# Energetic‐Particle‐Driven Instabilities in General Toroidal Configurations

**ABSTRACT** Energetic-particle driven instabilities have been extensively observed in both tokamaks and stellarators. In order for such devices to ultimately succeed as D-T fusion reactors, the super-Alfvénic 3.5 Mev fusion-produced alpha particles must be sufficiently well confined. This requires the evaluation of losses from classical collisional transport processes as well as from energetic particle-driven instabilities. An important group of instabilities in this context are the discrete shear Alfvén modes, which can readily be destabilized by energetic particles (with velocities of the order of vAlfvén) through wave-particle resonances. While these modes in three-dimensional systems have many similarities to those in tokamaks, the detailed implementation of modeling tools has required development of new methods. Recent efforts in this direction will be described here, with an emphasis on reduced models (© 2010 WILEY-VCH Verlag GmbH & Co. KGaA, Weinheim)

**0**

**0**

**·**

**0**Bookmarks

**·**

**42**Views

- [show abstract] [hide abstract]

**ABSTRACT:**Energetic particle populations in magnetic confinement systems are sensitive to symmetry-breaking effects due to their low collisionality and long confined path lengths. Broken symmetry is present to some extent in all toroidal devices. As such effects preclude the existence of an ignorable coordinate, a fully three-dimensional analysis is necessary, beginning with the lowest order (equilibrium) magnetic fields. Three-dimensional techniques that have been extensively developed for stellarator configurations are readily adapted to other devices such as rippled tokamaks and helical states in reversed field pinches. This paper will describe the methods and present an overview of recent examples that use these techniques for the modeling of energetic particle confinement, Alfvén mode structure and fast ion instabilities.Physics of Plasmas 04/2011; 18(5):056109-056109-8. · 2.38 Impact Factor

Page 1

?? 1??

Notice: This manuscript has been authored by UT-Battelle, LLC, under Contract No. DE-AC05-00OR22725

with the U.S. Department of Energy. The United States Government retains and the publisher, by accepting the

article for publication, acknowledges that the United States Government retains a non-exclusive, paid-up,

irrevocable, world-wide license to publish or reproduce the published form of this manuscript, or allow others

to do so, for United States Government purposes.

Energetic particle-driven instabilities in general toroidal configurations

D. A. Spong1, B. N. Breizman2, D.L. Brower3, E. D’Azevedo1, C. B. Deng3, A. Konies4,

Y. Todo5, K. Toi5

1Oak Ridge National Laboratory, Oak Ridge, Tennessee, U.S.A.

2Institute for Fusion Studies, The University of Texas, Austin, Texas, USA

3Department of Physics, University of California, Los Angeles, CA, USA

4Max-Planck Institut für Plasmaphysik, EURATOM-Association, Greifswald, Germany

5National Institute for Fusion Science, Japan

e-mail address: spongda@ornl.gov

Key words: energetic particles, Alfvén eigenmodes, stellarator, toroidal plasmas, three-

dimensional effects

PACS: 52.55.Pi, 52.55.Tn, 52.35.Bj, 52.55.Hc

Abstract

Energetic-particle driven instabilities have been extensively observed in both tokamaks and

stellarators. In order for such devices to ultimately succeed as D-T fusion reactors, the super-

Alfvénic 3.5 Mev fusion-produced alpha particles must be sufficiently well confined. This

requires the evaluation of losses from classical collisional transport processes as well as from

energetic particle-driven instabilities. An important group of instabilities in this context are

the discrete shear Alfvén modes, which can readily be destabilized by energetic particles

(with velocities of the order of vAlfvén) through wave-particle resonances. While these modes

in three-dimensional systems have many similarities to those in tokamaks, the detailed

implementation of modeling tools has required development of new methods. Recent efforts

in this direction will be described here, with an emphasis on reduced models.

Page 2

?? 2??

1. Introduction

An improved understanding of energetic particle driven instabilities in three-dimensional

systems is motivated both by the difficulties they may cause as well as opportunities that may

be associated with these instabilities. In the former are concerns about first wall damage, the

negative impact of enhanced fast ion losses on heating efficiency [1] and thermal plasma

confinement. Under the topic of opportunities are the potential for new ways of inferring

diagnostic information via MHD spectroscopy [2] (e.g., i profile, fast ion density profile),

Alfvén mode driven transport barriers [3], bootstrap current profile shaping, possibilities for

stellarator shape optimization [4] of Alfvén instabilities, selective excitation of modes for ash

removal, and alpha channeling for direct ion heating [5]. All of these areas will require

development and experimental validation of improved modeling capabilities, ranging from

rapidly applied reduced models to more comprehensive first principles calculations. This

paper will describe the physics components that are necessary to understand the frequency

spectrum, mode structure and stability of energetic particle-driven Alfvén instabilities in

three-dimensional equilibria. These tools will be illustrated through applications to several

stellarator configurations

2. Alfvén-Sound continua

The existence of Alfvén modes possessing a global mode structure in toroidal systems can be

attributed to the poloidal (tokamak) and toroidal (stellarator + rippled tokamak) spatial

variations in the equilibrium magnetic field. In the case of a straight cylindrical plasma with

uniform magnetic field, the Alfvén spectrum is degenerate, as a result of the crossing of the

adjacent continuum ( ω2= k

remove this degeneracy and create frequency gaps at locations where the continua would

have intersected in the cylindrical limit. The first step in identifying experimentally observed

Alfvén modes is the correlation of measured frequencies with these gaps. A number of

models have been developed for the calculation of such continua in stellarators [6,7,8] and

generally provide reasonable agreement with frequency lines that are measured in

experiments, to within uncertainties related to imprecise knowledge of the i and density

profiles, average ion mass and Doppler shifts related to plasma flows.

2vA

2) lines. Variations of the magnetic field within flux surfaces

A topic of recent interest both for tokamaks [9,10] and stellarators [4,6,8,11] has been the

inclusion of sound wave couplings to the shear Alfvén continua. In a three-dimensional

system these couplings might be expected to become of importance when

km,n

mode numbers,

vA= B2/ µ0nionmion

(

⎡⎣

density, mion ion mass, Telectron,ion = electron/ion temperatures, Γ = adiabatic index, and Z = ion

charge state. Normally, the small size of Cs

minimize such couplings. However, due to differences in magnitude between the coupled

k's (especially in the case of stellarators where Δn = jNfp; j =1,2,...; Nfp= field period)

the Alfvén and sound continua can become coupled even at moderate values of βelectron. An

example of the overlapping of the sound continua with the Alfvén continua as βelectron is

2

vA

2≈ km+Δm,n+Δn

2

Cs

2 where Δm, Δn are the coupling intervals in the poloidal and toroidal

(

the

Cs= Γ ZTelectron+Tion

)/ mion

⎤⎦

)

1/2is Alfvén velocity and

1/2is the sound speed. Here µ0 = 4π × 10-7 H/m, nion = ion

2/ vA

2= 0.5 ΓZβelectronmight be expected to

Page 3

?? 3??

increased for an LHD discharge is illustrated in Fig. 1 based on using the STELLGAP model

[7] with acoustic couplings included.

Figure 1 – Coupled Alfvén-sound continua with increasing β for n = 1 modes in LHD. Pink curves

are dominated by acoustic (sound) couplings while blue curves are Alfvén dominated. Far right-hand

figure is a magnification of the β = 0.002 case showing small Alfvén-sound induced gaps.

For simplicity, the plots in this figure show only the n = 1 mode continua. Inclusion of

Alfvén-sound coupling effects in these continua introduces several new effects. One is the

existence of new gaps where the Alfvén and sound continua intersect (these are present on a

fine-scale in the case of Fig. 1). A second is the presence of a finite frequency minimum in

the coupled continua. The latter effect is illustrated in Fig. 2 for several time slices in an LHD

discharge [12] where a local minimum was present in the i profile. In this plot, couplings to

the acoustic mode have been included, but the sound continua have been removed for clarity.

The minima in the coupled Alfvén-sound continua of Fig. 2(b) generally agree with the

frequency minima measured experimentally. Alfvén-sound couplings can introduce new

eigenmodes near the minima of these continua, such as the BAAE [10,11] (beta-induced

Alfvén-acoustic eigenmode) and EGAM [13] (energetic-particle-induced geodesic acoustic

mode).

Figure 2 – (a) Reversed shear rotational transform profiles for two times in LHD RSAE discharge

(inset shows measured frequency spectrogram); (b) associated n = 1 shear Alfvén only continua

(lighter lines) and coupled Alfvén-sound continua (bolder lines).

Page 4

?? 4??

Sound wave coupling effects have also been studied in the HSX stellarator experiment [14].

In this device coupled sound-Alfvén modes were initially suspected. However, systematic

experimental variation of the rotational transform profile indicated that the observed

frequencies were insensitive to changes in i. This led to the conclusion that the ECH-

produced electron tail predominantly excited sound waves with only weak Alfvénic

couplings [14]. In Fig. 3 a sequence of n = 1 coupled Alfvén-sound continua are shown for

HSX equilibria with increasing i. The i variation causes frequency up-shifts in the central

m = 1, n = 1 Alfvén-sound gap to a greater degree than was observed in the experimental

frequency lines, suggesting that the observed modes were at least not associated with this

particular gap. As reported in ref. [14], sound waves existing in the m,n = 5,1 and 7,1

continua (large dots in Fig. 3) were consistent with the measured frequencies (dashed lines in

Fig. 3) and their scalings. The question remains as to why these specific modes, out of the

available multitude of sound and Alfvén waves were destabilized. In order to understand this

both the drive (from the energetic electron tail) and damping mechanisms (continuum, e,i

Landau, etc.) will need to be evaluated for the different modes in this frequency range; also,

other mechanisms, such as non-ideal effects (resistivity, viscosity) and sheared plasma flows

could influence the structure of these continua. These remain topics for future research.

Figure 3 – Variation of n = 1 coupled Alfvén-sound continua in HSX with central value of rotational

transform. Color-coding is used to indicate the strength of the sound vs. Alfvén components. Magenta

dashed lines indicate the experimental frequencies, which were not observed to change significantly

with variation in i.

3. Alfvén eigenmodes in stellarators

The next step in the analysis of Alfvén modes is the calculation of the eigenmode structures.

These are the eigenmodes of the ideal MHD operator. Such an approximation is appropriate

for modes that are weakly driven and near marginal stability. For this paper results from the

AE3D code [15] are used, which is based on a low β, reduced MHD model, and currently

does not include acoustic couplings. An efficient, solution technique has recently been

developed [15] that provides eigenmodes clustered about a user specified frequency; this

simplifies the process of sorting out modes that are likely to be more readily de-stabilized

(i.e., less affected by continuum damping). The targeted frequencies are likely to be readily

known either from experimental measurements or from the location of open gap regions in

the calculated continua. An example of such an eigenmode calculation for the NCSX

compact stellarator [16] is shown in Fig. 4. This is an HAE (helical Alfvén eigenmode) with

Page 5

?? 5??

strong poloidal and toroidal couplings. The continuum plot given on the left also shows

evidence of continuum-crossing gap structures [17], which are often present in the continua

of three-dimensional systems.

Figure 4 – (a) Strongly coupled n = 1 mode family continua (left figure) for NCSX compact

stellarator; (b) example of an HAE eigenmode with global radial structure (upper right figure); (c)

three dimensional mode structure in potential function (lower right figure).

4. Stability analysis using a wave-particle energy transfer method

The linear stability of Alfvén modes in stellarators has been addressed by both continuum

kinetic calculations [18] and more recently [19] using particle based methods. Due to the

large deviations of trapped and transitional particle populations in some stellarators, finite

orbit width effects (FOW) are expected to be of significance since they allow energetic

particles to sample the Alfvén mode structure over a larger radial width than if they were

confined close to fixed flux surfaces. These effects have been analyzed previously using

kinetic [20] methods. In order to address these issues using particles, a technique [19] has

been developed that evaluates the stability of a fixed, oscillating Alfvén mode by tracking the

accumulated wave-particle energy transfers between the wave and a large collection of test

particles. This method has been successfully benchmarked against a tokamak case for which

results are available from other codes. Several example applications to stellarators have been

made; Fig. 4 shows results from one such application to the LHD configuration. This was for

a case (not an experimental discharge) where the ion density was chosen to align the n = -1

gaps in radius, resulting in a rather global m, n = (2, -1) mode at 74.1 kHz with coupling to

(1, -1) and (3, -1) sidebands. In the left-hand plot of Fig. 5 the time variation of the growth

rate is plotted as the ratio of the average fast ion velocity to the Alfvén velocity is increased.

A distribution function that was Maxwellian in energy and beam-like in pitch angle [i.e.,

Page 6

?? 6??

f ∝δ(µ /ε)] was used here. As the plot shows, the growth rate function is initially

oscillatory for several wave periods as the particle markers acquire and average over resonant

perturbations from the wave. For later times the growth rate settles into a quasi-stationary

state with small oscillations that are presumably related to the various particle

bounce/precession/transit motions. A dual weight δf scheme has been developed that

removes the fixed driving frequency of the waves. The averaged growth becomes positive

(unstable) at around < vf> /vA ≈ 0.3 and increases with increasing < vf> /vA. In the right-

hand figure, the time-averaged growth rates are plotted vs. < vf> /vAfor both a beam and an

isotropic fast ion distribution, showing that they reach a maximum and then start to decrease.

This drop-off is caused both by the fact that for 〈vf〉 > vA the fast ion population is moving out

of Landau resonance (v|| = vA) with the wave and by the increasing FOW effects at the fast

ion energies associated with these parameters. The decreased growth rate for the isotropic

distribution vs. the beam distribution is also related to FOW effects and the greater dispersion

of particle velocities in the case of the isotropic distribution – resulting in a smaller fraction

of the distribution being in resonance with the wave.??

Figure 5 – (a) Time evolution of linear TAE growth rate for n = -1 mode family in LHD as a function

of <vf>/vA; (b) Dependence of time-averaged growth rates on <vf>/vA for beam-like and isotropic

distributions.

5. Conclusions

Development of the theoretical/computational techniques needed to understand energetic

particle-driven instabilities in three-dimensional systems is an important component of

stellarator physics and will be essential for the projection to future stellarator fusion reactors.

The basic steps in the analysis of such instabilities have been outlined here and consist of

calculation of the coupled Alfvén-sound continuum (identifies frequency windows where

such modes are likely), computation of eigenmode structures (useful for comparison with

experiment and perturbative stability analysis), and assessment of stability, including finite

orbit effects (allows mapping out unstable parameter regimes). In addition, the nonlinear

evolution of such instabilities and their impact on confinement must be considered and is a

Page 7

?? 7??

topic of current research. The techniques developed for energetic particle physics in

stellarators are also applicable to other three-dimensional systems, such as tokamaks with

symmetry-breaking effects [4] and self-organized helical states in reversed field pinches [21].

Acknowledgements?? –?? Research?? sponsored?? by?? the?? U.S.?? Department?? of?? Energy?? under??

Contract?? DE-‐AC05-‐00OR22725?? with?? UT-‐Battelle,?? LLC.??

?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ??

1?? M.?? Osakabe,?? S.?? Yamamoto,?? K.?? Toi,?? et?? al.,?? Nucl.?? Fusion?? 46,?? S911?? (2006).??

2?? S.?? E.?? Sharapov,?? D.?? Testa,?? B.?? Alper,?? et?? al.,?? Physics?? Letters?? A,?? Vol.?? 289,?? 127?? (2001).??

3?? ?? K.?? Toi,?? M.?? Isobe,?? K.?? Osakabe,?? D.?? Spong,?? et?? al.,?? submitted?? to?? Contributions?? in?? Plasma?? Physics??

(2009).??

4?? D.?? A.?? Spong,?? Y.?? Todo,?? L.?? A.?? Berry,?? et?? al.?? ,?? paper?? TH/3-‐4,?? 22nd?? IAEA?? Fusion?? Energy?? Conference,??

Geneva,?? Switzerland?? (Oct.,?? 2008).??

5?? A.?? I.?? Zhmoginov,?? N.?? J.?? Fisch,?? Phys.?? Plasmas?? 16,?? 112511?? (2009).??

6?? O. P. Fesenyuk, Ya. I. Kolesnichenko, H. Wobig, Yu. V. Yakovenko, International Workshop

“Innovative Concepts and Theory of Stellarators,” Kyiv, Ukraine, 28-31 May 2001, Kyiv, ISSN 1606-

6723, pg. 105 (2001).

7?? D.?? A.?? Spong,?? R.?? Sanchez,?? A.?? Weller,?? Phys.?? of?? Plasmas?? 10,?? 3217?? (2003).??

8?? A.?? Könies,?? D.?? Eremin,?? to?? be?? published?? in?? Physics?? of?? Plasmas.??

9?? B.?? N.?? Breizman,?? M.?? S.?? Pekker,?? S.?? E.?? Sharapov,?? Phys.?? of?? Plasmas?? 12,?? 112506?? (2005).??

10?? N.?? N.?? Gorelenkov,?? H.?? L.?? Berk,?? E.?? Fredrickson,?? et?? al.,?? Phys.?? Lett.?? A?? 370,?? 70?? (2007).??

11?? D.?? Eremin,?? A.?? Könies,?? to?? be?? published?? in?? Physics?? of?? Plasmas.??

12?? K. Toi, M. Isobe, M. Osakabe, et al., Fusion Science and Technology, LHD Special issue, to be

published (2010).??

13?? G.?? Y.?? Fu,?? Phys.?? Rev.?? Lett.?? 101,?? 185002?? (2008).??

14?? C.?? Deng, D. L. Brower, B. N. Breizman, D. A. Spong, et al., Phys. Rev. Lett. 103 103, 025003 (2009).??

15?? D.?? A.?? Spong,?? E.?? D’Azevdo,?? Y.?? Todo,?? submitted?? to?? Phys.?? Plasmas?? (2009).??

16?? M.?? C.?? Zarnstorff,?? L.?? A.?? Berry,?? A.?? Brooks?? et?? al.,?? Plasma?? Phys.?? Controlled?? Fusion?? 43,?? A237?? (2001).??

17?? Yu?? V.?? Yakovenko,?? A.?? Weller,?? A.?? Werner,?? et?? al.,?? Plasma?? Physics?? and?? Controlled?? Fusion?? 49,?? 535??

(2007).??

18?? A.?? Könies,?? Phys.?? Plasmas?? 7,?? 1139?? (2000).??

19?? D.?? A.?? Spong,?? A.?? Könies,?? conference?? proceedings?? of?? the?? 2009?? 11th?? IAEA?? TM?? on?? Energetic??

Particles?? in?? Magnetic?? Confinement?? Systems,?? Kyiv,?? Ukraine,?? Sept.?? 21-‐23,?? 2009.??

20?? Ya.?? I.?? Kolesnichenko,?? V.?? V.?? Lutsenko,?? A.?? Weller,?? et?? al.,?? Nucl.?? Fusion?? 46?? (2006)?? 753.??

Page 8

?? 8??

?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ?? ??

21?? ?? R.?? Lorenzini,?? E.?? Martines,?? P.?? Piovesan,?? et?? al.,?? Nature?? Physics?? 5,?? 570?? (2009).??

#### View other sources

#### Hide other sources

- Available from D. A. Spong · Jan 23, 2013
- Available from utexas.edu