paper, we show how small amount He²⁺ change the FLRs structure. The simulation results suggest that several resonant waves between the ion gyrofrequencies can occur at a certain location and show wave amplitude beating in time histories. Therefore, it could possible to observe two or three different resonant frequencies in Mercury’s magnetosphere. In addition, because the IIH resonance is the result of ion-ion effects and those frequencies are affected only by the relative ion density ratio rather than the absolute number density, the wave frequency could be used to estimate the local heavy ion density if a spacecraft detects multiple resonances (Kim et al., 2008).

In this study, a cold plasma model is adopted. However, because of the small dimensions of Mercury’s magnetosphere (for instance, magnetopause is located near 1.4 R _m ~ 3400 km and the large gyro radii of ions ~100–1000 km, kinetic effects can play an important role for the generation and propagation of ULF waves (Glassmeier et al., 2004; Glassmeier and Espley, 2006; Slavin et al., 2009). When the kinetic effects are included, the compres-sional wave can be converted into the short wavelength ion Bernstein and/or ion cyclotron waves at the IIH resonance. These mode converted waves can be strongly damped in the vicinity of the mode-conversion surface via electron Landau damping or damped by ions at the Doppler broadened ion cyclotron resonances (e.g., Phillips et al., 1995; Intrator et al., 1986; Jaeger et al., 2003, 2006). Therefore, although the cold plasma wave simulation in this study shows the resonant absorption characteristics near the IIH and Alfvén resonance clearly, more detailed investigations on mode-converted waves including kinetic effects at Mercury’s multi-ion plasmas are necessary.