In this work, we study spontaneous electron to ion root transitions in TJ-II using Langmuir probes. By scanning the probe position on a shot to shot basis, we reconstruct a spatiotemporal map of the evolution of important turbulent quantities in the plasma edge region. We pay particular attention to the evolution of the cross phase between transport-relevant variables, showing the spatiotemporal evolution of this quantity for the first time, revealing the outward propagation of the changes associated with the transition. We also compute the intermittence parameter, which allows us to conclude that the turbulence, although its amplitude increases, condenses in a reduced number of dominant modes and becomes less bursty. The causal relationship between variables is studied using the transfer entropy, clarifying the interactions between the main variables and offering a rather complete picture of the complex evolution of the plasma across the confinement transition.

## I. INTRODUCTION

Fusion plasmas are strongly driven systems, exhibiting some of the steepest temperature gradients of all known systems, and are, therefore, far from thermodynamic equilibrium. These systems exhibit phase transitions (confinement transitions) in which order arises spontaneously out of strong turbulence in the form of zonal flows, associated with the establishment of a radial electric field and a transport barrier involving the modification of turbulence.^{1} The complex interactions between radial transport (profiles) and turbulence remain a subject of intense study, in view of the importance of transport barriers for the efficiency and viability of putative fusion reactors. In this work, we study the regulation of transport by sheared flows through the cross phase between fluctuating variables,^{2–5} with unprecedented spatiotemporal resolution, and use some advanced techniques [the transfer entropy (TE) and intermittence] to provide deeper insight into these processes.

## II. EXPERIMENTAL SETUP

TJ-II is a flexible Heliac^{6} with toroidal magnetic field $BT\u22431$ T, major radius $R0=1.5$ m, and minor radius *a *<0.22 m.^{7} Plasmas can be heated using two Electron Cyclotron Resonance Heating (ECRH) beam lines delivering up to 300 kW each at a frequency of 53.2 GHz (X mode) and two Neutral Beam Injector (NBI) systems (co and counter) with up to 2 × 700 kW port-through power. The line average electron density is measured using a microwave interferometer.^{8}

In this work, we analyze a set of similar ECR heated discharges with a magnetic configuration (labelled “100_46_65”) characterized by low magnetic shear and a rotational transform $\iota \u2212(0)\u22431.575$ and $\iota \u2212(1)\u22431.665$. The vacuum configuration has some important rational surfaces in the edge region ($\iota \u2212=5/3$ at $\rho \u22431$ and $\iota \u2212=18/11$ at $\rho \u22430.86$). Since both plasma pressure and internal plasma currents are small, the actual magnetic configuration closely matches the externally imposed configuration.^{9}

TJ-II is fitted with two reciprocating probe drives. Probe drive D (located at toroidal position $\varphi =38.2\xb0$) is fitted with a staircase head containing three triple probes.^{10,11} Each triple probe consists of three pins, measuring *V _{f}*, $Isat$, and

*V*, respectively, where

_{f}*V*is the floating potential and $Isat$ is the ion saturation current. Probe drive B (at $\varphi =195\xb0$) is fitted with a rake probe, containing a triple probe at its tip and several radially distributed pins along its side.

_{f}^{12}

## III. METHODS

The difference of the two *V _{f}* measurements of the triple probe, aligned poloidally, divided by their distance $d\theta $, provides an estimate of the poloidal electric field, $E\theta $, at the same location as the $Isat$ measurement. The sign convention of $E\theta $ follows Ref. 13. Likewise, the radial electric field

*E*can be estimated from the difference of two

_{r}*V*signals divided by their radial distance

_{f}*d*using two radially spaced probe pins.

_{r}The fluctuating particle flux Γ can be estimated from $\Gamma =\u27e8n\u0303E\u0303\theta \u27e9/B$. The ion saturation current $Isat$ is assumed proportional to the fluctuating density $n\u0303$. Thus, the fluctuating particle flux is proportional to the fluctuation amplitudes or root-mean-square values RMS $(Isat)$ and RMS $(E\theta )$, as well as the cosine of the phase angle $\Delta \varphi $ between these two quantities, $cos\u2009(\Delta \varphi )$.^{1} Hence, these quantities play a major role in the understanding of particle transport and are the prime focus of this work.

The probe data also allow estimating the phase velocity $v\theta $ using the two-point correlation technique^{14} applied to the mentioned two poloidally aligned *V _{f}* signals. Thus, using this probe setup, a rather complete set of data are accessible to study turbulence evolution during confinement transitions.

The phase angle is estimated using two alternative techniques. The complex coherence $\gamma (f)$ of two signals *x*(*t*) and *y*(*t*) over a time window $T={t0\u2264t<t1}$ is calculated by subdividing this time window in a small number *N* of subwindows, calculating the complex Fourier transforms *X*(*f*) and *Y*(*f*) for each subwindow, and evaluating $\gamma =\u2009\u27e8XY*\u27e9N/\u27e8|X|2\u27e9N\u27e8|Y|2\u27e9N$. Here, $\u27e8\xb7\u27e9N$ denotes an average over the *N* subwindows. The frequency-averaged cross phase $\Delta \varphi coh$ of the coherence is estimated over a range of frequencies using $exp\u2009(i\Delta \varphi coh)=\u2009\u2211f\gamma /\u2211f|\gamma |$.

Alternatively, the Hilbert cross phase is calculated for a time window *T* by calculating the fluctuating part of the signals, $x\u0303(t)=x(t)\u2212\u27e8x\u27e9T$, where $\u27e8\xb7\u27e9T$ is the average over *T* and similar for *y*. Then, the Hilbert transform is applied to $x\u0303$ and $y\u0303$, yielding complex signals $x\u0302(t)$ and $y\u0302(t)$. The Hilbert cross phase $\Delta \varphi H$ is defined from $exp\u2009(i\Delta \varphi H)=\u27e8x\u0302y\u0302*\u27e9T/\u27e8|x\u0302|2\u27e9T\u27e8|y\u0302|2\u27e9T$.

The intermittence parameter arises in the field of chaos theory.^{15,16} The fluctuation level of a time series of length *N* is characterized by its normalized root-mean-square (RMS) value *ϵ*, calculated over subtime windows with length $n\u2264N$: $\u03f5=RMSn/RMSN$. The moments $\u27e8\u03f5q\u27e9n$, averaged over all available subwindows with length *n*, are expected to decay as a power of the window length, namely, $\u27e8\u03f5q\u27e9n\u221dn\u2212K(q)$. Since we are interested in the turbulent (high frequency) characteristics of the fluctuations, we determine $K(q)$ from a linear fit of a set of values of $log\u2009\u27e8\u03f5q\u27e9$ vs $log\u2009n$, for a range of values of $n=1,\u2026,n1$, where *n*_{1} is small, e.g., $n1=8$. When *K* is linear in $q$, the time series is considered to be monofractal, otherwise it is multifractal. The intermittence parameter *C*_{1} is defined as the derivative $dK/dq$ evaluated at $q=1$ and ranges from 0 for a monofractal time series to 1 for a multifractal time series.^{17} It is rather insensitive to random noise.^{18} Signals with high value of *C*_{1} are more “bursty” in nature than signals with low *C*_{1}.

The Transfer Entropy (TE) is a nonlinear analysis technique, related to the mutual information, that has proven useful for determining causal relations between fluctuating variables^{19} and the study of heat transport in stellarators,^{20} among others. It measures the “information transfer” between two time series $x(ti)$ and $y(ti)$ by quantifying the number of bits by which the prediction of the next sample of signal *y* can be improved by using the time history of not only the signal *y* itself, but also that of signal *x*. We use a simplified version of the transfer entropy that can be written as

where the *p*'s are multidimensional probability distributions calculated from the data. Only a single historical value (*i* − *k*) of *x* and *y* is used to determine the impact on the next value of *y* (at *i *+* *1). Thus, we compute $TX\u2192Y$ for a range of values *k* to study the causal impact at various “time lags.” If the prediction of the signal *y* is improved by the information contained in signal *x*, $TX\u2192Y$ will be significant and there is a flow of information $x\u2192y$, which can be interpreted in the sense that *x* impacts *y* or has a causal influence on *y*. Unlike the mutual information and the standard linear correlation (which merely quantifies a similarity of waveform), this quantity is directional (from *x* to *y*), as would be required of any quantifier of causality. Even so, as with any quantifier of causality, one can never rule out the existence of a third (possibly undetected) variable *z* that affects both *x* and *y*, so the transfer entropy only provides an indication of causality and no proof.

## IV. EXPERIMENTAL RESULTS

In TJ-II ECRH plasmas, when the line average electron density is raised above a critical value of $ne\xaf\u22430.6\xd71019$ m^{−3}, the plasma performs a spontaneous transition from electron root to ion root confinement.^{21–23} Among other things, this transition is characterized by a change of sign of the radial electric field *E _{r}* in the edge region.

In the discharges analyzed here, these spontaneous confinement transitions were achieved repetitively and systematically by modulating the gas puff. In previous work, the global evolution of profiles (potential, density) and fluctuations from edge Langmuir probes were studied, and the formation of the edge particle transport barrier was visualized.^{22} Magnetic activity was studied using Mirnov pickup coils and poloidal flow using Doppler reflectometry.^{24} Heat transport was analyzed using electron cyclotron emission data in Ref. 20 and core intermittence using heavy ion beam probe data in Ref. 18.

Figure 1 shows some typical time traces. Apart from the top time trace (a), all data are obtained from the D probe system, located inside the plasma at $\rho \u22430.92$. The transition roughly occurs when the line average electron density $ne\xaf$, Fig. 1(a), crosses the value $\u223c0.6\xd71019$ m^{−3}. The root-mean-square fluctuation amplitude of the density time trace increases during the transition, as reported in previous work.^{25}

Figure 1(b) shows that the smoothed floating potential (averaged over two poloidally spaced *V _{f}* probe tips) changes sign at the transition, as does the poloidal velocity $v\theta $ shown in Fig. 1(c). Figure 1(c) also shows the smoothed radial electric field

*E*. Assuming that the poloidal velocity is dominated by the

_{r}*E*×

*B*flow and considering that the TJ-II magnetic field $B\u22431$ T, the numerical values of

*E*and $v\theta $ should be very close, and so they are, except near the transition, where

_{r}*E*appears to be affected by a strong zonal flow contribution. A zonal flow structure is poloidally and toroidally symmetric and, therefore, would not affect $v\theta $, which is derived from two poloidally displaced probe pins. This interpretation is reinforced by the fact that long range correlations

_{r}^{21}between the remote B and D probes have been detected around this time,

^{22}another hallmark of zonal flows.

Prior to the transition, the turbulence amplitude as quantified by the RMS values of $E\theta $ and $Isat$ [shown in Fig. 1(d)] is roughly constant, but at *t *=* *1090 ms, it significantly increases. Figure 1(e) shows that the cross phase between $E\theta $ and $Isat$, calculated using the two methods described above, gradually changes from about $\u2212\pi /2$ for *t *< 1090 ms to $\u223c0$ for *t *> 1110 ms. Figure 1(f) shows that the intermittence parameter *C*_{1} for these two quantities is roughly constant for *t *< 1090 ms and then significantly drops at $t\u22431100$ ms.

Figure 2 shows the spectrogram of $E\theta $ for the discharge shown in Fig. 1. It shows an increase in low-frequency activity following the transition, consistent with the increase in RMS ($E\theta $). The very low frequency activity (*f *<10 kHz) is particularly intense around the time of the transition and is presumed to be related to the mentioned zonal flow. The later, higher frequency activity ($20<f<30$ kHz) is known to be related to a rotating MHD mode, as reported in Ref. 24 on the basis of Mirnov coil analysis.

In this discharge, the B probe was located at approximately the same radial position ($\rho \u22430.9$) as the D probe. One of the pins of the B probe was setup to measure *T _{e}* using the fast swept probe technique.

^{26}Results are shown in Fig. 3. It is observed that the electron temperature slightly increases following the transition, but can be discarded as the cause of the observed phase changes.

Probe B was radially moved on a shot to shot basis. This allows obtaining not only the temporal, but also the spatial variation of many quantities. To compare discharges with slightly varying transition times, we defined a critical time $tcrit$ as the time at which $v\theta $ changes sign and then displayed the quantities as a function of $t\u2212tcrit$.

Results are shown in Fig. 4. The vertical axis shows the position of probe B in each shot (in terms of the normalized minor radius, *ρ*). Colors indicate the value of the quantity shown above each panel.

Figures 4(a) and 4(b) show the evolution of the RMS fluctuation amplitude of $Isat$ and $E\theta $. Both significantly increase following the transition, more strongly so in the inner half ($\rho \u22720.93$) of the examined region. Figures 4(c) and 4(d) show the intermittence of $Isat$ and $E\theta $. It decreases after the transition, mainly in the same region where the fluctuation amplitude increases.

Figure 4(e) shows the cross phase between $E\theta $ and $Isat$, calculated using the coherence technique (integrating over frequencies <50 kHz). At small values of $\rho \u22720.91$, the phase increases from around $\u2212\pi /2$ to $\u223c0$ or less across the transition. At larger values of *ρ*, the phase increases even more, similar to Fig. 1 (probe D), and reaches values $>\pi /2$ at the outermost positions. Black contours are drawn at multiples of $\pi /2$ to facilitate understanding. Before the transition, the radial phase profile is almost flat, but after the transition strong radial variation exists, such that the cross phase is maximal near $\rho \u22430.96$ and minimal near $\rho \u22430.88$. In the region of the transport barrier ($\rho \u22430.95$), the temporal variation of the RMS is only mild, whereas the temporal variation of the cross phase is very significant.

Figure 4(f) shows the poloidal phase velocity, calculated using the two-point correlation technique. It evolves from positive to negative across the transition, similar to Fig. 1, although values differ according to radius. The configuration of this probe did not allow calculating *E _{r}*.

From previous work, it is known that the line average electron density $ne\xaf$ plays the role of a control parameter for spontaneous confinement transitions at TJ-II.^{10} Figure 5 shows the Transfer Entropy (TE) between this parameter and various relevant quantities at different time lags (horizontal axis). It should be remembered that the vertical axis corresponds to the probe position, which was varied on a shot to shot basis.

Several things are immediately clear: (1) The TE values of the graphs $ne\xaf\u2192X$ are generally much larger than those of the graphs $X\u2192ne\xaf$, indicating that information flows from $ne\xaf$ to the other quantities, consistent with the idea that $ne\xaf$ acts as a control parameter. (2) Radial variation is significant. The largest values of TE are achieved around $\rho \u22430.95\u20130.96$, roughly where the transport barrier is formed.^{22} (3) The time lags corresponding to the maxima of TE are $\tau \u224325$ ms, which is of the order of the transition time.

We draw attention to the fact that the values of TE are very high compared to the maximum value possible [$\u2009log2(3)\u22431.6$]. Interestingly, the impact of $ne\xaf$ on the cross phase $\Delta \varphi coh(E\theta ,Isat)$ occurs earlier for $\rho \u22430.91$ than for $\rho \u22430.96$ [cf., Fig. 5(h)]. This is consistent with Fig. 4(e), where the phase change is seen to propagate outward following the transition time.

Figure 6 shows the TE between several selected quantities of interest. One particular variable is seen to have a significant causal impact: RMS($E\theta $), i.e., the turbulence level; it has a large impact on the cross phase $\Delta \varphi coh(E\theta ,Isat)$ [cf., Fig. 6(d)], significant impact on the intermittence, $C1(E\theta )$ [cf., Fig. 6(b)], and to a lesser degree on the poloidal phase velocity $v\theta $ [Fig. 6(f)]. Here also, the influence appears to occur earlier at more inward positions of the probe.

## V. DISCUSSION

The analysis performed here reveals the complexity of the dynamical interactions between turbulence and transport across the confinement transition. On the one hand, the plasma rapidly switches from electron to ion root conditions as the electric field is reversed.^{23} On the other hand, the increase in the electron density modifies the intrinsic dynamics of the turbulence by modifying the driving gradients. These two mechanisms (background transport and turbulence) dynamically interact in a complex way.

We study the evolution of several key variables, in particular the cross phase between $E\theta $ and $Isat$, appearing in the turbulent particle flux, $\Gamma =\u27e8E\u0303\theta n\u0303\u27e9/B$, providing new information regarding the transition process. First, key variables are visualized on a spatiotemporal grid in the relevant plasma edge region. Second, several additional quantities are studied to facilitate further understanding, namely, the intermittence and the transfer entropy. Here, it should be noted that the e- to i-root transition itself, marked by the change of sign of $v\theta $ and *E _{r}*, occurs fast, which does not allow extracting its impact from these analyses. However, it is possible to elucidate causal relations on the slower timescale of continuous variations across the transition, as exemplified in Fig. 1.

The line integrated density, $ne\xaf$, is the key control parameter for the transition. Increasing $ne\xaf$ implies a global increase in the density gradients, while the establishment of the edge transport barrier implies a local increase in the density gradients, both of which increase the turbulence drive; cf. the impact on RMS($E\theta $) in Fig. 5(d). It is interesting to note that this impact occurs first at inward positions and later at positions that are further outward.

The enhanced turbulence affects the cross phase $\Delta \varphi coh(E\theta ,Isat)$ [Fig. 6(d)] and causes $C1(E\theta )$ to drop [Figs. 4(c), 4(d) and 6(b)]. The latter implies that a dominant low-order helicity is growing (Fig. 2), which causes changes in $v\theta $ via Reynolds stress [Fig. 6(f)]. The poloidal flow velocity $v\theta $ is considered crucial for the actual transition.

The fact that $C1(E\theta )$ drops suggests that the sheared flow can at least in part be ascribed to the presence of low-order rational surfaces (e.g., $\iota \u2212=5/3$ at $\rho \u22431$ and $\iota \u2212=18/11$ at $\rho \u22430.86$).^{17} This idea might explain why the various quantities respond earlier at positions close to the inner part of the observational domain, $\rho \u22430.86$ ($\iota \u2212=18/11$): the transition would be initiated near that location. The interaction between turbulence and such dominant low-order modes, therefore, possibly plays a key role in the formation and maintenance of the sheared flow and the transport barrier.

The poloidal flow, $v\theta $, and cross phase, $\Delta \varphi (E\theta ,Isat)$, visualized in Figs. 4(e) and 4(f), respectively, appear to evolve in parallel. On physical grounds, the sheared flow (i.e., the shearing rate) is expected to be the key driving force of the change in the cross phase, even if the corresponding graphs of Fig. 6, the TE between $v\theta $ and $\Delta \varphi (E\theta ,Isat)$, are not very impressive. It should be noted, though, that both $v\theta $ and $\Delta \varphi (E\theta ,Isat)$ are the result of a certain level of numerical processing, which may obfuscate delicate causal relationships. In any case, the zone of maximum shearing rate [roughly, the light green band in Fig. 4(f)] is seen to propagate outwards prior to the consequential phase change. We note that the change in cross phase is very significant ($\u2273\pi /2$).

At the time of the transition, when $v\theta $ changes sign, a short-lived, large amplitude zonal flow structure is observed (Fig. 1), characterized by a significant deviation of *E _{r}* from $v\theta $. This temporal behaviour is similar to what has been observed elsewhere.

^{27}

After the transition, the plasma is in a new state (the ion root) and is maintained in that state by neoclassical requirements (ambipolarity).^{23} It is interesting to note that the changed cross phase is maintained at its new value (Fig. 1), associated with the new equilibrium profiles in the ion root state, in particular, the $v\theta $ or flow profile.

## VI. CONCLUSIONS

In this work, we have studied the spontaneous electron to ion root transition using Langmuir probe data in the plasma edge region, with both spatial and temporal resolution. The probe layout allowed studying a number of relevant quantities: turbulence amplitude [RMS($E\theta $) and RMS($Isat$)], *E _{r}*, $E\theta ,\u2009v\theta ,\u2009\Delta \varphi (E\theta ,Isat)$, as well as the intermittence $C1(E\theta )$ and $C1(Isat)$. The causal relation between the various quantities was studied using the transfer entropy.

It was found that the turbulence experiences significant simultaneous changes across the transition, as reflected by the evolution of all mentioned quantities (Fig. 1): The turbulence amplitude (RMS) and the cross phase ($\Delta \varphi $) increase, while the intermittence (*C*_{1}) drops. The spatiotemporal evolution obtained by varying the probe position ($0.87\u2264\rho \u22640.99$) in similar discharges (Fig. 4) shows, for example, that the cross phase $\Delta \varphi (E\theta ,Isat)$ changes first in inward positions and then propagates outward. The poloidal velocity $v\theta $ also experiences such an outward propagating change.

Analysis with the transfer entropy reveals that the line average electron density $ne\xaf$ acts as a control parameter of the transition, presumably indirectly, via the local density gradient that acts as a turbulence drive. Note that the edge density gradient roughly increases by a factor of 2, as reported in Ref. 22. The time delay between the density change and the response of the plasma is approximately 25 ms. Again, the change is seen to propagate outward (Fig. 5). Finally, the transfer entropy between various relevant turbulent quantities was studied, showing that the main drive is the turbulence amplitude RMS($E\theta $), which mainly impacts the intermittence $C1(E\theta $) and the poloidal velocity $v\theta $.

## ACKNOWLEDGMENTS

This work has been carried out within the framework of the EUROfusion Consortium and has received funding from the Euratom research and training programme 2014–2018 and 2019–2020 under Grant Agreement No. 633053 and project Y2018/NMT-4750 [PROMETEO-CM] Comunidad de Madrid. The views and opinions expressed herein do not necessarily reflect those of the European Commission. Research sponsored in part by the Ministerio de Ciencia, Innovación y Universidades of Spain under Project No. PGC2018-097279-B-I00. B.A.C. gratefully acknowledges support for the research from the DOE office of Fusion Energy under U. S. Department of Energy Contract No. DE-SC0018076.

## DATA AVAILABILITY

The data that support the findings of this study are available from the corresponding author upon reasonable request.