Dust-Acoustic Nonlinear Waves in a Nanoparticle Fraction of Ultracold (2K) Multicomponent Dusty Plasma

Abstract

The nonlinear dust-acoustic instability in the condensed submicron fraction of dust particles in the low-pressure glow discharge at ultra-low temperatures is experimentally and theoretically investigated. The main discharge parameters are estimated on the basisof the dust-acoustic wave analysis. In particular, the temperature and density of ions, as well as the Debye radius, are determined. It is shown that the ion temperature exceeds the temperature of the neutral gas. The drift characteristics of all plasma fractions are estimated. The reasons for the instability excitation are considered.

1. Introduction

Dusty plasma is a plasma containing fractions of charged microparticles along with electrons and ions. Such plasmas are common in space and have many technological applications [1]. The main methods of dust fraction formation are injection of dust particles in plasma, chemical reactions in plasma, and ion sputtering of various materials in plasma [1]. In rare and poorly studied cases, several mechanisms are involved simultaneously [2]. The presence of low-frequency wave modes is one of the features of dusty plasma. For example, the frequencies of well-understood dust-acoustic waves are in the range of 0.1–100 Hz.

In recent years, studies of cryogenic dusty plasma have become relevant, which is due to various fundamental and technological aspects [3,4,5,6,7,8,9,10]. Notably, the study of ultra-low-temperature discharges is an independent physical problem [11,12,13]. Among the open questions, one can single out the gas-to-ion temperature ratio, the magnitude of the screening scale, etc. For example, dusty plasma in a glow discharge at liquid nitrogen and helium temperatures was investigated in [4]. It was assumed that the temperatures of ions and neutral gas are equal. In this case, the ion Debye radius is of the order of one micron at a gas temperature of 4.2 K, pressure p = 4 Pa, and the ratio of the electric field to the density of a neutral gas E/N~10 Td. The same results are presented in a study by [6]. On the other hand, in [9], by studying the dust interparticle distance, it was found that the screening radius exceeds the Debye ionic radius by an order of magnitude assuming that the ionic and atomic temperatures are equal. Possible explanations for this phenomenon can be a nonlinear screening of a particle charge [14,15], overheating of ions in the discharge plasma [16,17,18,19,20,21], etc. Nevertheless, this issue remains open. The ion parameters were measured within a wide range of temperature and for different values of the E/N ratio using mass spectroscopy methods [16,17,18]. It was shown that in cryogenic discharges, at E/N > 10 Td, the effective temperature of the ions can exceed the temperature of the parent gas by an order of magnitude. These results are in good accordance with the conclusions of recent theoretical [19,20] and experimental [21] works. A similar result, but for dusty plasma, was obtained in [22] both experimentally and in the framework of the Monte Carlo method. It also shows that the main ions in a cryogenic discharge are atomic helium He⁺ ions if E/N exceeds 10 Td. Thus, the determination of the Debye radius and ion temperature in the cryogenic discharge remains an unsolved problem.

In this paper, the nonlinear dust-acoustic instability (with nonlinear waves excitation) in a multicomponent plasma at the buffer gas temperature of ~2 K (pressure p = 5 Pa, E/N~10 Td) is studied in detail. The plasma consisted of electrons, helium ions, micron-sized particles injected into the discharge, and condensed nanoparticles. As mentioned above, the properties of such plasma configuration are poorly understood. We found only one publication [2], which describes the radio-frequency RF discharge plasma containing both injected and condensed (grown) dust fractions. Ion sputtering of the surface of the injected dust particles led to the formation of a condensed fraction. Recently, such multicomponent DC discharge plasma was investigated in [23,24,25]. In [23,24], wave processes were observed; however, they were not studied in detail. The proposed research is a logical continuation of works [23,24]. Dust-acoustic waves can be an effective tool for plasma diagnostics because their main parameters can be accurately measured. In turn, the wave parameters are related to the plasma parameters by known relations. In this research, wave analysis is carried out in the framework of a simple hydrodynamic model. The screening length, ion temperature, drift velocities, and some other discharge parameters are determined independently.

2. Results

2.1. Plasma Parameters

The wave process observed in the experiment (Section 4) is rather complex, and its detailed description is beyond the scope of this work. However, our estimates allow us to reasonably describe the observed phenomena.

The process begins with an estimate of the Debye radius—λ_D; this problem at ultralow temperatures was discussed in [4,9,22]. For λ_D, we can write

$${\lambda }_D^{-2}={\lambda }_{De}^{-2}+{\lambda }_{Di}^{-2}$$

(1)

where λ_De,i = (ε₀T_e,i/e²n_e,i)^1/2 are the Debye radii for electrons and ions, respectively. The width of the observed soliton-like dust density profiles is L ≈ 100 µm (see Section 4). As follows from theoretical work [26], large-amplitude dust-acoustic soliton widths are about 1–3 λ_D. The width of the soliton was meant the width of the dust density profile. This parameter is easy to measure experimentally; thus, it is analogous to “standard candles” in astrophysics. In our case, Δ₊ ≈ 100 μm, therefore, we have λ_D ≈ 30–100 μm, which agrees well with [9,22] and significantly exceeds the estimates presented in [4,6]. We set λ_D = 30 μm;that is, we assume that the width of the wave crest density profile contains at least three Debye radii (upper bound from the study by [26]). From Equation (1) and data in

Table 1. The main parameters of the plasma.

Plasma Parameters	Value
Neutralgas pressure.	PHe = 5 Pa
Discharge current	I = 35 ± 15 μA
Discharge voltage	U = 3.21 kV
Neutralgas density	nHe = 1.8 × 1023 m−3
Temperature of the neutral gas (the walls of the discharge tube)	Ta ≈ 2 K
Radius of the first fraction dust particles	rd1 ≈ 1–5 μm
Radius of the second fraction dust particles	rd2 ≈ 15–35 nm
Mass density of the first fraction dust particles	ρ1 = 7200 kg/m3
Mass density of the second fraction dust particles	ρ2 = 1100–1500 kg/m3
Electric field strength	E ≈ 2000 V/m
Reduced electric field strength	E/N ≈ 10 Td

, it follows that λ_D corresponds to the ion Debye radius λ_D = λ_Di, which indicates that the ion drift is subsonic. With supersonic drift, we have λ_D = λ_De (see, for example, [27]). In this case, by setting T_e ≈ 1 eV (

Table 2. Calculated plasma parameters.

Plasma Parameters	Value
Density of the first fraction particles	nd1 = 3.0 × 105 cm−3
Density of the second fraction particles	nd2 = 3.7 × 107 cm−3
Charge of the first fraction dust	Z1 ≈ 500
Charge of the second fraction dust	Z2 = 2
Electron density	ne ≈ 1 × 107 cm−3
Ion density	ni ≈ 2.3 × 108 cm−3
Electron temperature	Te ≈ 104 K
Ion temperature	Ti ≈ 45 K
Electron Debye length	λDe = 2.2 × 10−1 cm
Ion Debye length	λDi = 3.0 × 10−3 cm
Ion free path	li = 5.5 μm
Gravitational force for the first fraction particles	FG1 = 1.6 × 10−13 N
Gravitational force for the second fraction particles	FG2 = 2.0 × 10−18 N
Electric force for the first fraction particles	FE1 = 1.6 × 10−13 N
Electric force for the second fraction particles	FE2 = 3.2 × 10−16 N
Ion drag force for the first fraction particles	Fid1 = 3.0 × 10−14 N
Ion drag force for the second fraction particles	Fid2 = 4.9 × 10−18 N
Neutral drag force for the first fraction particles at u0d1 = 5 × 10−3 m/s	Fnd1 = 1.6 × 10−15 N
Neutral drag force for the second fraction particles at u0d2 = 0.2 m/s, γ = 1 + π/8	Fnd2 = 2.2 × 10−16 N
Electron thermal velocity	υTe = 4 × 107 cm/s
Ion thermal velocity	υTi = 3 × 104 cm/s

), we have λ_De >> λ_Di; therefore, the width of the nonlinear wave profiles should be much larger than the observed value.

Having λ_D one can estimate the initial density of dust particles of the second fraction—n_0d2. The density n_0d2 is large enough for the effective scattering of laser radiation on the wave profile; however, in the unperturbed state, the condensed particles weakly scatter light. We assume that the particle charge is proportional to the radius as well as that Z = 10³ for r = 0.5 μm. Then, we obtain Z₂ = 5 for r = r_d2. According to [22,28,29] when the discharge temperature decreases to cryogenic values, Z decreases by 2–3 times, compared with normal conditions; thus, finally, we have Z₂ = 1–2. For such small charges, it can be assumed that the interparticle distance is equal to the Debye radius L₂ ≈ λ_Di ≈ 30 μm, then n_0d2 = λ_Di⁻³ = 3.7 × 10⁷ cm⁻³. Further, from the quasi-neutrality condition n_0i − n_0e − Z₁·n_0d1 − Z₂·n_0d2 = 0, we obtain n_0i = n_0e + Z₁·n_0d1 + Z₂·n_0d2. Taking into account the data in Table 2, we can obtain n_0i = 2.3 × 10⁸ cm⁻³. Next, from (1), we obtain the estimate for the ion temperature T_i = 45 K. Thus, analysis of the wave process implies T_i >> T_a at E/N ≈ 10 Td, which confirms the results of [16,17,18,19,20,22], obtained by other methods. The value of n_0e can be approximately estimated from the expression for the discharge current I/S ≈ j = en_0eu_0e, where S = πR² is the cross-sectional area of the discharge tube, j is the current density, and u_0e is the drift velocity of electrons. For various glow discharge strata in different experiments u_0e/υ_Te~0.1–1, where υ_Te = (T_e/m_e)^1/2 is an electron thermal velocity. Then, setting I = 50 μA (the upper estimate for the discharge current in our experiment), we obtain n_0e~I/πR²eAυ_Te~10⁶–10⁷ cm⁻³, with A = u_0e/υ_Te = 0.1–1. The value of n_0e on the discharge axis may be several times higher than the obtained estimate due to the radial inhomogeneity of the current. Finally, we estimate the mean free path of ions by the formula l_i = (n_aσ_in)⁻¹ [30], where σ_in is the cross section for the scattering of ions on helium atoms. In accordance with the data listed in Table IIa from [18] σ_in = 10⁻¹⁴ cm², with T_a = 4.35 K (there are no data at T_a = 2 K) and E/N = 10 Td, then l_i = 5.5 μm. Thus, λ_D > l_i (the ions are collisional). The calculated data are provided in Table 2, according to which the forces acting on the dust particles need to be calculated.

2.2. The Main Forces

The ion drift velocity, in accordance with the data listed in Table IIa from [18], is u_0d2 = 5.2·10³ cm/s at E/N = 10 Td, considering that the main ions are He⁺ [22]. It is worth noting that the type of ion is not so important for the estimates, since the mobilities of the He⁺, He₂⁺, and He₃⁺ ions are not very different [31,32]. Assuming that T_i = 45 K, we can obtain an estimate for the ion thermal velocity υ_Ti = (T_i/m_i)^1/2 = 3.05 × 10⁴ cm/s, hence u_0d2 << υ_Ti.

In the vertical direction, the main forces to be considered are the gravitational force F_G, the electric force due to a vertical discharge electric field F_E, the neutral drag force F_nd, and ion drag force F_id. The first three forces are described by simple expressions as follows:

$$F_G=\frac{4}{3}\pi r_d^3{\rho }_{d}g,$$

(2)

$$F_E=-e{Z}_{a}E,$$

(3)

$$F_{nd}=\frac{8}{3}\sqrt{2\pi }{r}_d^2{m}_n{n}_n\gamma {\upsilon }_{Tn}{\upsilon }_{da}\equiv m_d{\nu }_{nd}{\upsilon }_{da}$$

(4)

where r_d and ρ_d are the radius and mass density of dust particles, a = 1, 2 for particles of the first and second fractions, respectively, g = 981 cm/s², m_n, n_n, and ${\upsilon }_{Tn}=\sqrt{T_n/m_n}$ are the mass, density, and thermal velocity of the neutral gas atoms, respectively, υ_da is the speed of dust particles relative to a neutral gas, ν_nd is dust-neutral collision frequency, γ is a coefficient on the order of unity that depends on the exact processes proceeding on the particle surface, and γ takes values from 1 to 1 + π/8 [1].

Ion drag forces were calculated in accordance with [33] (Equation (11)). The values of the main forces are provided in Table 2 (taking into account Table 1 data).

As can be seen from Table 2, for large particles (fraction «1»), gravity is balanced by electrostatic force. Large particles are visible, so their motion parameters can be easily determined. The large particles’ speed is small, so the neutral drag force, as well as the ion drag force, can be neglected for them. Particles of fraction 2 are invisible, and only the modulation of their density caused by waves is available for observations. However, this is sufficient to determine the important parameters of particle motion. From Table 2, it follows that F_E ≈ F_nd2 >> F_G~F_id2, i.e., the electric force can be balanced only by the neutral drag force in the presence of a drift u_0d2 ≈ 20 cm/s, directed upwards. Taking into account the data of Table 1 and Table 2 and putting Z₂ = 2, we obtain u_0d2/C_d2 = 4.7, where $C_{d2}=\sqrt{\frac{Z_2^2{n}_{0d2}{T}_e{T}_i}{m_{d2\left(n_{0e}{T}_i+n_{0i}{T}_e\right)}}}$ is the dust-acoustic speed for fraction 2 [34,35]. Thus, the drift of fraction 2 is supersonic. Under these conditions, the phase state “liquid” or “gas” is most likely for fraction 2. The soliton-like wave crests move downward relative to the particles of the second fraction with a speed equal to or greater than u_0d2. At the same time, in a fixed coordinate system, the wave speed is V₀ ≤ 1 cm/s. In the first approximation, waves can be considered as standing in a fixed coordinate system because |V₀/u_0d2| << 1. A similar situation for micron size particles is described in [36]. Knowing the basic parameters of the dusty plasma, we turn to the calculation of the parameters of the nonlinear waves.

2.3. Hydrodynamic Wave Model

We assume that in the unperturbed state, the dust particles of the second fraction are affected only by the electric force F_E2 and the neutral drag force F_nd2 (due to the particle drift directed upward). Other forces are negligible (Table 2). The waves have almost no effect on the parameters of the first fraction, so we assume that N_d1 = n_d1/n_0d1 = 1. The dynamics of dust particles can be described by a system of one-dimensional hydrodynamic equations. In the frame of the second fraction—namely, in the frame moving upward with the speed u_0d2, the equations take the following form:

$$\frac{\partial {\upsilon }_{d2}}{\partial t}+{\upsilon }_{d2}\frac{\partial {\upsilon }_{d2}}{\partial z}=-\frac{e{Z}_2}{m_{d2}}\left(E+E^{\prime }\right)-{\nu }_{nd2}\left({\upsilon }_{d2}-u_{0d2}\right)$$

(5)

$$\frac{\partial n_{d2}}{\partial t}+\frac{\partial n_{d2}{\upsilon }_{d2}}{\partial z}=0$$

(6)

where υ_d2, n_d2, m_d2 are the velocity, density, and mass of the second fraction particles, $E^{\prime }=-\partial \varphi /\partial z$ is the electrostatic field of the wave, φ is potential, and ν_nd2 is the dust-neutral collisions frequency, which is easy to find from Equation (4); all other parameters are listed in Table 1 and Table 2. Considering that ${\displaystyle \sum F_0}=0$, where F₀ is zero-order forces (i.e., ${\nu }_{nd2}{u}_{0d2}-e{Z}_{2}E/m_{d2}=0$), Equation (5) can be rewritten as

$$\frac{\partial {\upsilon }_{d2}}{\partial t}+{\upsilon }_{d2}\frac{\partial {\upsilon }_{d2}}{\partial z}=-\frac{e{Z}_2}{m_{d2}}{E}^{\prime }-{\nu }_{nd2}{\upsilon }_{d2}.$$

(7)

In the first approximation, considering ${\nu }_{nd2}{\upsilon }_{d2}=0$, in the stationary case, according to [34], Equations (6) and (7) can be converted to the following form:

$$N_{d2}(\Phi )=\frac{n_{d2}}{n_{0d2}}=\frac{M}{\sqrt{M^2+2Z_2\Phi }},$$

(8)

where Φ = eφ/C_d2²m_d2 is the normalized potential, M = V/C_d2 is the Mach number, and V is the steady-state wave velocity in the moving frame. The density of electrons and ions can be described by the Boltzmann distribution as follows:

$$N_e(\Phi )=\frac{n_e}{n_{0e}}=\exp \left(\frac{e\phi }{T_e}\right)\equiv \exp \left(\frac{Z_2\Phi }{{\delta }_1+\beta {\delta }_2}\right),$$

(9)

$$N_i(\Phi )=\frac{n_i}{n_{0i}}=\exp \left(-\frac{e\phi }{T_i}\right)\equiv \exp \left(-\frac{Z_2\Phi \beta }{{\delta }_1+\beta {\delta }_2}\right),$$

(10)

where $\beta =T_e/T_i$, ${\delta }_1=n_{0e}/Z_2{n}_{0d2}$, ${\delta }_2=n_{0i}/Z_2{n}_{0d2}$. Equations (8)–(10) are connected with the stationary Poisson equation.

$$\frac{d^2\Phi }{d{S}^2}=\frac{1}{Z_2}\left({\delta }_1{N}_e-{\delta }_2{N}_i+{\delta }_3{N}_{d2}\right),$$

(11)

where $S=\left(z-Vt\right)/{\lambda }_{Di}$, ${\delta }_3=n_{0d1}/Z_2{n}_{0d2}$. The quasi-neutrality condition yields Δ₁ − Δ₂ + Δ₃ + 1 = 0.

Equation (11) can have solutions in the form of a soliton, nonlinear (cnoidal) wave, or linear wave, depending on the initial conditions. To describe large-amplitude soliton-like dust-acoustic waves, we use the soliton solution of Equation (11). Such solutions of Equation (11) are well studied (see, for example, [1]). Figure 1 shows the numerically obtained soliton profiles at M = 1.55 and M = 1.7. Other parameters of the model are β = 222, Δ₁ = 0.135, Δ₂ = 3.16, Δ₃ = 2.03 (Table 2). When integrating, the Runge–Kutta algorithm is used, the boundary conditions are as follows: Φ(−10) = −5 × 10⁻⁴ and Φ’(−10) = 10⁻⁵ at M = 1.7; Φ(−10) = −8·10⁻⁴ and Φ’(−10) = 10⁻⁵ at M = 1.55.

From Figure 1, it can be seen that the wave width is Δφ ≈ 3–5 λ_Di, and the width of the particle density profile is ΔN_d2 ≈ 1 λ_Di. Our simple “cold” plasma model does not take into account the pressure of the dust fraction. However, in more realistic and complex models, the width of solitons can increase by several times (see, for example, the “warm” plasma model in [1]). Therefore, we assumed ΔN_d2 = 3λ_Di in the above reasoning. The density of dust in the center of the soliton is increased up to 4–10 times. With such an increase in density, the soliton-like profiles can be easily observed in the optical range due to light scattering.

The electric field inside the soliton is perturbed by the value of ΔE’ < 0.5 V/cm (Figure 1c). Due to the fulfillment of the inequality ΔE’ << E, the nonlinear waves do not have a noticeable effect on the first fraction particles, which is confirmed experimentally. The wave velocity is V = 7 cm/s, which corresponds in order of magnitude to u_0d2, but this is not enough for the observed slow wave motion downward in a fixed coordinate system. For a more accurate description of the experiment, additional research is needed. We return to this issue in the discussion.

3. Discussion

The reasons for the instability excitation can be ions (electrons) drift and ion drag force [37,38,39,40,41,42], dust charge perturbation [43,44,45], neutral drag force caused by the dust drift relative to a stationary neutral gas [46]. The third reason, in our opinion, dominates in the case under consideration. Indeed, first, the instability conditions obtained in [46] are satisfied, such as n_0e/n_0i << 1 and E/N > E_crit/N, where E_crit is the minimum value of the electric field sufficient to excite the instability. Secondly, the nonlinear waves are plane, occupying almost the entire radial cross section of the tube, far beyond the boundaries of the large particles cloud. The neutral drag force can be considered constant in the radial direction. The electric forces and the ion drag force should have a radial gradient, as evinced by the shape of the large particles cloud. If the forces of F_E2 and F_id2 caused the instability, the solitons would have a lenticular shape. The radial homogeneity of solitons can also be explained by the small charge of condensed particles (Z₂ ~ 1) since the discharge boundaries do not affect them significantly. A detailed analysis of the causes of instability is certainly of interest and will be carried out in the future.

In conclusion, we highlight the finding that continuous ion sputtering of the cone surface should lead to a loss of its mass Δm, which can be estimated by the formula Δm = m_d2·n_0d2·π·R²·u_0d2·Δt. During the experiment Δt ≈ 1.2·10³ s, the mass loss can be neglected, as Δm < 10⁻⁶ kg.

4. Experiment

The experiments were carried out in the Janis SVT-200 cryostat, which allows operation within the temperature range from 1.5 to 300 K [25]. A DC glow discharge was created in helium gas inside a vertical glass tube with an inner diameter of 2 cm. The distance between electrodes was equal to 60 cm. The experimental setup is shown schematically in Figure 2a. Polydisperse CeO₂ particles (0.1–200 μm) were used to form a dust cloud in the lowest stratum of the discharge.

The pressure was measured using a Granville-Phillips 275 convectron, while the temperature was determined by a LakeShore 335 temperature controller connected to the TPK-1.5/60-22 semiconductor sensor calibrated within the working range of 1.5–60 K and attached to the discharge tube wall at the level of the lowest stratum. The waves were recorded using a high-speed digital camera (up to 1000 fps), a “laser knife” (with the cross section of 0.22 × 6 mm, 85 mW at 532 nm) was used for illumination of the dust cloud.

The operating temperatures were achieved by reducing the discharge current to 35 ± 15 μA at a voltage of 3.2 kV and a pressure of 5 Pa. In such a low-power mode, the temperature gradient between the anode and cathode did not exceed 2–3 K. As shown in Figure 2b, the initial shape of the dust cloud is close to spherical, the mean interparticle distance was ≈170 μm. At the same time, the particles formed the structure of the liquid type, containing randomly moving fast and slow particles. Fast particles formed intense vortex flows on the periphery of the cloud.

Approximately 20 min after the discharge had been generated, we detected scattering of laser radiation on moving local inhomogeneities as shown in Figure 3. At about the same time, the average distance between micron size particles decreased to ≈120 μm. It is clear from Figure 3, that there are no visible separate particles in the inhomogeneities. These facts indicate the appearance of a new submicron dust fraction, which was formed in the plasma during the experiment. The geometry of moving inhomogeneities indicates the excitation of dust-acoustic instability involving submicron particles. In what follows, subscripts 1 and 2 refer to injected (micron) and condensed (submicron) dust particles, respectively. As shown in [24], the appearance of fraction 2 was due to ionic sputtering of the dielectric cone material (8 on Figure 2a). The cone was used to focus the flow of electrons on the axis of the discharge tube. A flow of ions was also focused in the region of the cone and sputtered its surface. This hypothesis was confirmed during an additional experiment carried out at room temperature, which revealed an intense glow near the cone outlet. It is well known that polymer surfaces are easily sputtered in strata of the DC glow discharge [47,48]. Therefore, we can expect rather an efficient sputtering of the cone material because it contains acrylic polymer [24]. The condensed fraction properties were studied in detail in a few studies [23,24].

The shape of the condensed particles is close to spherical, and the diameter does not exceed 75 nm with a large dispersion. The appearance of the condensed fraction led to some changes in the parameters of the initial dust cloud. For example, as mentioned above, the density of large particles increased (probably due to a decrease in the charge of large particles with the appearance of an additional submicron dust fraction and, therefore, due to competition for electrons and ions). A detailed study of the effect of fraction 2 on the evolution of the cloud is beyond the scope of this work. Notably, some parameters of the discharge slowly changed during the experiment. For example, the temperature of liquid helium varied in the range from 1.6 to 2.17 K. The main parameters of the discharge are listed in Table 1.

Considering the waves in fraction 2, as can be seen from Figure 3, fraction 2 fills a wider part of the tube than fraction 1. The waves were investigated in the same axial region where the particles of fraction 1 levitated. The observed wave process was rather complicated. However, some of its features can be considered. We use the one-dimensional approximation since the waves can be considered planes. Once the axis OZ is directed vertically downward (from the anode to the cathode), it can be inferred that the wave perturbation of the submicron particle (fraction 2) density cannot be described by a harmonic function (Δn_d2 ≠ exp(iωt + ikz)). Indeed, the width of the compression regions, Δ₊, is noticeably smaller than the width of the rarefaction regions, Δ₋; therefore, the waves are nonlinear. In addition, Δ₊ ≈ 100 μm for all cases, while Δ₋ depended on z and t. Such behavior is characteristic of strongly nonlinear waves. The amplitudes of the individual wave crests were especially large (bright bands on Figure 3). These crests had soliton-like dust density profiles. The speed of the nonlinear waves was different in different parts of the dust structure but did not exceed 1 cm/s (V ≤ 1 cm/s). According to our estimates (see below), the dust-acoustic velocity for the submicron dust fraction should significantly exceed the observed wave velocity (C_d2 >> V). Such a low velocity of nonlinear dust-acoustic waves can be explained either within the framework of the model [49] (where the self-consistent charge of particles was taken into account), within the framework of research [50] (where dust compression waves in electrorheological dusty plasma were studied), or by the presence of submicron particle drift (second fraction particles).Under the considered experimental conditions, the drift hypothesis appears to be the most reasonable. It is important that the drift velocity of the second fraction particles should be approximately equal to the phase velocity of the waves. The effect of the observed waves on the particles of the first fraction was insignificant. Consequently, the electric field of the discharge significantly exceeded the electric field of the waves. We use standard models of a glow discharge dusty plasma for the theoretical interpretation of the experiment. The hydrodynamic model is used to calculate the parameters of the waves.

5. Conclusions

The nonlinear dust-acoustic instability excited in the condensed submicron fraction of dust in the four-component dusty plasma of the DC glow discharge at the gas temperature of ~2 K was studied in detail. The plasma contained injected CeO₂ particles of micron size and condensed nanoparticles, as well as electron and ion background. The nanoscale fraction was aggregated from products of ion sputtering of the polymer cone, which performed the function of focusing the electron stream. To analyze the observed waves, a simple hydrodynamic model was used, which made it possible to estimate important discharge parameters: λ_Di, T_i, particle drift velocities, etc. Independently of other authors [16,17,18,19,20,21,22], it was shown that the ions in the discharge are overheated in the presence of a significant electric field. The screening length was determined by the ions (λ_D ≈ λ_Di). The obtained estimates for λ_Di are in good agreement with the results of [9] and are several times higher than the estimates of [4,6]. This discrepancy is due to the fact that T_i = T_a was assumed in [4,6], while our analysis resulted in T_i >> T_a. Estimates of other discharge parameters—namely, E/N, l_i, are consistent with [4].

Analysis of the acting forces showed that the second (invisible) fraction of dust drifts upward at the speed exceeding the dust-acoustic speed several times. The calculated electric field of strongly nonlinear waves proved to be an order of magnitude smaller than the field of discharge, which explains the absence of a relationship between waves and micron particles of the first fraction. The reasons for the excitation of the instability were briefly considered. The most likely cause is the neutral drag force, arising in the presence of significant drift of the second fraction particles. The linear stage of such instability was theoretically considered in [46].

In accordance with the assumptions made, the wave velocity V must be either equal to or slightly higher than the drift velocity u_0d2 (i.e.,V ≥ u_0d2). In our estimates, the soliton velocity and the drift velocity coincide only in order of magnitude; what is more, V < u_0d2. One can achieve the fulfillment of the condition V = u_0d2 in two ways. First, by increasing the velocity of the nonlinear waves to M ~ 4–5. Secondly, by reducing the drift velocity u_0d2. Future research will help clarify the values of V and u_0d2.