# Low Temperature Conductivity inn-Type Noncompensated Silicon below Insulator-Metal Transition

Authors: A. L. Danilyuk; A. G. Trafimenko; A. K. Fedotov; I. A. Svito; S. L. Prischepa
Journal: Advances in Condensed Matter Physics
 (2017)

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## Abstract

We investigate the transport properties ofn-type noncompensated silicon below the insulator-metal transition by measuring the electrical and magnetoresistances as a function of temperature T for the interval 2–300 K. Experimental data are analyzed taking into account possible simple activation and hopping mechanisms of the conductivity in the presence of two impurity bands, the upper and lower Hubbard bands (UHB and LHB, resp.). We demonstrate that the charge transport develops with decreasing temperature from the band edge activation (110–300 K) to the simple activation with much less energy associated with the activation motion in the UHB (28–90 K). Then, the Mott-type variable range hopping (VRH) with spin dependent hops occurs (5–20 K). Finally, the VRH in the presence of the hard gap (HG) between LHB and UHB (2–4 K) takes place. We propose the empiric expression for the low T density of states which involves both the UHB and LHB and takes into account the crossover from the HG regime to the Mott-type VRH with increasing temperature. This allows us to fit the low T experimental data with high accuracy.


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## Body

## 1. Introduction

Interest in studies of conductivity mechanisms in semiconductor materials, including traditional doped semiconductors near the metal-insulator transition (MIT), does not stop currently [1, 2]. This is due to both the fundamental problems of electron transport in the vicinity of such transition and applied aspects related to the development of highly sensitive sensors of magnetic and electric fields. In particular, it is not yet fully understood mechanisms of low temperature electrical conductivity in doped semiconductors involving multiply charged localized states, mechanisms of positive and negative magnetoresistance (MR), as well as mechanisms of localization and peculiarities of the energy band structures of impurity and localized states. Due to the above the detailed investigation of the conductivity of doped semiconductors near the MIT in a wide temperature range, influence on it the magnetic field is still relevant. Actually, the MIT in three dimensional (3D) system occurs when the Mott criterion Nc1/3aB≈0.25 is satisfied, where Nc is the critical concentration of the localized states for the MIT and aB is the effective Bohr radius of an insulated defect center [3]. The validity of this criterion was confirmed in various experiments [4–6]. However, some ambiguity in correct understanding of the temperature dependence of the conductivity and MR near the critical concentration of the localized sites still does present. The main reason for this is related to the competition between various types of hopping conductivity, mechanisms of weak localization, percolation and metallic and/or impurity bands (Hubbard bands) conductivity. Therefore, a series of crossovers could be observed between different types of conductivity in a wide temperature range. This inevitably leads to the need for their very careful consideration during the processing of the experimental data. In particular, with decreasing temperature, the crossover from band edge activation (ϵ1) to hopping (ϵ3) conductivity is observed in doped semiconductors [6].Hopping is one of the most likely mechanisms that determines the overall conductivity on the insulating side of the MIT. Among various types of hops, the variable range hopping (VRH) is one of the most relevant. The VRH mechanism, in turn, could be classified as the Mott mechanism, for which the density of states (DOS) on the Fermi level is constant,g(EF)=const [3] and the Efros-Shklovskii (ES) mechanism, which implies the soft Coulomb gap (CG), g(E)~|E-EF|2 [7, 8]. From a practical point of view, at a constant T, the Mott-type VRH occurs when the doping concentration Nd is far less than the Nc value, Nd<0.5Nc, and one can neglect the Coulomb interaction [9]. The ES mechanism, in turn, dominates when Nd>0.6Nc and the CG has to be taken into account [10, 11]. From the literature a few models of crossovers between the Mott and ES hopping are known quite [12–14].The temperature dependence of the resistivity for both mechanisms is described by the well-known expression(1)ρT=ρ0exp⁡ThTp,where ρ0 is the preexponential factor and Th and p are the characteristic temperature and exponent, respectively. Last two quantities depend on the mechanism of hopping. In particular, for 3D systems and for the Mott mechanism, the exponent p=1/4, while for the ES VRH p=1/2 [3, 6]. The exponent p can be obtained from the experiment.Actually, the concept of hopping between disorder-induced localized electronic states near the MIT is a universal feature of disordered Mott systems. In particular, it was successfully applied to describe transport in amorphous/nanocrystalline silicon hybrids [15], semiconductor nanocrystals [16], ruthenate [17], carbon nanotube fibers [18], as well as transport of single (few) donors in a silicon nanoscale transistor [19, 20]. Known models of crossover between different types of VRH are characterized by two different approaches to the calculation of the exponent p from (1). The first approach is based on the analysis of the percolation problem [12, 13, 21], while the second deals with the optimization of the exponent p using the interpolation expression for the DOS [14, 22, 23].In general, the percolation approach can be applied when the spatial correlation length for the random potential is much larger than the phase coherence length [24, 25]. This is a very powerful tool for the description of charge transport in disordered systems with localized states, which occurs due to the electron hops from one site to another [26, 27]. It should be noted that the percolation theory was applied to explain the properties not only of doped semiconductors, but also granular metals [28], manganese oxides [29], quantum Hall plateau transistors [30], high-Tc cuprates [31], and so forth. Moreover, the percolation phase was directly observed in vanadium dioxide close to the Mott transition by means of nanoscale X-ray imaging [32].The second approach is less stringent and leads to a noticeable overestimation of the width of the crossover region. General description of the crossover from the Mott to ES VRH on the basis of rather complex multivariable integral equation, which cannot be solved analytically and needs rather difficult numerical analysis, was proposed in [13]. In [14, 22, 23] the procedure based on the optimization of the exponent in the expression for the hopping probability and using the interpolation expression for the DOS, g(E)~|E-EF|n (here n is integer which is equal to 0 for the Mott mechanism and to 2 for the ES VRH), has been proposed. This approach leads to quite simple analytical expressions but, as we mentioned above, is less stringent than the percolation task.In addition to the crossover from the Mott to ES VRH, there is another, less studied lowT crossover, between VRH and a simple activation dependence (SAD) [33]. For the SAD the temperature behavior of resistivity is described by (1) but with the exponent p=1. Actually, the SAD may occur for different reasons. At high T it could indicate the nearest neighbor hopping (NNH) [23, 34–36], or a band conductivity [6, 37]. At low T, however, the probability of both the NNH and band conductivity becomes negligibly small. Thus, the SAD at low T is usually associated with a hard gap (HG) in the DOS [38], that is, in a certain energy range g|E|≈0. One of the reason of the HG in doped semiconductors could be the Coulomb interaction [39, 40]. The manifestation of these mechanisms depends not only on the concentration of the main impurities Nd, but also on the degree of compensation of the semiconductor, K.Traditional Mott, ES, and NNH mechanisms are based on hops to the empty impurity centers. Therefore, the availability of sufficient number of empty donor cites is important for such kind of hops inn-type semiconductor. At low temperatures, this can only be achieved by compensation of semiconductor. Arisen due to compensation charged donors and acceptors create dispersion of the donor energy levels due to their chaotic potential. This dispersion exceeds significantly the exponentially small splitting of levels of neighbor donors caused by the overlap of the wave functions. The characteristic feature of noncompensated semiconductor (K≪1) is the rapid decrease of the empty (ionized) donors with decreasing temperature. In weakly compensated semiconductors, in a limited range of concentrations (close to the MIT), in addition to the band and hopping conductivity another activation mechanism develops in the temperature dependence of conductivity, ϵ2 conductivity. This mechanism exhibits in the intermediate between band and hopping conductivity temperature interval [41–43]. It is believed that the ϵ2 conductivity involves migration of electrons on the single occupied neutral donors (D- states). They have large radius and, consequently, at the intermediate impurity concentrations are strongly overlapped. The result is a wide band of D- states. This band is an analogue of the upper Hubbard band (UHB), formed in a disordered systems [6]. The decrease in donor impurity concentration leads to a strong narrowing of a D- band. On the other hand, in the absence of compensation, when ϵ3 conductivity is zero, there are most favorable conditions for ϵ2 conductivity; that is, the concentration of neutral donors is the highest. The increase of the compensation improves significantly conditions for the ϵ3 conductivity and worsens the ϵ2 conductivity.Electron hopping (ϵ3 conductivity) may occur not only on free localized but also on occupied sites via the spin dependent transport [44]. In fact, for doped semiconductors, the spin degree of freedom could play a significant role in the electron hops. If, for example, the width of the distribution function of the energies of the localized sites overcomes the Coulomb repulsion between electrons, double occupancy of the site becomes possible, as was first argued by Kurobe and Kamimura [44]. In this case, two types of hops contribute to the transport. The first occurs between singly occupied (SO) and unoccupied (UO) sites, while the second type of hops involves doubly occupied sites (DO) with opposite electron spins. As a result, the spin dependent charge transport could occur in this case. The UO site is considered as a singly ionized site with the elementary charge +1e. Consequently, SO site has charge 0e, and DO site has charge −1e. Developing of a quantitative theory of the ϵ2 conductivity faced with very great difficulties. The main difficulty is that in this concentration range the overlap of the wave functions play a role comparable to the Coulomb interaction of electrons with impurities and with each other. In addition, disorder in the distribution of impurities significantly complicates the analysis of experimental data. Therefore, many problems related to the interpretation of the experimental data for doped semiconductors, in which ϵ2 conductivity is observed, are still unclear. In this regard, for doped semiconductors with a low degree of compensation, in which ϵ2 conductivity is manifested, the study of the mechanisms of low temperature conductivity and crossover between ϵ2 and hopping conductivity is a topical problem.Therefore, the correct interpretation of the experimentalρ(T) data measured in a wide T range can be significantly hampered, because, in order to compare the experimental values of the parameters with the calculated ones, it is important to identify and properly describe the transport mechanisms in different temperature intervals.In this work we performed a thorough investigation of the low temperature (2K<T<90K) conductivity of n-type noncompensated silicon close to the MIT taking into account possible VRH, SAD, and spin dependent mechanisms. We show that above 30 K the conductivity is of the activation type and is carried out in the UHB, while in the T range 5–25 K the Mott-type VRH dominates and is accompanied by the spin dependent charge transport. Below 5 K the crossover from the VRH to SAD occurs. We demonstrate that the reason for the SAD in this T range is the HG in the DOS. We developed a model of this crossover based on the percolation task, using the expression for DOS, which takes into account the evolution of the DOS from the HG at T<5K to the Mott-type at T>5K. This approach allowed us to fit the experimental ρ(T) dependence with high accuracy.


## 2. Samples and Experimental Details

Single crystallinen-type Si (100) grown by Czochralski method and doped with Sb was used in this work. Samples of rectangular shape with a width of 1 mm and a thickness of 0.5 mm were covered with 6 indium contacts as electric probes using ultrasonic soldering. Two contacts were for current supply, 2 were for Hall measurements, and, finally, last 2 contacts were for voltage measurements. All contacts were ohmic in the whole studied temperature range which was proved by the linear current-voltage characteristics. A dc current of 10 μA generated by multimeter Keithley 6430 was used to bias the sample during the resistivity measurements and to measure the voltage drop down to 5 μV. For low resistivity samples we used the two-channel nanovoltmeter Keithley 2182A. Samples were inserted into the cryogen free measuring system (Cryogenic Ltd., London) with the superconducting magnet. The system allowed performing measurements in the T range between 2 and 300 K in magnetic fields up to H=80 kOe. Lakeshore controller allowed 0.1 K/min sweeping rate of temperature during the ρ versus T measurements and stabilizing temperature with the accuracy of ±0.005K during the sweep of the magnetic field or current-voltage characteristics acquisition. Semiconducting GaAs thermometer was calibrated with an accuracy better than 0.1%. On the basis of measurements of the T dependence of the Hall effect the Sb concentration was estimated as Nd=1×1018cm-3, which is 3 times less than the critical Mott concentration for Sb in Si [45, 46]. Therefore, our samples are on the insulating side of the MIT. Actually, a series of samples cut from different Si wafers belonging to the same technological set of fabrication were measured. All the data are in nice agreement with each other. Here we present typical results obtained on the investigated samples.


## 3. Results

In Figure1 we show the resistivity versus temperature measured in the range 2–300 K at zero magnetic field and at the maximum applied field of 80 kOe. The strong change in ρ (4 orders of magnitude) is evident. The ρ(T) dependence at H=0 is linear in the Arrhenius coordinates in the temperature range 28–300 K, as is clearly seen from the inset to Figure 1. Actually, in this temperature interval there are two significantly different activation energies: ϵ1≈10.35meV for the T range 110–300 K and ϵ2≈1.73meV for 28–90 K. Resistivity in the first T range is increased by two times, while in the second interval it is increased by only 1.2 times.Figure 1
Temperature dependence of the resistivity atH=0 (black circles) and H=80 kOe (red circles) in the range 2–300 K. Inset: resistivity versus T-1 (symbols). Experimental data are explained by two activation energies, ϵ1≈10.35meV for 110–300 K and ϵ2≈1.73meV for 28–90 K.Below 20 K atH=0 the SAD is changed to the Mott-type VRH. In Figure 2(a) we show the ln⁡ρ(T-1/4) data for the temperature interval 5–20 K (red color). The obtained in these coordinates linear dependence unambiguously proves the Mott-type VRH. At T<5K the Mott-type VRH is no longer valid and crossover to the SAD with the exponent p=1 and activation energy ϵ4≈1.48meV occurs (blue color).Figure 2
(a)ln⁡ρ versus T-1/4 (red symbols), left and bottom red axis. ln⁡ρ versus T-1 (blue symbols), right and upper blue axis. Solid lines are the result of the best linear fit in these coordinates. Data are for H=0. (b) ln⁡ρ versus T-1/4 (red symbols), left and bottom red axis. ln⁡ρ versus T-1 (blue symbols), right and upper blue axis. Solid blue line is the result of the best linear fit in these coordinates. Dashed black line is tangent to the experimental data. Data are for H=80 kOe.
(a) (b)Data atH=80 kOe below 20 K reveal similar features as for zero field. However, only on the basis of the exponent p in (1) we cannot successfully fit experimental data in the T range 5–20 K. As it follows from Figure 2(b), red symbols, exponent p=1/4 is not suitable to describe the experimental dependence. Other reasonable exponents in (1) also do not give satisfactory agreement with the experiment. Nevertheless, at lower T we can identify interval, where the exponent p=1 is valid, see blue color in Figure 2(b). It turns out that low T SAD still exists even at high magnetic field.For a more accurate identification of the observed lowT SAD in Figure 3 by symbols we plot ln⁡ρ versus T-p dependence at zero field for two different p values, 1/2 (blue color, corresponds to SE VRH) and 1 (red color, corresponds to SAD). Solid lines in Figure 3 correspond to the result of the best linear fit. It follows from Figure 3 that exponent p=1/2 gives worse agreement with the experiment. The same analysis for data measured in the presence of the magnetic field leads to similar result, namely, presence of SAD below T=4K.Figure 3
ln ⁡ ρ versus T-1 (red symbols), left and bottom red axis. ln⁡ρ versus T-1/2 (blue symbols), right and upper blue axis. Solid lines are the result of the best linear fit in these coordinates. Data are for H=0.


## 4. Discussion

### 4.1. Qualitative Analysis

The obtained experimental data revealed the following. In theT interval 110–300 K the conventional band edge activation caused by the transition from the Fermi level located in the tail of the lower Hubbard band (LHB) to the conduction band of silicon (the ϵ1 conductivity [6]) takes place.Another simple activation mechanism is manifested in the temperature dependence of the resistivity in the interval 28–90 K (ϵ2 conductivity). It is believed that the ϵ2 conductivity is associated with the activation motion of electrons along singly occupied neutral donors and corresponds to the states in the upper Hubbard band (UHB) [5, 6, 20, 37]. In this temperature interval the characteristic value of the thermal energy kBT is greater than the activation energy ϵ2 and all states are delocalized. Moreover, only slight increase in the resistivity as the temperature decreases or magnetic field increases indicates the extended UHB.In theT range 5–20 K the Mott-type hopping ϵ3 conductivity is observed in the absence of the magnetic field. Finally, in the temperature interval 2–4 K again the SAD with the activation energy ϵ4≈1.48meV is realized. At first glance, this is a reentrance of the previously observed within the temperature interval 28–90 K SAD with the activation energy ϵ2≈1.73meV. On the other hand, for the range 2–4 K the activation energy ϵ4 is greater than the energy of thermal fluctuations, ϵ4≈(3–7)kBT. It means that all states are localized; that is, the charge transport is hopping-like, but the mechanism of hops is different from usual VRH.The reentrance of the SAD after VRH is well known for some dilute magnetic [38, 47, 48] and classical doped semiconductors, like Si:B [33] and Si:As [49] with doping concentration less than Nc, and for amorphous compounds like In/InOx [50] or amorphous silicon after implantation of Au or Si ions [51]. For all these materials evidences of ϵ2 conductivity before VRH were never reported. Typically, as T decreases first one observes the NNH, which is characterized by the exponent p=1, then the VRH followed by SAD, again with the exponent p=1. Moreover, for dilute magnetic semiconductors and for Si:B strong magnetic field removes the reentrance effect. But for In/InOx the reentrance effect is insensitive to the magnetic field [50]. It is worth mentioning that for the electronic Si:As semiconductor the influence of the magnetic field on the reentrance effect was not studied. In our system, the reentrance effect in the presence of the magnetic field still does exist, see Figure 2(b). Moreover, the peculiar feature of the appearance of the SAD reentrance in our case is that not only the VRH, but also the ϵ2 conductivity (not NNH) preceded it.Thus, the performed brief qualitative analysis of the data disclosed that, in the range 28–90 K, the influence of both the temperature and magnetic field on the resistivity is very low. This indicates that the electron transport in this temperature range has apparently a band character, is realized in the relatively wide UHB and states are delocalized. In the range 5–20 K the electron transport is transformed to the hoppingϵ3 conductivity. With further T decrease, below 4 K, the Mott-type VRH is transformed into more complicated hopping mechanism which formally corresponds to the SAD, but now states are localized.Actually, the SAD at lowT indicates the formation of the HG in the DOS [38]. The energy ϵ4 characterizes the width of the HG, where the DOS is equal or close to zero. The magnetic field does not suppress the SAD. The reason of the HG appearance is hidden. In order to understand better the nature of the reentrance effect and the origin of the HG, we need to perform the quantitative analysis of the data.


### 4.2. Quantitative Analysis

#### 4.2.1. Spin Dependent Hopping

For theT range 5–20 K the resistivity is described according to the Mott law, (1) [3, 6], in which Th=TM and p=1/4. Here TM=βMgMaM3kB-1 is the Mott parameter, βM=21.2±1.2 is the numerical factor, gM=const is DOS at the Fermi level, aM is the localization length of the states around the Fermi level. We calculated the gM and aM values analyzing the experimental data ρ(T) at zero magnetic field in the Mott coordinates (ρ-T-1/4) and applying the evaluation expressions [3, 6, 52, 53](2)gM=Nd2kBTMTvM31/4,aM=βM1/3kBTMgM1/3,where TvM is the temperature of the onset of the Mott-type VRH. Equation (2) gives approximate values of gM and aM. Note that on the basis of (1) and (2) the obtained gM and aM values must be temperature independent. On the other hand, the MR data allow checking whether these quantities are really T independent. Indeed, within the standard approach of the Mott-type VRH the positive MR which is usually related to the contraction of the wave function of the localized states in magnetic field is expressed as [6](3)ln⁡ρHρ0=t3aM4lH4TMT3/4~H2,where numerical factor t3=5/2016, lH=ħ/eμ0H is the magnetic length, and ρ(0) is the zero field resistivity.On the basis of (3), knowing TM, H, and MR, we calculated the aM values at different T. Moreover, knowing already aM, the value of gM from results of the MR measurements can be calculated using the expression for the Mott parameter TM.The results of calculations of hopping parameters according to theρ(T) dependence and MR data at different T are summarized in Table 1. The Mott parameter was evaluated from (1) as TM=1.524×104 K. The temperature TvM was obtained from the ρ(T) data as TvM≈20K [54].Table 1
Parameters of the Mott-type VRH obtained within two different approaches.
Parameter ρ ( T ) data MR data a M, nm 6.6 6.0–8.5 g M, eV-1×cm-3 5.408 × 1 0 19 4.7 × 1 0 19It follows from Table1 that the obtained within two different approaches aM and gM values are in good agreement with each other.The surprising result, which we obtained, analyzing theaM values from the MR measurements, is their T dependence. This result for H=80 kOe is presented in Figure 4, from which it follows that the aM(T) function is not constant. In particular, for the range 5–20 K the aM values decrease from 8.3 to 6.0 nm. This means that the standard model of positive MR, which takes into account only the contraction of the electronic wave function in magnetic field and leads to the temperature independent localization length, cannot explain the obtained aM(T) result.Figure 4
Temperature dependence of the localization lengthaM. Data are for H=80 kOe.In Figure5 we show the dependencies of ln(ρ(H)/ρ(0)) versus H2 in the temperature range 4–20 K together with the results of the best fit procedure according to (3). It is seen that the ln(ρ(H)/ρ(0))~H2 law in the considered temperature range is valid only at H<(50–60) kOe. From the results presented in Figures 2(b), 4 and 5 it follows that the transport mechanism at low T becomes more complicated than conventional Mott-type VRH. To clarify the hopping mechanism, we examine other possible types of hops, to the occupied localized sites, which are accompanied by a spin flip [44].Figure 5
l n ρ ( H ) / ρ ( 0 ) versus H2 at different temperatures (symbols). Lines correspond to the results of the best linear fit in these coordinates.The MR for a system of sites occupied by more than one electron was considered in detail some time ago by Kurobe and Kamimura [44], Matveev et al. [55], Meir [56], and Demishev and Pronin [57]. In particular, if the Coulomb repulsion between two electrons is smaller than the width of the Hubbard bands, 2 types of hops, on unoccupied (SO → UO, DO → UO) and occupied (SO → SO, DO → SO) sites are relevant. All these possibilities are shown in Figure 6, where we schematically draw the energy diagrams for each type of hops.Figure 6
Possible electron hops considered for low temperature conductivity. For more details, see the text.In general case, spin independent hops to unoccupied sites could be characterized by the localization lengtha1 and DOS g1, while spin dependent hops to occupied sites could be described, in turn, by a2 and g2. The quantity g1 is assigned to the DOS in the LHB, and g2 corresponds to the DOS in the UHB. The relation between g1 and g2 as well as between a1 and a2 is still an open question and different assumptions were put forward to simplify the task. Typically, it is assumed that the localization length for the DO state is more than for the SO, a2>a1 [44]. In [56] the possibility of spin dependent transport was discussed considering inequality between two densities of states and two localization lengths. From a practical point of view, it seems problematic to separate these quantities in the framework of such general approach. It is necessary to introduce additional assumptions associated with the density of states or the localization length.In [55] the spin polarized mechanism of MR was investigated in terms of the approach proposed by Kurobe and Kamimura [44]. It was supposed that both the states, UO and SO, are characterized by the same localization length, a1=a2=a, while densities of states differ from each other, g1≠g2.We failed in the attempts to fit the experimental data of Figure2(b) applying theoretical approaches of Refs. [55, 56]. We believe this is due to the fact that applied theoretical approaches do not take into account all complexity of the transport mechanisms. Further we investigate this problem in detail within the approach proposed by Demishev et al. [57, 58]. Authors [57], following Kurobe and Kamimura [44], considered only intrasite correlations and neglect the long range Coulomb repulsion. On the basis of [57] it is possible to determine which type of conductivity under the external magnetic field dominates: spin dependent or spin independent. In particular, the modified expression for the MR, which takes into account both types of hops, was deduced [58]:(4)ln⁡ρHρ0=TMT1/414AeffTμ0μBHkBT2,where(5)AeffT=A+4bTTM3/2.In (5) parameters A=(g2a23-g1a13)/(g2a23+g1a13) and b=t3a24(e2kB2TM2/ħ2μB2). According to Demishev et al. [58], parameter A depends on the probability of hops, which involve both D0 and D- states, and is determined by the degree of polarization of the spin part of the wave function of these states in the magnetic field. Parameter b is determined by the contribution of the mechanism of the wave function contraction to the MR that acts on both types of hops.Therefore, on the basis of the temperature dependenceAeff(T) it is possible to conclude which type of contribution determines the MR in the hopping region. If the spin dependent mechanism dominates, then Aeff(T)=const. Otherwise, Aeff(T) tends to 0 at T→0 according to the law T3/2. When both types of contributions are comparable, the dependence of Aeff(T) is expected to be more complicated, it does not tend to 0 at T→0 [57, 58].In Figure7 we plot the Aeff(T) dependence obtained from the experiment applying (4). Data are for H=80 kOe. As can be seen, the Aeff(T) dependence has two distinct regions. In one of them, in the T range 5–11 K, the Aeff value is temperature independent and the results of the fitting procedure give A=0.47±0.03, b=0 (blue line in Figure 7). Therefore, in this T range the spin dependent hopping prevails. In addition, the relation between DOS for two different types of hops can be estimated via the quantity kg=g2a23/g1a13. In this case kg≈2.8.Figure 7
Evaluated temperature dependenceAeff(T) at H=80 kOe (symbols). Lines are plotted according to (5). Inset: the temperature dependence of the calculated coefficient kg.In theT range 11–20 K the linear approximation Aeff(T)~T3/2 explains well the experimental data (red line in Figure 7), but Aeff does not tend to 0 at T→0. Consequently, the obtained result proves the absence of the dominant role of the spin independent hops in this temperature interval. From the fitting procedure we obtained coefficients A=0.29 and b=0.96×104. That gives a2=5.5nm and a1≈a2/4=1.38nm. The parameter kg in this case depends on T. The obtained overall kg(T) dependence is shown in the inset to Figure 7. From kg values we may estimate the g1/g2 relation, which is equal to 21.3 for T range 5–10 K and to 10.7 at T=20K.


#### 4.2.2. Gap in the DOS

Thus, the performed estimations and calculations showed that, in the temperature range 5–20 K, on the whole, the Mott-type VRH is realized. Nevertheless, we obtained that two types of hops, traditional hops on UO sites and spin dependent hops on SO sites, have to be taken into account. Therefore, one needs to consider two localization lengths and two DOS. On the other hand, previously introducedg1 and g2 values are essentially model parameters that do not give information about the influence of the DOS on the mechanism of hopping conductivity. It should also be noted that neither approach [55] nor work [57] gives any information about the gap between two Hubbard bands.Generally speaking, the origin of the gap could be twofold. First, it could be due to the CG; second, the HG between lower and upper Hubbard bands could be the reason. The soft CG at the energy minimum does not have a characteristic shelf,g(E)~|E-EF|2, while the true gap has the shelf of the width Δ. Moreover, the presence of the soft CG leads to the exponent p=1/2, which we did not observe.Below we propose the model expression for the DOS and evaluate the influence of the shape and parameters of the proposed model DOS on theT dependence of the hopping resistivity, which, in turn, is characterized by the critical values of the exponent ξ(T)=ln⁡[ρ(T)/ρ0] [21]. The relation between the critical exponent ξ(T) and the exponent p is ξ(T)~(Th/T)p. Estimations are performed within the model of the low temperature crossover VRH-SAD.To model this crossover let us consider the problem of the charge flow in the lattice of impurity atoms. In the theory of hopping conductivity, problems of charge flow in the system of random nodes, chaotically distributed in space, play the most important role. In this case the average number of nodes in a unit volume is supposed to be given and equal to the concentration of the impuritiesNd. The average distance between nodes is rd=(3/4πNd)1/3. For such a lattice, the percolation radius rc is found from the condition of the connectivity of two and more nodes which form an infinite cluster [6], so that the value of rc depends only on the nodes concentration Nd. Typically, the dimensionless threshold value Bc is used, having a meaning of the average number of bonds per node. In the 3D case [6](6)Bc=4π3rc3Nd.For random lattice theBc value is typically determined numerically and varied in the range 2.65–2.76 [6]. Consequently, the percolation radius is given by rc=(0.865±0.015)Nd-1/3. In this case rc is always larger than rd. In particular, in our case rc=8.64nm>rd=6.2nm. In other words, the symmetry of the lattice is irrelevant and only the number of sites inside radius rc determines the transport mechanism.On the basis of the aforementioned estimations, we then developed a model of the VRH-SAD crossover; this model is based on a simplified procedure for solving the percolation problem using the empiric expression for the DOS valid for both types of the temperature dependent hopping. We start from the following expression for the dimensionless concentration of sites:(7)Nξ=2∫0Emaxrmax3gEdE,which satisfies the condition of connectivity for the exponent of the hopping resistivity less than a certain value ξmin [6, 13]. Here, Emax and rmax are maximal values of the energy and intersite spacing, respectively, which still allow the connectivity. The dimensionless concentration N(ξ) in (7) is determined as a product of the concentration of sites with the energy E<Emax and the volume of these sites. This procedure for the temperature dependent DOS is not completely rigorous and the connectivity condition should be considered for each energy value separately, which leads to the complicated integral equation [13]. Here we will follow the procedure described in [21], which simplifies significantly the calculations.Values ofrmax and Emax are specified in the percolation theory by the relations [6] (see also Equation (4.30) in [59])(8)rmax=a2ξ2,Emax=kBTξ.Substituting (8) into (7) and equating N(ξ) to 2Bc, we get the following expression:(9)2Bc=a2ξ23∫0kBTξgEdE,which allows calculating the T dependence of ξ and compare it with the experimental data ρ(T). The above procedure was carried out using three different types of expressions for the DOS.First, we used the interpolation expression proposed in [22, 23]. Thus, the change of the DOS from constant value for the VRH Mott-type to the DOS g(E)~|E-EF|n, where for the SAD n>2, was taken into account. In this case the DOS models, presumably, only the CG-like, but with steeper dependence on the energy. According to [22], the crossover at different exponent values of p=(n+1)/(n+4) could be described applying the following expression for the DOS:(10)gE,T=g0E-EF/Esgn1+E-EF/Esgn.Parameter Esg depends on the exponent n and, when it is fixed, is constant. Parameter g0 is a constant related to gM. For the case n=2, (10) coincides with the expression used in [14] for the description of the crossover from the Mott to ES VRH.Substituting (10) into (9) and using the previously obtained values, a2 and Esg=ϵ4, we calculated the dependencies ξ(T) for the fixed values of the exponent n in (10), which were compared with the experimental data ln⁡[ρ(T)/ρ0]. We obtained that theoretical results coincide with the experimental data only varying values of the exponent n with temperature [60]. For example, in the interval 5–25 K the agreement is observed only for n=0 (the Mott-type VRH), while for 2–5 K to obtain the agreement between theory and experiment much greater value of n, n>6, is required, Figure 8. Calculations of the p(T) dependencies for different n values using the relation p=-∂log⁡ξ(T)/∂log⁡T=-T/ξ(T)∂ξ(T)/∂T [21] and evaluated the ξ(T) dependence showed that, to achieve the value of the exponent p, close to unity, it is necessary to significantly increase n, that is, the variable n needs to tend to infinity, Figure 9. At n=0 expressions for the crossover give the exact value p=1/4. Thus, (10) for the DOS in this case has limited application because, firstly, it requires a change of the exponent n with T and, secondly, the value of n, which provides the exponent p→1, tends to infinity.Figure 8
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (10) ξ(T) dependencies. Red and blue lines correspond to n=0 and 15, respectively.Figure 9
Temperature dependencies of the exponentp for different n values. From top to down, n = 200, 100, 50, 15, 5, and 2, respectively.In the second attempt, we take into account the gap smearing withT increase [61],(11)gE,T=g0γT+1-γTE-EFnΔT/2n+E-EFn.The parameter γ describes a “residual” DOS at the Fermi level and Δ is the width of the gap.Substitution of the modified expression (11) to (9) allowed comparing the value of the critical exponent ξ with the experimental data and finding the temperature dependencies γ(T) and Δ(T), which adequately describe the experiment. This result is presented in Figure 10 for two n values, n=2.5 and 3.0.Figure 10
γ ( T ) and Δ(T) dependencies as obtained using (11) for fitting the ρ(T) data. Calculated curves correspond to the range of the exponent n=2.5–3.0. The γ values are in arbitrary units. The Δ values are normalized to ϵ4.It follows from Figure10 that γ varies in the range 0.1–1. At T>10K, γ→1, and the first constant term in (11) dominates. This corresponds to the Mott-type VRH. When γ=1 (i.e., at T>15K), the result becomes insensitive to the Δ values. At low temperatures γ≪1 and the main contribution is due to the term |E-EF|n. The parameter Δ, which characterizes the width of the gap, decreases with increasing temperature, which is in contradiction with the result usually reported [61, 62]. Thus, the result of the fitting procedure found that the agreement with the experiment is achieved only taking into account the filling of the gap states between the Hubbard bands and suggested the narrowing of the gap with increasing temperature, during the crossover to the Mott-type DOS. In addition, insensitivity of the model to the value of n at n>3 has been revealed. Therefore, it is obvious that there is a need to modify the formula for the DOS, in order to reflect the tendency both for smearing of the gap and its growth with increasing temperature. These are characteristic features of the HG. Moreover, the integer exponent n should be temperature independent.Within these assumptions the reasonable approximation for the DOS is of the following empiric type:(12)gE,T=g0αTw4E+βTw2E+γT×exp-wEσT4,where w(E)=E-EF/0.5ϵ4 and α, β, γ, and σ are phenomenologicaltemperature dependent coefficients.The shape of the DOS in this case depends onT according to the α, β, γ and σ versus T dependencies. In particular, the first term corresponds to the HG, the second one is for the soft gap, the parameter γ is responsible for the filling of the HG with T and σ is responsible for the width of the Hubbard band. Indeed, the exponential term serves for smoothing of the overall DOS and for modelling of the Hubbard bands, in particular, their width. In other words, empirical expression (12) allows reproducing not only the HG, its filling, but also the width of the Hubbard bands. In this work, we assumed the identical widths of the upper and lower Hubbard bands. Widening of the UHB was taken into account by filling the HG. Function (12) reflects the change of the DOS with T, from HG at low T (with the dip between Hubbard bands) to the constant DOS close to the Fermi level at high T. This was enough for the experimental data interpretation. The fitting procedure was as for previous expressions for the DOS; that is, we substitute (12) into (9) and looked for such ξ values which adequately describe the ρ(T) data. The result of the fitting procedure is shown in Figure 11. It follows that we were able to describe experimental data with very high accuracy in the T range 2–20 K. On the basis of the obtained ξ(T) dependence it is possible to evaluate rmax, the maximal hopping length which still allows the connectivity. For the range 5–20 K we get rmax=17.6–22.0nm, while for the interval 2–4 K the result is rmax=27.5–38.5nm.Figure 11
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (12) ξ(T) dependencies.On the basis of the obtained model parameters, it is possible to reproduce the DOS at different temperatures. This result is shown in Figure12. As it follows, the DOS evolves from HG at 2 K to almost filled states between Hubbard bands at 15 K. At that the widening of the Hubbard bands also occurs (within our approach, UHB and LHB are symmetrical; actually, they may differ in width and height, but this issue requires additional investigation and is outside the objectives of this work). Parameters of the model are changed as follows. The parameter α, which corresponds to the HG width is almost constant and is equal to 1 for the whole T range. The parameter β (characteristic of the soft gap) is almost constant with temperature, β=-0.7 except the region 15–21 K, where β=-2. The parameter γ, which is responsible for the HG filling, is changed from 0 at 2 K to 6 at 21 K. Finally, the parameter σ, the characteristic of the width of the Hubbard bands, also increases with temperature, from 1.5 to 2.3.Figure 12
DOS at different temperatures as obtained from the experimental data within the proposed model (see (12)).At the end of this section we summarize that, the conductivity in theT interval 5–20 K is of the hopping-type. On the whole, it obeys the Mott law and is determined by two type of hops: to UO neutral and to SO impurity sites. In the range 5–11 K the contribution of the spin dependent hopping dominates. This is valid also in the range 2–4 K. Simulations of the DOS revealed that in this T range hops are regulated by the HG. The presence of nonsmeared HG between Hubbard bands in the T range 2–4 K together with the spin dependent hops in the UHB provides reentrance of the SAD.The latter provides a nonlinearity of the current-voltage characteristics at small bias voltage, which leads to negative differential resistance at electrical fields smaller than 1 V/cm [63]. It is unlikely that this effect may be due to the ES VRH, for which the delocalization occurs at significantly higher electrical fields.


## 4.1. Qualitative Analysis

The obtained experimental data revealed the following. In theT interval 110–300 K the conventional band edge activation caused by the transition from the Fermi level located in the tail of the lower Hubbard band (LHB) to the conduction band of silicon (the ϵ1 conductivity [6]) takes place.Another simple activation mechanism is manifested in the temperature dependence of the resistivity in the interval 28–90 K (ϵ2 conductivity). It is believed that the ϵ2 conductivity is associated with the activation motion of electrons along singly occupied neutral donors and corresponds to the states in the upper Hubbard band (UHB) [5, 6, 20, 37]. In this temperature interval the characteristic value of the thermal energy kBT is greater than the activation energy ϵ2 and all states are delocalized. Moreover, only slight increase in the resistivity as the temperature decreases or magnetic field increases indicates the extended UHB.In theT range 5–20 K the Mott-type hopping ϵ3 conductivity is observed in the absence of the magnetic field. Finally, in the temperature interval 2–4 K again the SAD with the activation energy ϵ4≈1.48meV is realized. At first glance, this is a reentrance of the previously observed within the temperature interval 28–90 K SAD with the activation energy ϵ2≈1.73meV. On the other hand, for the range 2–4 K the activation energy ϵ4 is greater than the energy of thermal fluctuations, ϵ4≈(3–7)kBT. It means that all states are localized; that is, the charge transport is hopping-like, but the mechanism of hops is different from usual VRH.The reentrance of the SAD after VRH is well known for some dilute magnetic [38, 47, 48] and classical doped semiconductors, like Si:B [33] and Si:As [49] with doping concentration less than Nc, and for amorphous compounds like In/InOx [50] or amorphous silicon after implantation of Au or Si ions [51]. For all these materials evidences of ϵ2 conductivity before VRH were never reported. Typically, as T decreases first one observes the NNH, which is characterized by the exponent p=1, then the VRH followed by SAD, again with the exponent p=1. Moreover, for dilute magnetic semiconductors and for Si:B strong magnetic field removes the reentrance effect. But for In/InOx the reentrance effect is insensitive to the magnetic field [50]. It is worth mentioning that for the electronic Si:As semiconductor the influence of the magnetic field on the reentrance effect was not studied. In our system, the reentrance effect in the presence of the magnetic field still does exist, see Figure 2(b). Moreover, the peculiar feature of the appearance of the SAD reentrance in our case is that not only the VRH, but also the ϵ2 conductivity (not NNH) preceded it.Thus, the performed brief qualitative analysis of the data disclosed that, in the range 28–90 K, the influence of both the temperature and magnetic field on the resistivity is very low. This indicates that the electron transport in this temperature range has apparently a band character, is realized in the relatively wide UHB and states are delocalized. In the range 5–20 K the electron transport is transformed to the hoppingϵ3 conductivity. With further T decrease, below 4 K, the Mott-type VRH is transformed into more complicated hopping mechanism which formally corresponds to the SAD, but now states are localized.Actually, the SAD at lowT indicates the formation of the HG in the DOS [38]. The energy ϵ4 characterizes the width of the HG, where the DOS is equal or close to zero. The magnetic field does not suppress the SAD. The reason of the HG appearance is hidden. In order to understand better the nature of the reentrance effect and the origin of the HG, we need to perform the quantitative analysis of the data.


## 4.2. Quantitative Analysis

### 4.2.1. Spin Dependent Hopping

For theT range 5–20 K the resistivity is described according to the Mott law, (1) [3, 6], in which Th=TM and p=1/4. Here TM=βMgMaM3kB-1 is the Mott parameter, βM=21.2±1.2 is the numerical factor, gM=const is DOS at the Fermi level, aM is the localization length of the states around the Fermi level. We calculated the gM and aM values analyzing the experimental data ρ(T) at zero magnetic field in the Mott coordinates (ρ-T-1/4) and applying the evaluation expressions [3, 6, 52, 53](2)gM=Nd2kBTMTvM31/4,aM=βM1/3kBTMgM1/3,where TvM is the temperature of the onset of the Mott-type VRH. Equation (2) gives approximate values of gM and aM. Note that on the basis of (1) and (2) the obtained gM and aM values must be temperature independent. On the other hand, the MR data allow checking whether these quantities are really T independent. Indeed, within the standard approach of the Mott-type VRH the positive MR which is usually related to the contraction of the wave function of the localized states in magnetic field is expressed as [6](3)ln⁡ρHρ0=t3aM4lH4TMT3/4~H2,where numerical factor t3=5/2016, lH=ħ/eμ0H is the magnetic length, and ρ(0) is the zero field resistivity.On the basis of (3), knowing TM, H, and MR, we calculated the aM values at different T. Moreover, knowing already aM, the value of gM from results of the MR measurements can be calculated using the expression for the Mott parameter TM.The results of calculations of hopping parameters according to theρ(T) dependence and MR data at different T are summarized in Table 1. The Mott parameter was evaluated from (1) as TM=1.524×104 K. The temperature TvM was obtained from the ρ(T) data as TvM≈20K [54].Table 1
Parameters of the Mott-type VRH obtained within two different approaches.
Parameter ρ ( T ) data MR data a M, nm 6.6 6.0–8.5 g M, eV-1×cm-3 5.408 × 1 0 19 4.7 × 1 0 19It follows from Table1 that the obtained within two different approaches aM and gM values are in good agreement with each other.The surprising result, which we obtained, analyzing theaM values from the MR measurements, is their T dependence. This result for H=80 kOe is presented in Figure 4, from which it follows that the aM(T) function is not constant. In particular, for the range 5–20 K the aM values decrease from 8.3 to 6.0 nm. This means that the standard model of positive MR, which takes into account only the contraction of the electronic wave function in magnetic field and leads to the temperature independent localization length, cannot explain the obtained aM(T) result.Figure 4
Temperature dependence of the localization lengthaM. Data are for H=80 kOe.In Figure5 we show the dependencies of ln(ρ(H)/ρ(0)) versus H2 in the temperature range 4–20 K together with the results of the best fit procedure according to (3). It is seen that the ln(ρ(H)/ρ(0))~H2 law in the considered temperature range is valid only at H<(50–60) kOe. From the results presented in Figures 2(b), 4 and 5 it follows that the transport mechanism at low T becomes more complicated than conventional Mott-type VRH. To clarify the hopping mechanism, we examine other possible types of hops, to the occupied localized sites, which are accompanied by a spin flip [44].Figure 5
l n ρ ( H ) / ρ ( 0 ) versus H2 at different temperatures (symbols). Lines correspond to the results of the best linear fit in these coordinates.The MR for a system of sites occupied by more than one electron was considered in detail some time ago by Kurobe and Kamimura [44], Matveev et al. [55], Meir [56], and Demishev and Pronin [57]. In particular, if the Coulomb repulsion between two electrons is smaller than the width of the Hubbard bands, 2 types of hops, on unoccupied (SO → UO, DO → UO) and occupied (SO → SO, DO → SO) sites are relevant. All these possibilities are shown in Figure 6, where we schematically draw the energy diagrams for each type of hops.Figure 6
Possible electron hops considered for low temperature conductivity. For more details, see the text.In general case, spin independent hops to unoccupied sites could be characterized by the localization lengtha1 and DOS g1, while spin dependent hops to occupied sites could be described, in turn, by a2 and g2. The quantity g1 is assigned to the DOS in the LHB, and g2 corresponds to the DOS in the UHB. The relation between g1 and g2 as well as between a1 and a2 is still an open question and different assumptions were put forward to simplify the task. Typically, it is assumed that the localization length for the DO state is more than for the SO, a2>a1 [44]. In [56] the possibility of spin dependent transport was discussed considering inequality between two densities of states and two localization lengths. From a practical point of view, it seems problematic to separate these quantities in the framework of such general approach. It is necessary to introduce additional assumptions associated with the density of states or the localization length.In [55] the spin polarized mechanism of MR was investigated in terms of the approach proposed by Kurobe and Kamimura [44]. It was supposed that both the states, UO and SO, are characterized by the same localization length, a1=a2=a, while densities of states differ from each other, g1≠g2.We failed in the attempts to fit the experimental data of Figure2(b) applying theoretical approaches of Refs. [55, 56]. We believe this is due to the fact that applied theoretical approaches do not take into account all complexity of the transport mechanisms. Further we investigate this problem in detail within the approach proposed by Demishev et al. [57, 58]. Authors [57], following Kurobe and Kamimura [44], considered only intrasite correlations and neglect the long range Coulomb repulsion. On the basis of [57] it is possible to determine which type of conductivity under the external magnetic field dominates: spin dependent or spin independent. In particular, the modified expression for the MR, which takes into account both types of hops, was deduced [58]:(4)ln⁡ρHρ0=TMT1/414AeffTμ0μBHkBT2,where(5)AeffT=A+4bTTM3/2.In (5) parameters A=(g2a23-g1a13)/(g2a23+g1a13) and b=t3a24(e2kB2TM2/ħ2μB2). According to Demishev et al. [58], parameter A depends on the probability of hops, which involve both D0 and D- states, and is determined by the degree of polarization of the spin part of the wave function of these states in the magnetic field. Parameter b is determined by the contribution of the mechanism of the wave function contraction to the MR that acts on both types of hops.Therefore, on the basis of the temperature dependenceAeff(T) it is possible to conclude which type of contribution determines the MR in the hopping region. If the spin dependent mechanism dominates, then Aeff(T)=const. Otherwise, Aeff(T) tends to 0 at T→0 according to the law T3/2. When both types of contributions are comparable, the dependence of Aeff(T) is expected to be more complicated, it does not tend to 0 at T→0 [57, 58].In Figure7 we plot the Aeff(T) dependence obtained from the experiment applying (4). Data are for H=80 kOe. As can be seen, the Aeff(T) dependence has two distinct regions. In one of them, in the T range 5–11 K, the Aeff value is temperature independent and the results of the fitting procedure give A=0.47±0.03, b=0 (blue line in Figure 7). Therefore, in this T range the spin dependent hopping prevails. In addition, the relation between DOS for two different types of hops can be estimated via the quantity kg=g2a23/g1a13. In this case kg≈2.8.Figure 7
Evaluated temperature dependenceAeff(T) at H=80 kOe (symbols). Lines are plotted according to (5). Inset: the temperature dependence of the calculated coefficient kg.In theT range 11–20 K the linear approximation Aeff(T)~T3/2 explains well the experimental data (red line in Figure 7), but Aeff does not tend to 0 at T→0. Consequently, the obtained result proves the absence of the dominant role of the spin independent hops in this temperature interval. From the fitting procedure we obtained coefficients A=0.29 and b=0.96×104. That gives a2=5.5nm and a1≈a2/4=1.38nm. The parameter kg in this case depends on T. The obtained overall kg(T) dependence is shown in the inset to Figure 7. From kg values we may estimate the g1/g2 relation, which is equal to 21.3 for T range 5–10 K and to 10.7 at T=20K.


### 4.2.2. Gap in the DOS

Thus, the performed estimations and calculations showed that, in the temperature range 5–20 K, on the whole, the Mott-type VRH is realized. Nevertheless, we obtained that two types of hops, traditional hops on UO sites and spin dependent hops on SO sites, have to be taken into account. Therefore, one needs to consider two localization lengths and two DOS. On the other hand, previously introducedg1 and g2 values are essentially model parameters that do not give information about the influence of the DOS on the mechanism of hopping conductivity. It should also be noted that neither approach [55] nor work [57] gives any information about the gap between two Hubbard bands.Generally speaking, the origin of the gap could be twofold. First, it could be due to the CG; second, the HG between lower and upper Hubbard bands could be the reason. The soft CG at the energy minimum does not have a characteristic shelf,g(E)~|E-EF|2, while the true gap has the shelf of the width Δ. Moreover, the presence of the soft CG leads to the exponent p=1/2, which we did not observe.Below we propose the model expression for the DOS and evaluate the influence of the shape and parameters of the proposed model DOS on theT dependence of the hopping resistivity, which, in turn, is characterized by the critical values of the exponent ξ(T)=ln⁡[ρ(T)/ρ0] [21]. The relation between the critical exponent ξ(T) and the exponent p is ξ(T)~(Th/T)p. Estimations are performed within the model of the low temperature crossover VRH-SAD.To model this crossover let us consider the problem of the charge flow in the lattice of impurity atoms. In the theory of hopping conductivity, problems of charge flow in the system of random nodes, chaotically distributed in space, play the most important role. In this case the average number of nodes in a unit volume is supposed to be given and equal to the concentration of the impuritiesNd. The average distance between nodes is rd=(3/4πNd)1/3. For such a lattice, the percolation radius rc is found from the condition of the connectivity of two and more nodes which form an infinite cluster [6], so that the value of rc depends only on the nodes concentration Nd. Typically, the dimensionless threshold value Bc is used, having a meaning of the average number of bonds per node. In the 3D case [6](6)Bc=4π3rc3Nd.For random lattice theBc value is typically determined numerically and varied in the range 2.65–2.76 [6]. Consequently, the percolation radius is given by rc=(0.865±0.015)Nd-1/3. In this case rc is always larger than rd. In particular, in our case rc=8.64nm>rd=6.2nm. In other words, the symmetry of the lattice is irrelevant and only the number of sites inside radius rc determines the transport mechanism.On the basis of the aforementioned estimations, we then developed a model of the VRH-SAD crossover; this model is based on a simplified procedure for solving the percolation problem using the empiric expression for the DOS valid for both types of the temperature dependent hopping. We start from the following expression for the dimensionless concentration of sites:(7)Nξ=2∫0Emaxrmax3gEdE,which satisfies the condition of connectivity for the exponent of the hopping resistivity less than a certain value ξmin [6, 13]. Here, Emax and rmax are maximal values of the energy and intersite spacing, respectively, which still allow the connectivity. The dimensionless concentration N(ξ) in (7) is determined as a product of the concentration of sites with the energy E<Emax and the volume of these sites. This procedure for the temperature dependent DOS is not completely rigorous and the connectivity condition should be considered for each energy value separately, which leads to the complicated integral equation [13]. Here we will follow the procedure described in [21], which simplifies significantly the calculations.Values ofrmax and Emax are specified in the percolation theory by the relations [6] (see also Equation (4.30) in [59])(8)rmax=a2ξ2,Emax=kBTξ.Substituting (8) into (7) and equating N(ξ) to 2Bc, we get the following expression:(9)2Bc=a2ξ23∫0kBTξgEdE,which allows calculating the T dependence of ξ and compare it with the experimental data ρ(T). The above procedure was carried out using three different types of expressions for the DOS.First, we used the interpolation expression proposed in [22, 23]. Thus, the change of the DOS from constant value for the VRH Mott-type to the DOS g(E)~|E-EF|n, where for the SAD n>2, was taken into account. In this case the DOS models, presumably, only the CG-like, but with steeper dependence on the energy. According to [22], the crossover at different exponent values of p=(n+1)/(n+4) could be described applying the following expression for the DOS:(10)gE,T=g0E-EF/Esgn1+E-EF/Esgn.Parameter Esg depends on the exponent n and, when it is fixed, is constant. Parameter g0 is a constant related to gM. For the case n=2, (10) coincides with the expression used in [14] for the description of the crossover from the Mott to ES VRH.Substituting (10) into (9) and using the previously obtained values, a2 and Esg=ϵ4, we calculated the dependencies ξ(T) for the fixed values of the exponent n in (10), which were compared with the experimental data ln⁡[ρ(T)/ρ0]. We obtained that theoretical results coincide with the experimental data only varying values of the exponent n with temperature [60]. For example, in the interval 5–25 K the agreement is observed only for n=0 (the Mott-type VRH), while for 2–5 K to obtain the agreement between theory and experiment much greater value of n, n>6, is required, Figure 8. Calculations of the p(T) dependencies for different n values using the relation p=-∂log⁡ξ(T)/∂log⁡T=-T/ξ(T)∂ξ(T)/∂T [21] and evaluated the ξ(T) dependence showed that, to achieve the value of the exponent p, close to unity, it is necessary to significantly increase n, that is, the variable n needs to tend to infinity, Figure 9. At n=0 expressions for the crossover give the exact value p=1/4. Thus, (10) for the DOS in this case has limited application because, firstly, it requires a change of the exponent n with T and, secondly, the value of n, which provides the exponent p→1, tends to infinity.Figure 8
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (10) ξ(T) dependencies. Red and blue lines correspond to n=0 and 15, respectively.Figure 9
Temperature dependencies of the exponentp for different n values. From top to down, n = 200, 100, 50, 15, 5, and 2, respectively.In the second attempt, we take into account the gap smearing withT increase [61],(11)gE,T=g0γT+1-γTE-EFnΔT/2n+E-EFn.The parameter γ describes a “residual” DOS at the Fermi level and Δ is the width of the gap.Substitution of the modified expression (11) to (9) allowed comparing the value of the critical exponent ξ with the experimental data and finding the temperature dependencies γ(T) and Δ(T), which adequately describe the experiment. This result is presented in Figure 10 for two n values, n=2.5 and 3.0.Figure 10
γ ( T ) and Δ(T) dependencies as obtained using (11) for fitting the ρ(T) data. Calculated curves correspond to the range of the exponent n=2.5–3.0. The γ values are in arbitrary units. The Δ values are normalized to ϵ4.It follows from Figure10 that γ varies in the range 0.1–1. At T>10K, γ→1, and the first constant term in (11) dominates. This corresponds to the Mott-type VRH. When γ=1 (i.e., at T>15K), the result becomes insensitive to the Δ values. At low temperatures γ≪1 and the main contribution is due to the term |E-EF|n. The parameter Δ, which characterizes the width of the gap, decreases with increasing temperature, which is in contradiction with the result usually reported [61, 62]. Thus, the result of the fitting procedure found that the agreement with the experiment is achieved only taking into account the filling of the gap states between the Hubbard bands and suggested the narrowing of the gap with increasing temperature, during the crossover to the Mott-type DOS. In addition, insensitivity of the model to the value of n at n>3 has been revealed. Therefore, it is obvious that there is a need to modify the formula for the DOS, in order to reflect the tendency both for smearing of the gap and its growth with increasing temperature. These are characteristic features of the HG. Moreover, the integer exponent n should be temperature independent.Within these assumptions the reasonable approximation for the DOS is of the following empiric type:(12)gE,T=g0αTw4E+βTw2E+γT×exp-wEσT4,where w(E)=E-EF/0.5ϵ4 and α, β, γ, and σ are phenomenologicaltemperature dependent coefficients.The shape of the DOS in this case depends onT according to the α, β, γ and σ versus T dependencies. In particular, the first term corresponds to the HG, the second one is for the soft gap, the parameter γ is responsible for the filling of the HG with T and σ is responsible for the width of the Hubbard band. Indeed, the exponential term serves for smoothing of the overall DOS and for modelling of the Hubbard bands, in particular, their width. In other words, empirical expression (12) allows reproducing not only the HG, its filling, but also the width of the Hubbard bands. In this work, we assumed the identical widths of the upper and lower Hubbard bands. Widening of the UHB was taken into account by filling the HG. Function (12) reflects the change of the DOS with T, from HG at low T (with the dip between Hubbard bands) to the constant DOS close to the Fermi level at high T. This was enough for the experimental data interpretation. The fitting procedure was as for previous expressions for the DOS; that is, we substitute (12) into (9) and looked for such ξ values which adequately describe the ρ(T) data. The result of the fitting procedure is shown in Figure 11. It follows that we were able to describe experimental data with very high accuracy in the T range 2–20 K. On the basis of the obtained ξ(T) dependence it is possible to evaluate rmax, the maximal hopping length which still allows the connectivity. For the range 5–20 K we get rmax=17.6–22.0nm, while for the interval 2–4 K the result is rmax=27.5–38.5nm.Figure 11
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (12) ξ(T) dependencies.On the basis of the obtained model parameters, it is possible to reproduce the DOS at different temperatures. This result is shown in Figure12. As it follows, the DOS evolves from HG at 2 K to almost filled states between Hubbard bands at 15 K. At that the widening of the Hubbard bands also occurs (within our approach, UHB and LHB are symmetrical; actually, they may differ in width and height, but this issue requires additional investigation and is outside the objectives of this work). Parameters of the model are changed as follows. The parameter α, which corresponds to the HG width is almost constant and is equal to 1 for the whole T range. The parameter β (characteristic of the soft gap) is almost constant with temperature, β=-0.7 except the region 15–21 K, where β=-2. The parameter γ, which is responsible for the HG filling, is changed from 0 at 2 K to 6 at 21 K. Finally, the parameter σ, the characteristic of the width of the Hubbard bands, also increases with temperature, from 1.5 to 2.3.Figure 12
DOS at different temperatures as obtained from the experimental data within the proposed model (see (12)).At the end of this section we summarize that, the conductivity in theT interval 5–20 K is of the hopping-type. On the whole, it obeys the Mott law and is determined by two type of hops: to UO neutral and to SO impurity sites. In the range 5–11 K the contribution of the spin dependent hopping dominates. This is valid also in the range 2–4 K. Simulations of the DOS revealed that in this T range hops are regulated by the HG. The presence of nonsmeared HG between Hubbard bands in the T range 2–4 K together with the spin dependent hops in the UHB provides reentrance of the SAD.The latter provides a nonlinearity of the current-voltage characteristics at small bias voltage, which leads to negative differential resistance at electrical fields smaller than 1 V/cm [63]. It is unlikely that this effect may be due to the ES VRH, for which the delocalization occurs at significantly higher electrical fields.


## 4.2.1. Spin Dependent Hopping

For theT range 5–20 K the resistivity is described according to the Mott law, (1) [3, 6], in which Th=TM and p=1/4. Here TM=βMgMaM3kB-1 is the Mott parameter, βM=21.2±1.2 is the numerical factor, gM=const is DOS at the Fermi level, aM is the localization length of the states around the Fermi level. We calculated the gM and aM values analyzing the experimental data ρ(T) at zero magnetic field in the Mott coordinates (ρ-T-1/4) and applying the evaluation expressions [3, 6, 52, 53](2)gM=Nd2kBTMTvM31/4,aM=βM1/3kBTMgM1/3,where TvM is the temperature of the onset of the Mott-type VRH. Equation (2) gives approximate values of gM and aM. Note that on the basis of (1) and (2) the obtained gM and aM values must be temperature independent. On the other hand, the MR data allow checking whether these quantities are really T independent. Indeed, within the standard approach of the Mott-type VRH the positive MR which is usually related to the contraction of the wave function of the localized states in magnetic field is expressed as [6](3)ln⁡ρHρ0=t3aM4lH4TMT3/4~H2,where numerical factor t3=5/2016, lH=ħ/eμ0H is the magnetic length, and ρ(0) is the zero field resistivity.On the basis of (3), knowing TM, H, and MR, we calculated the aM values at different T. Moreover, knowing already aM, the value of gM from results of the MR measurements can be calculated using the expression for the Mott parameter TM.The results of calculations of hopping parameters according to theρ(T) dependence and MR data at different T are summarized in Table 1. The Mott parameter was evaluated from (1) as TM=1.524×104 K. The temperature TvM was obtained from the ρ(T) data as TvM≈20K [54].Table 1
Parameters of the Mott-type VRH obtained within two different approaches.
Parameter ρ ( T ) data MR data a M, nm 6.6 6.0–8.5 g M, eV-1×cm-3 5.408 × 1 0 19 4.7 × 1 0 19It follows from Table1 that the obtained within two different approaches aM and gM values are in good agreement with each other.The surprising result, which we obtained, analyzing theaM values from the MR measurements, is their T dependence. This result for H=80 kOe is presented in Figure 4, from which it follows that the aM(T) function is not constant. In particular, for the range 5–20 K the aM values decrease from 8.3 to 6.0 nm. This means that the standard model of positive MR, which takes into account only the contraction of the electronic wave function in magnetic field and leads to the temperature independent localization length, cannot explain the obtained aM(T) result.Figure 4
Temperature dependence of the localization lengthaM. Data are for H=80 kOe.In Figure5 we show the dependencies of ln(ρ(H)/ρ(0)) versus H2 in the temperature range 4–20 K together with the results of the best fit procedure according to (3). It is seen that the ln(ρ(H)/ρ(0))~H2 law in the considered temperature range is valid only at H<(50–60) kOe. From the results presented in Figures 2(b), 4 and 5 it follows that the transport mechanism at low T becomes more complicated than conventional Mott-type VRH. To clarify the hopping mechanism, we examine other possible types of hops, to the occupied localized sites, which are accompanied by a spin flip [44].Figure 5
l n ρ ( H ) / ρ ( 0 ) versus H2 at different temperatures (symbols). Lines correspond to the results of the best linear fit in these coordinates.The MR for a system of sites occupied by more than one electron was considered in detail some time ago by Kurobe and Kamimura [44], Matveev et al. [55], Meir [56], and Demishev and Pronin [57]. In particular, if the Coulomb repulsion between two electrons is smaller than the width of the Hubbard bands, 2 types of hops, on unoccupied (SO → UO, DO → UO) and occupied (SO → SO, DO → SO) sites are relevant. All these possibilities are shown in Figure 6, where we schematically draw the energy diagrams for each type of hops.Figure 6
Possible electron hops considered for low temperature conductivity. For more details, see the text.In general case, spin independent hops to unoccupied sites could be characterized by the localization lengtha1 and DOS g1, while spin dependent hops to occupied sites could be described, in turn, by a2 and g2. The quantity g1 is assigned to the DOS in the LHB, and g2 corresponds to the DOS in the UHB. The relation between g1 and g2 as well as between a1 and a2 is still an open question and different assumptions were put forward to simplify the task. Typically, it is assumed that the localization length for the DO state is more than for the SO, a2>a1 [44]. In [56] the possibility of spin dependent transport was discussed considering inequality between two densities of states and two localization lengths. From a practical point of view, it seems problematic to separate these quantities in the framework of such general approach. It is necessary to introduce additional assumptions associated with the density of states or the localization length.In [55] the spin polarized mechanism of MR was investigated in terms of the approach proposed by Kurobe and Kamimura [44]. It was supposed that both the states, UO and SO, are characterized by the same localization length, a1=a2=a, while densities of states differ from each other, g1≠g2.We failed in the attempts to fit the experimental data of Figure2(b) applying theoretical approaches of Refs. [55, 56]. We believe this is due to the fact that applied theoretical approaches do not take into account all complexity of the transport mechanisms. Further we investigate this problem in detail within the approach proposed by Demishev et al. [57, 58]. Authors [57], following Kurobe and Kamimura [44], considered only intrasite correlations and neglect the long range Coulomb repulsion. On the basis of [57] it is possible to determine which type of conductivity under the external magnetic field dominates: spin dependent or spin independent. In particular, the modified expression for the MR, which takes into account both types of hops, was deduced [58]:(4)ln⁡ρHρ0=TMT1/414AeffTμ0μBHkBT2,where(5)AeffT=A+4bTTM3/2.In (5) parameters A=(g2a23-g1a13)/(g2a23+g1a13) and b=t3a24(e2kB2TM2/ħ2μB2). According to Demishev et al. [58], parameter A depends on the probability of hops, which involve both D0 and D- states, and is determined by the degree of polarization of the spin part of the wave function of these states in the magnetic field. Parameter b is determined by the contribution of the mechanism of the wave function contraction to the MR that acts on both types of hops.Therefore, on the basis of the temperature dependenceAeff(T) it is possible to conclude which type of contribution determines the MR in the hopping region. If the spin dependent mechanism dominates, then Aeff(T)=const. Otherwise, Aeff(T) tends to 0 at T→0 according to the law T3/2. When both types of contributions are comparable, the dependence of Aeff(T) is expected to be more complicated, it does not tend to 0 at T→0 [57, 58].In Figure7 we plot the Aeff(T) dependence obtained from the experiment applying (4). Data are for H=80 kOe. As can be seen, the Aeff(T) dependence has two distinct regions. In one of them, in the T range 5–11 K, the Aeff value is temperature independent and the results of the fitting procedure give A=0.47±0.03, b=0 (blue line in Figure 7). Therefore, in this T range the spin dependent hopping prevails. In addition, the relation between DOS for two different types of hops can be estimated via the quantity kg=g2a23/g1a13. In this case kg≈2.8.Figure 7
Evaluated temperature dependenceAeff(T) at H=80 kOe (symbols). Lines are plotted according to (5). Inset: the temperature dependence of the calculated coefficient kg.In theT range 11–20 K the linear approximation Aeff(T)~T3/2 explains well the experimental data (red line in Figure 7), but Aeff does not tend to 0 at T→0. Consequently, the obtained result proves the absence of the dominant role of the spin independent hops in this temperature interval. From the fitting procedure we obtained coefficients A=0.29 and b=0.96×104. That gives a2=5.5nm and a1≈a2/4=1.38nm. The parameter kg in this case depends on T. The obtained overall kg(T) dependence is shown in the inset to Figure 7. From kg values we may estimate the g1/g2 relation, which is equal to 21.3 for T range 5–10 K and to 10.7 at T=20K.


## 4.2.2. Gap in the DOS

Thus, the performed estimations and calculations showed that, in the temperature range 5–20 K, on the whole, the Mott-type VRH is realized. Nevertheless, we obtained that two types of hops, traditional hops on UO sites and spin dependent hops on SO sites, have to be taken into account. Therefore, one needs to consider two localization lengths and two DOS. On the other hand, previously introducedg1 and g2 values are essentially model parameters that do not give information about the influence of the DOS on the mechanism of hopping conductivity. It should also be noted that neither approach [55] nor work [57] gives any information about the gap between two Hubbard bands.Generally speaking, the origin of the gap could be twofold. First, it could be due to the CG; second, the HG between lower and upper Hubbard bands could be the reason. The soft CG at the energy minimum does not have a characteristic shelf,g(E)~|E-EF|2, while the true gap has the shelf of the width Δ. Moreover, the presence of the soft CG leads to the exponent p=1/2, which we did not observe.Below we propose the model expression for the DOS and evaluate the influence of the shape and parameters of the proposed model DOS on theT dependence of the hopping resistivity, which, in turn, is characterized by the critical values of the exponent ξ(T)=ln⁡[ρ(T)/ρ0] [21]. The relation between the critical exponent ξ(T) and the exponent p is ξ(T)~(Th/T)p. Estimations are performed within the model of the low temperature crossover VRH-SAD.To model this crossover let us consider the problem of the charge flow in the lattice of impurity atoms. In the theory of hopping conductivity, problems of charge flow in the system of random nodes, chaotically distributed in space, play the most important role. In this case the average number of nodes in a unit volume is supposed to be given and equal to the concentration of the impuritiesNd. The average distance between nodes is rd=(3/4πNd)1/3. For such a lattice, the percolation radius rc is found from the condition of the connectivity of two and more nodes which form an infinite cluster [6], so that the value of rc depends only on the nodes concentration Nd. Typically, the dimensionless threshold value Bc is used, having a meaning of the average number of bonds per node. In the 3D case [6](6)Bc=4π3rc3Nd.For random lattice theBc value is typically determined numerically and varied in the range 2.65–2.76 [6]. Consequently, the percolation radius is given by rc=(0.865±0.015)Nd-1/3. In this case rc is always larger than rd. In particular, in our case rc=8.64nm>rd=6.2nm. In other words, the symmetry of the lattice is irrelevant and only the number of sites inside radius rc determines the transport mechanism.On the basis of the aforementioned estimations, we then developed a model of the VRH-SAD crossover; this model is based on a simplified procedure for solving the percolation problem using the empiric expression for the DOS valid for both types of the temperature dependent hopping. We start from the following expression for the dimensionless concentration of sites:(7)Nξ=2∫0Emaxrmax3gEdE,which satisfies the condition of connectivity for the exponent of the hopping resistivity less than a certain value ξmin [6, 13]. Here, Emax and rmax are maximal values of the energy and intersite spacing, respectively, which still allow the connectivity. The dimensionless concentration N(ξ) in (7) is determined as a product of the concentration of sites with the energy E<Emax and the volume of these sites. This procedure for the temperature dependent DOS is not completely rigorous and the connectivity condition should be considered for each energy value separately, which leads to the complicated integral equation [13]. Here we will follow the procedure described in [21], which simplifies significantly the calculations.Values ofrmax and Emax are specified in the percolation theory by the relations [6] (see also Equation (4.30) in [59])(8)rmax=a2ξ2,Emax=kBTξ.Substituting (8) into (7) and equating N(ξ) to 2Bc, we get the following expression:(9)2Bc=a2ξ23∫0kBTξgEdE,which allows calculating the T dependence of ξ and compare it with the experimental data ρ(T). The above procedure was carried out using three different types of expressions for the DOS.First, we used the interpolation expression proposed in [22, 23]. Thus, the change of the DOS from constant value for the VRH Mott-type to the DOS g(E)~|E-EF|n, where for the SAD n>2, was taken into account. In this case the DOS models, presumably, only the CG-like, but with steeper dependence on the energy. According to [22], the crossover at different exponent values of p=(n+1)/(n+4) could be described applying the following expression for the DOS:(10)gE,T=g0E-EF/Esgn1+E-EF/Esgn.Parameter Esg depends on the exponent n and, when it is fixed, is constant. Parameter g0 is a constant related to gM. For the case n=2, (10) coincides with the expression used in [14] for the description of the crossover from the Mott to ES VRH.Substituting (10) into (9) and using the previously obtained values, a2 and Esg=ϵ4, we calculated the dependencies ξ(T) for the fixed values of the exponent n in (10), which were compared with the experimental data ln⁡[ρ(T)/ρ0]. We obtained that theoretical results coincide with the experimental data only varying values of the exponent n with temperature [60]. For example, in the interval 5–25 K the agreement is observed only for n=0 (the Mott-type VRH), while for 2–5 K to obtain the agreement between theory and experiment much greater value of n, n>6, is required, Figure 8. Calculations of the p(T) dependencies for different n values using the relation p=-∂log⁡ξ(T)/∂log⁡T=-T/ξ(T)∂ξ(T)/∂T [21] and evaluated the ξ(T) dependence showed that, to achieve the value of the exponent p, close to unity, it is necessary to significantly increase n, that is, the variable n needs to tend to infinity, Figure 9. At n=0 expressions for the crossover give the exact value p=1/4. Thus, (10) for the DOS in this case has limited application because, firstly, it requires a change of the exponent n with T and, secondly, the value of n, which provides the exponent p→1, tends to infinity.Figure 8
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (10) ξ(T) dependencies. Red and blue lines correspond to n=0 and 15, respectively.Figure 9
Temperature dependencies of the exponentp for different n values. From top to down, n = 200, 100, 50, 15, 5, and 2, respectively.In the second attempt, we take into account the gap smearing withT increase [61],(11)gE,T=g0γT+1-γTE-EFnΔT/2n+E-EFn.The parameter γ describes a “residual” DOS at the Fermi level and Δ is the width of the gap.Substitution of the modified expression (11) to (9) allowed comparing the value of the critical exponent ξ with the experimental data and finding the temperature dependencies γ(T) and Δ(T), which adequately describe the experiment. This result is presented in Figure 10 for two n values, n=2.5 and 3.0.Figure 10
γ ( T ) and Δ(T) dependencies as obtained using (11) for fitting the ρ(T) data. Calculated curves correspond to the range of the exponent n=2.5–3.0. The γ values are in arbitrary units. The Δ values are normalized to ϵ4.It follows from Figure10 that γ varies in the range 0.1–1. At T>10K, γ→1, and the first constant term in (11) dominates. This corresponds to the Mott-type VRH. When γ=1 (i.e., at T>15K), the result becomes insensitive to the Δ values. At low temperatures γ≪1 and the main contribution is due to the term |E-EF|n. The parameter Δ, which characterizes the width of the gap, decreases with increasing temperature, which is in contradiction with the result usually reported [61, 62]. Thus, the result of the fitting procedure found that the agreement with the experiment is achieved only taking into account the filling of the gap states between the Hubbard bands and suggested the narrowing of the gap with increasing temperature, during the crossover to the Mott-type DOS. In addition, insensitivity of the model to the value of n at n>3 has been revealed. Therefore, it is obvious that there is a need to modify the formula for the DOS, in order to reflect the tendency both for smearing of the gap and its growth with increasing temperature. These are characteristic features of the HG. Moreover, the integer exponent n should be temperature independent.Within these assumptions the reasonable approximation for the DOS is of the following empiric type:(12)gE,T=g0αTw4E+βTw2E+γT×exp-wEσT4,where w(E)=E-EF/0.5ϵ4 and α, β, γ, and σ are phenomenologicaltemperature dependent coefficients.The shape of the DOS in this case depends onT according to the α, β, γ and σ versus T dependencies. In particular, the first term corresponds to the HG, the second one is for the soft gap, the parameter γ is responsible for the filling of the HG with T and σ is responsible for the width of the Hubbard band. Indeed, the exponential term serves for smoothing of the overall DOS and for modelling of the Hubbard bands, in particular, their width. In other words, empirical expression (12) allows reproducing not only the HG, its filling, but also the width of the Hubbard bands. In this work, we assumed the identical widths of the upper and lower Hubbard bands. Widening of the UHB was taken into account by filling the HG. Function (12) reflects the change of the DOS with T, from HG at low T (with the dip between Hubbard bands) to the constant DOS close to the Fermi level at high T. This was enough for the experimental data interpretation. The fitting procedure was as for previous expressions for the DOS; that is, we substitute (12) into (9) and looked for such ξ values which adequately describe the ρ(T) data. The result of the fitting procedure is shown in Figure 11. It follows that we were able to describe experimental data with very high accuracy in the T range 2–20 K. On the basis of the obtained ξ(T) dependence it is possible to evaluate rmax, the maximal hopping length which still allows the connectivity. For the range 5–20 K we get rmax=17.6–22.0nm, while for the interval 2–4 K the result is rmax=27.5–38.5nm.Figure 11
Experimental (symbols)ln⁡[ρ(T)/ρ0] and calculated (lines) according to (12) ξ(T) dependencies.On the basis of the obtained model parameters, it is possible to reproduce the DOS at different temperatures. This result is shown in Figure12. As it follows, the DOS evolves from HG at 2 K to almost filled states between Hubbard bands at 15 K. At that the widening of the Hubbard bands also occurs (within our approach, UHB and LHB are symmetrical; actually, they may differ in width and height, but this issue requires additional investigation and is outside the objectives of this work). Parameters of the model are changed as follows. The parameter α, which corresponds to the HG width is almost constant and is equal to 1 for the whole T range. The parameter β (characteristic of the soft gap) is almost constant with temperature, β=-0.7 except the region 15–21 K, where β=-2. The parameter γ, which is responsible for the HG filling, is changed from 0 at 2 K to 6 at 21 K. Finally, the parameter σ, the characteristic of the width of the Hubbard bands, also increases with temperature, from 1.5 to 2.3.Figure 12
DOS at different temperatures as obtained from the experimental data within the proposed model (see (12)).At the end of this section we summarize that, the conductivity in theT interval 5–20 K is of the hopping-type. On the whole, it obeys the Mott law and is determined by two type of hops: to UO neutral and to SO impurity sites. In the range 5–11 K the contribution of the spin dependent hopping dominates. This is valid also in the range 2–4 K. Simulations of the DOS revealed that in this T range hops are regulated by the HG. The presence of nonsmeared HG between Hubbard bands in the T range 2–4 K together with the spin dependent hops in the UHB provides reentrance of the SAD.The latter provides a nonlinearity of the current-voltage characteristics at small bias voltage, which leads to negative differential resistance at electrical fields smaller than 1 V/cm [63]. It is unlikely that this effect may be due to the ES VRH, for which the delocalization occurs at significantly higher electrical fields.


## 5. Conclusions

In conclusion, we performed the systematic study of the transport mechanisms inn-type noncompensated Si in the temperature range 2–300 K. Samples were grown by the Czochralski method, containing donor impurities of Sb with a concentration of 1×1018cm-3, It was found that, depending on the temperature range, it is possible to identify 4 different mechanisms of the electron transport. All of them include the upper and lower Hubbard bands.In theT range 110–300 K the usual activation to the edge of the conduction band occurs.At lowerT, in the range 2–90 K, the conductivity of silicon is mainly due to the impurities and is caused by the hopping and band electron transport involving two Hubbard bands. In the high T range of this interval (28–90 K) electronic states are delocalized and charge transport occurs via the SO neutral donors, while in the low T range (2–20 K) electronic states are localized and the hopping prevails. The hopping region is characterized by two types of hops, on UO and SO sites, as well as by two modes, the Mott-type and SAD. The Mott regime, in turn, is characterized by two types of hops and two mechanisms of the MR, mainly the spin polarized mechanism in the T range 5–11 K and the mechanism, for which contribution of the spin polarization is approximately equal to the contribution of the wave function contraction (11–20 K). In the T interval 2–4 K the conductivity is governed by the HG and the charge transport is associated mainly with the spin dependent hopping in the UHB.To improve the identification of the observed Mott-type VRH-SAD crossover and enhance the temperature interval of SAD the energy range of the impurity states as well as the level of the injection of the electrons should be increased [63].Simulation of the DOS within the model of crossover between the Mott-type VRH and SAD were carried out for two types of DOS, soft gap and HG. We showed that, the use of the interpolation expression for the CG-like DOS, but with the exponentn greater than 2 and neglecting the gap smearing, leads to the necessity of noticeable increase of the exponent n to get the exponent p=1 at T<4K. Simulation of the CG-like DOS taking into account the width of the gap and smearing of the region between Hubbard bands showed that, with increasing T both smearing and decreasing of the gap occurs that does not quite correspond to the T dependence of the soft gap known from literature. Finally, simulation within the HG approach considering smearing, growth of the HG, and widening of the Hubbard bands with increasing T allowed describing with high accuracy the experimental ρ(T) dependence in the low T range 2–20 K. The latter confirms the adequacy of the proposed HG model for interpretation of the conductivity in the range 2–4 K, although more detailed experimental and theoretical studies are required to clarify better the impact of the HG on the low T electron transport.In particular, direct spectroscopic measurements of the density of states or conductivity measurements for n-type Si with impurities of various energy levels and different compensation degree could be potentially useful for these purposes.



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