• Classical Transport
• Pfirsch-Schlüter and Banana-Plateau Transport
• Ware Pinch
• Bootstrap Current
PhD Network, Garching, 28.9.2010
R. Dux

Usually, neoclassical (collisional) transport is small compared to the turbulent transport.
Neoclassical transport is important:
• when turbulent transport becomes small
- transport barriers (internal, edge barrier in H-modes)
- central part of the plasma, where gradients are small
• to understand the bootstrap current and the plasma conductivity
• transport in a stellarator (we do not cover this)
PhD Network, Garching, 28.9.2010
R. Dux

The gradients of density, temperature and electric potential in the plasma disturb the Maxwellian velocity distribution of the particles, which would prevail in thermodynamic equilibrium.
The disturbance shall be small.
Coulomb collisions cause friction forces between the different species and drive fluxes of particles and energy in the direction of the gradients.
Coulomb collisions drive the velocity distribution towards the local thermodynamic equilibrium and the fluxes try to diminish the gradients.
We seek for linear relations between the fluxes and the thermodynamic forces
(gradients).
We concentrate on the particle flux: 
 n u
PhD Network, Garching, 28.9.2010
R. Dux

The formulation of the neoclassical theory is based on fluid equations, which describe the time evolution of moments of the velocity distribution.
We arrive at moments of the velocity distribution by integrating the distribution function times v k over velocity space
0. moment: particle density n a
  f a d
3 v
1. moment: fluid velocity
 u a

1  n a
 f a v d
3 v
2. moment: pressure and viscosity p a
 a

 m a
3
Tr
 m a
 f a
  v

 u a
  v

 u
 a
 d
3 v
 n a k
B
T a f a
 v

 u
 a
  v

 u
 a
 d
3 v
 p a
I

3. moment: (random) heat flux
 q a
 m a
2
 f a
  v
 u
 a
  v

 u
 a
 d
3 v
PhD Network, Garching, 28.9.2010
R. Dux

Integrating the kinetic equation times v k over velocity space yields the equations of motion for the moments of the velocity distribution (MHD equations)
0. moment: particle balance (conservation)
 n a
 t
 
 n a
 u a


0

C ab d
3 v

0
1. moment: momentum balance m a n a d u
 a dt
 m a n a


 u
 a
 t

 u
 a
 
 u
 a


 e a n a
 
E

 u a


B

  p a
    a
 b

 a

F ab

F ab
  m a
 v C ab d
3 v
   m b v

C ba d
3 v
 

F ba
In every equation of moment n appears the moment n+1 and an exchange term due to collisions (here: momentum exchange, friction force)
PhD Network, Garching, 28.9.2010
R. Dux

The force on particle a with velocity v a v b averaged over all impact parameters due to collisions with particles b with velocity d
 p ab dt
  e a
2 e b
2 ln
4

0
2
 m ab ab
 v a
 v a


 v b
 v b
3 n b
 
A ab
 v ab
 v ab
3 n b
A ab
 e a
2 e b
2 ln
4

0
2
 m ab ab v y
• formally equal to the attractive gravitational force
(in velocity space) f a • This result for point like velocity distributions can be extended to an arbitrary velocity distribution f particles b using a potential function h. b of v x d
 p ab dt
 
A ab
 v
 h ( v ) h ( v

)
  v

1

 v b f b
  b d
3 v b f b
The average force density on all the particles a with velocity distribution f a obtained by integrating the force per particle over the velocity distribution

F ab
 
A ab
 f a
 
 v
 h ( v ) d 3 v is
PhD Network, Garching, 28.9.2010
R. Dux

For undisturbed Maxwellian velocity distributions with thermal velocity v
T f
0
( v )


3 / n
2 v
T
3 exp

  v v
T
2
2

 v
T

2 k
B
T / m
The friction forces are zero.
For Maxwellian velocity distributions with small mean velocity u<<v
T f ( v )


3 / n
2 v
T
3 exp




  v
 v
2
T
 u

2


 u
 v
T f
0
( v )

 1

2
 v v
2
T
 u


 the average force density on the species a due to collisions with b is.

F ab
 m a n a
 ab
  u b

 u a

 

F ba
The collision frequency is for T a
=T b
:
 ab

4 2

3 ( 4

0
)
2 e a
2 e b
2 m ab
 
B
T
3 / ln
2
 ab n b m a
PhD Network, Garching, 28.9.2010
R. Dux

• In every equation of moment n appears the moment n+1.
• At one point one has to close the fluid equations by expressing the higher order moments in the lower ones
• In neoclassical theory one considers the first four moments : density, velocity, heat flux, ???-flux
• To estimate classical particle transport we use a simple approximation and just care about density and velocity ( first two moments )



F ab

0 a

 m a n a
 ab
  u b

 u a
 momentum balance m a n a d
 u a dt
 e a n a
 
E

 u a


B

  p a
 b

 a m a n a
 ab
 u
 b
 u
 a

PhD Network, Garching, 28.9.2010
R. Dux

momentum balance m
 a d
 u a n a
 dt
O (
 3
)
We assume :
 e
 
 
E

 u
O a
(


)

B


 p a
  b
 m
 a n a

 ab

  u
 b


 u a


O (
 2
)
• the strong magnetic field limit (magnetized plasma)
• to be close to thermal equilibrium  
 a

L n , T
 ca v
Ta
L n , T
• temporal equilibrium




1 a
 ca

 a m a e a
B

1
Expand fluid velocity
 u a

 u a
( 0 ) 
 u a
( 1 )
Lowest order of

: no friction
0
 e a n a
 
E

 u a
( 0 ) 

B

  p a
Next order of

: include friction with lowest order fluid velocities
0
 e a n
 a u a
( 1 ) 

B
 b

 a m a n a
 ab
  u b
( 0 ) 
 u a
( 0 )

PhD Network, Garching, 28.9.2010
R. Dux

zero order
0
 e a n a
 
E

 u a
( 0 ) 

B

  p a first order
0
 e a n
 a u a
( 1 ) 

B
 b

 a m a n a
 ab
  u b
( 0 ) 
 u a
( 0 )
 u
 a
( 0 ) 

B
 

E

 p a e a n a
 u a
( 1 ) 

B
 
Cross product with B-field yields perpendicular velocities: m a e a b

 a

  ab

 u
 b
( 0 )

B

 u
 a
( 0 )

 u

B
2

 u
( 0

,
) a


E


B
B 2

 p a


B e a n a
B 2
 u (

1
,
) a
 m a e a
B
2 b

 a
 ab
  u b
( 0 ) 

B
 u
 a
( 0 ) 

B

ExB drift + diamagnetic drift
 u
(

1
,
) a
 m a e a
B 2
 b
 a
 ab


 p b e b n b

 p e a n a a


Velocity in direction of pressure gradients
(ExB drops out, friction only due to diamagnetic drift)
PhD Network, Garching, 28.9.2010
R. Dux

zero order
 u
(

0 )
, a


E

B
2

B
 j
( 0

) 

 p a


B
 a e a n a u

(

0
,
) a

2 e a n a
E


B
B 2
 e a n a
 

0 Quasineutr ality
  a
 p a
B 2


B
 
 p


B
B 2
  p


 j
( 0 ) 

B
The zero order perpendicular current is consistent with the MHD equilibrium condition.
first order e a n a
 u
( 1 ) a


B e a n a
 u
(

1
,
) a

1
   b
 a m a n a
 ab
  u b
( 0 )
B 2 b

 a

F ab


B

 u a
( 0 )

   b
 a

F ab
 j
(

1 )   a e a n a u

(

1 )
, a

1
B 2
 a b

F ab

0 momentum conservati on


B

0
The first order perpendicular current is zero. The fluxes are ambipolar.
PhD Network, Garching, 28.9.2010
R. Dux

The position of the gyro centre and the gyrating particle are related by.
r
 gc
 r


 p
 qB 2

B
A collision between a and b changes the direction of the momentum vector and the position of the gyro centre changes by.
 r
 a gc 

 p e a a
B

2

B momentum conservati on


 p b
 e a
B
2

B
  e e b a
 r
 b gc
The displacement is ambipolar.
e a
 r
 a gc  e b
 r
 b gc 
0
No net transport for collisions within one species
( F aa
=0 in the fluid equation ).
 r
 a gc   r
 b gc 
0
The same argument does not hold for the energy transport
(exchange of fast and slow particle within one species).
PhD Network, Garching, 28.9.2010
R. Dux

 u (

1
,
) a
 m a e a
B
2
 b
 a
 ab


 p b e b n b

 p a e a n a

 p a
 n a k
B
T a
T a

T b

T
The radial particle flux density is thus (for equal temperatures):
 a
 n a m e a a k
B
B
2 b

 a
 ab

 n b

T

T
 n b e b n b
 n a

T e a
 n a
T
 n a


 m a k
B
T e a
2
B
2 b

 a
 ab
  n a
 n a e a e b
 n b n b


T
T

 1
 e e a b


It has a diffusive part and a convective part like in Fick’s 1st law:

 a
 
D a
CL
 n a
 v a
CL n a
The classical diffusion coefficient is identical to the diffusion coefficient of a ‘random walk’ with Larmor radius as characteristic radial step length and the collision frequency as stepping frequency. a
D
CL
 m a k
B
T e a
2
B
2 b

 a
 ab
 k
B
T e a
2
B
2 m a m a
2 b

 a
 ab

2 v
Ta
2

2 ca b

 a
 ab

 a
2
2
 b
 a
 ab a
D
CL

 a
2
 a
2
PhD Network, Garching, 28.9.2010
R. Dux

 a
 e a
B
 u dia , a v
Ta


2 k
B
T a m a e a
B

 p a


B e a n a
B
2 m a
Diamagnetic velocity depends on the charge and causes friction between different species, that drive radial fluxes.
PhD Network, Garching, 28.9.2010
R. Dux

D a
CL
 m a k
B
T e a
2
B
2 b

 a
 ab
 ab

4 2

3 ( 4

0
)
2 e a
2 e b
2 m ab
 
B
T
3 / ln
2
 ab n b m a a
D
CL

4 2

3 ( 4

0
)
2
B
2
1
 
B
1 / 2 b

 a m ab ln
 ab e b
2 n b
• The classical diffusion coefficient is (nearly) independent of the charge of the species.
• In a pure hydrogen plasma D
CL is the same for electrons and ions.
• For impurities, collisions with electrons m ae
 m e can be neglected compared to collisions with ions.
• The diffusion coefficient decreases with 1/B 2 due to the quadratic dependence on the Larmor radius
Our expression for the drift is still not the final result, since the friction force from the shifted Maxwellian is too crude ...
PhD Network, Garching, 28.9.2010
R. Dux

f
0
( v )
 n

3 / 2 v
T
3 exp

  v
2

 v
T
2 v
T

2 k
B
T / m r
L
 v
 c
The B-field shows in the y-direction. All gyro centres on a
Larmor radius around the point of origin contribute to the velocity distribution. There shall be a gradient of n and T in the x-direction. x gc
 v z
 c z x
 n

T
B
We calculate the perturbation by an expansion of the Maxwellian in the x-direction: f
 f
0


 f x
0 x

0 x gc
 f
0


 f x
0 x

0 v
 z c
 f
0
 f
1 old f
1
 f
0

 n ' n

3
2
T '

T v
2 v
T
2
T '
T

 v z
 c
 f
0 u dia


 v v
T
2
2

5
2

 k
B
T ' e a
B
2 v z v
T
2 f
1
 f
0
2 v z u dia v
T
2
The perturbation of the Maxwellian has an extra term besides the diamagnetic velocity, which we have neglected so far. It leads to the diamagnetic heat flux and an extra term in the friction force, the thermal force.
PhD Network, Garching, 28.9.2010
R. Dux

 q
(

0 )
, a
 
5
2 p a k
B

T a e a
B
2

B
This leads to new terms in the friction force which are proportional to the temperature gradient and are called the thermo-force.

F

, ab
  m a n a
 ab




 e b p n b b


 e a p n a a slipping force (diamagn.
velocity)

3 k
B


T



 e m b ab m b 
 e m a ab m a


 thermo force (diamagn.
heat flux)






B
B
2
Ion-ion collisions, equal directions of
 p and

T :
For m a
>m b
 the thermo-force is in the opposite direction than the
 p-term
Also for a simple hydrogen plasma the two forces are opposite.

F

, ei
  m e n e
 ei
 n p

3
2 k
B

T


B
B
2
PhD Network, Garching, 28.9.2010
R. Dux

The reason for thermal force is the inverse velocity dependence of the friction force:
Collisions with higher velocity difference are less effective than collisions with lower velocity difference.
This lowers the friction force due to the differences in the diamagnetic velocity.
PhD Network, Garching, 28.9.2010
R. Dux

 a
CL
  n a
 ab  b
 a
D
CL n a
 b
 a
D ab
CL e a e b
 n b n b


T
T



3 m ab
2 m b

1
 e b e a


3 m ab
2 m a


1




D ab
CL

 a
2
 ab
2
For a heavy impurity in a hydrogen plasma (collisions with electrons can be neglected):

Z
CL


2
Z

2
ZH 


  n
Z
 n
Z
Z


 n n
H
H

1
2

T
T





In equilibrium the impurity profile is much more peaked than the hydrogen profile (radial flux=0) inward outward (temperature screening)
 n
Z n
Z

Z


 n
H n
H

1
2

T
T


For a pure hydrogen plasma:
 e
CL

 e
2
 ei
2
  n

 n

 n n

1
2

T
T
 e
2
 ei
  i
2
 ie

 e
2
 ei
2

2
 n
 n
2

T
T

 i
CL ion and electron flux into the same direction and of equal size!
PhD Network, Garching, 28.9.2010
R. Dux

PhD Network, Garching, 28.9.2010
R. Dux

Similar:
•Classical and neo-classical particle fluxes have the same structure:
- diffusive term + drift term
- larger drift for high-Z elements (going inward with the density gradient)
- temperature screening
• The neo-classical diffusion coefficients are just enhancing the classical value by a geometrical factor.
Different:
• A coupling of parallel and perpendicular velocity occurs due to the curved geometry.
• The neo-classical transport is due to friction parallel to the field (not perpendicular).
• additional effects due to trapped particles: bootstrap current and Ware pinch
PhD Network, Garching, 28.9.2010
R. Dux

Helical field lines trace out magnetic surfaces.

B

RB t
   e t
  
( R , Z )

 e t the poloidal flux is 2
 and |

|=RB p
• The safety factor q gives the number of toroidal turns of a field line during one poloidal turn.
• The length of a field line from inboard to outboard is:  qR
• The transport across a flux surface is much slower than parallel to B.
• We assume constant density and temperature on the flux surface.
PhD Network, Garching, 28.9.2010
R. Dux

Density and temperature are (nearly) constant on a magnetic flux surface due to the much faster parallel transport and the transport problem is one dimensional.

 t n
   
We calculate the flux surface average of a quantity G
G

1

V


V
GdV

1

V


V
G
 r
 dS

 

V


V
G
  dS
G




V
 



1
 G
  dS

1
V '
 G
  dS
Tokamak:
  
RB p dS

Rd
 dl p
G

2

V '
 G
B p dl p
PhD Network, Garching, 28.9.2010
R. Dux

 n
 t
   
G

1
V '
 G
  dS
The average of the divergence of the flux is calculated using Gauss theorem:
V
  

 dV
 

 d

S
 


 
  dS

V '

  
 

 

 V '

  


 V '

  
   

V

V '

  

V '
   
V '
 

  






The one dimensional equation is then:
 n
 t
 
1
V '

 

V '

 

We have to determine the surface averages:

  
 q
  which are linear in the thermodynamic forces
 p a
  n a

T a
 
PhD Network, Garching, 28.9.2010
R. Dux

Take the toroidal component of the momentum equation, multiply with R and form a flux surface average. This leads to an expression for the radial flux due to toroidal friction forces:
 a
  
1 e a b

 a
RF ab , t

1 e a b

 a





F ab , ||
RB
 t
  neoclassic al transport

RB p
F ab ,

   classical transport





 e t

B t
B
 e
||

B p
B
 e

We need to know the differences of the parallel flow velocities to get the friction forces.
We can calculate this term by just forming the flux surface average from the old result
The classical diffusion flux with correct flux surface average:

 a
 
CL Diffusion
 
R 2 B p
2
B
2 m a k
B
T e a
2
 n a
  b

 a
 ab
PhD Network, Garching, 28.9.2010
R. Dux

One contribution two the parallel flows arises from the divergence of the diamagnetic and ExB drift:
 u
(

0 )
, a


E


B
B
2

 p a


B e a n a
B
2
 
 
 
 
B
2


B

 p a
 
  

B e a n a
B
2
  a
  

B
B
2
 a
 
 
 

1 e a n a
 p
  a pressure and particle density and electric potential are in lowest order constant on flux surface
  u

(

0
,
) a





 
 a
2
 
 

0
 






B

2
 a

2 u

(

0
,
) a


B
B

B
3
B
  
  a

B
 
 
1
B
2
  
 


B


 a
 
2
 
B 

0







B



  

B



B




0
 
   




0
 j

B


0
PhD Network, Garching, 28.9.2010
R. Dux

From the continuity equation:
 n a
 t
  
 n a u

(

0
,
) a

  n a
 
 u (

0
,
) a and the divergence of the diamagn. drift
  u

(

0
,
) a

 n t a

2
 n a

2
 u (

0
,
) a u

(

0
,
) a


B
B

B
B u di u de we find, that ions pile up on the top and electrons on the bottom of the flux surface (reverses with reversed B-field).
In the particle picture this is found from the torus drifts (curvature, grad-B drift).
This leads to a charge separation.
PhD Network, Garching, 28.9.2010
R. Dux

The separation of charge leads to electric fields along the field lines and a current is driven which prevents further charge separation.
Parallel electron and ion flows build up to cancel the up/down asymmetry.
The parallel and perpendicular dynamics are coupled.
The remaining charge separation leads in next order to a small ExB motion and causes radial transport.
PhD Network, Garching, 28.9.2010
R. Dux

A similar effect appears for the diamagnetic heat flow, which causes temperature perturbations inside the flux surface which is counteracted by parallel heat flows leading in higher order to a radial energy flux.
PhD Network, Garching, 28.9.2010
R. Dux

diamagnetic velocity
 u (

0
,
) a
  e a
1 n a

 p
 a
RB
B p
 e

PfirschSchlüter velocity
 u
( 0 )
||, a
 e a
1 n a
 p a
 
RB
 u
||,
( 0 a
)

B
 t



0
1
B

B
B
2



 e
|| form of total velocity (divergence free)
 u
( a
0 )  
R
 e t

K B
• not completely determined u
ˆ

B B this is also divergence free since div( B )=0
• it is caused by trapped particles ( 
Banana-Plateau transport)
PhD Network, Garching, 28.9.2010
R. Dux

PfirschSchlüter velocity
 u
||,
( 0 ) a

1 e a n a
 p a
 
RB t



1
B

B
B
2



 e
||

 a
  
1 e a
We use the shifted Maxwellian friction force and calculate the radial flux
 a
 
PS

  t
2



1
B 2

1
B 2


 m a n a e a b

 a
 ab


1 e b n b
 p b
 

1 e a n a
 p a
 


RB t
 b
 a
F ab , ||
B
The result has the same structure as in the classical case. The fluxes are enhanced by a geometrical factor.
g
PS

R
2
 
B
2 p t
2
B
2



1
B
2

1
B
2



For concentric circular flux surfaces with inverse aspect ratio

=r/R g
PS
 q 2
1


2

2
1
 
1

1

3


2
2
2
 
2 q 2

1

39
16

2 
29

4
8

...
The PfirschSchlüter flux is a factor 
2q 2 larger than the classical flux.
PhD Network, Garching, 28.9.2010
R. Dux

The PfirschSchlüter velocity
 u (
||,
0 ) a

1 e a n a
 p a
 
RB t



1
B

B
B
2



 e
|| changes its direction at the top/bottom of the flux surface.

Also the radial fluxes change direction.
The flux surface average is the integral over opposite radial fluxes at the inboard/outboard side.
the flux vectors can also show inward/outward at the outboard/inboard side
R. Dux PhD Network, Garching, 28.9.2010

Temperature screening in the PfirschSchlüter regime similar to classical case:
• consequence of the parallel heat flux, which develops due to the non-divergence free diamagnetic heat flux.
• temperature screening is reduced for strong collisional coupling of temperatures of different fluids ( that happens typ. for T < 100eV )
- energy exchange time comparable to transit time on flux surface
- up/down asymmetry of temperatures reduced due to collisions
- weaker parallel heat flows
- reduced or even reversed radial drift with temperature gradient
PhD Network, Garching, 28.9.2010
R. Dux

For the CL and PS transport, we were just using the fact, that the mean free path is large against the Larmor radius (
 a
<<
 ca
)
The mean free path increases with T 2 and can rise to a few kilometer in the centre. Thus, we arrive at a situation, where the mean free path is long against the length of a complete particle orbit on the flux surface once around the torus.
The trapped particle orbits become very important in that regime, since they introduce a disturbance in the parallel velocity distribution for a given radial pressure gradient. This extra parallel velocity ‘shift’ will lead to a new contribution in the parallel friction forces and to another contribution to the radial transport, the so called Banana-Plateau term.
PhD Network, Garching, 28.9.2010
R. Dux

Conservation of particle energy and magn. moment
E

1
2 mv
||
2 
1
2 mv 2

  mv 2

2 B leads to particle trapping.
At the low field side, v
|| v
||
2  2 v
|| LFS
 has a maximum.
v
2

LFS

 1

B
B
LFS


For a magnetic field of the form
B

1
 r
B
0 cos

/ R
0

1
 
B
0 cos
 v
|| becomes zero on the orbit for all particles with v
|| v

LFS

1

B
HFS
B
LFS

1

1

1




2

PhD Network, Garching, 28.9.2010
R. Dux

The fraction of trapped particles is obtained by calculating the part of the spherical velocity distribution, which is inside the trapping cone.
f t

1

3 B
2
4
 1 /
0
B max
 d
1



B
  
1 .
46

0 .
46
 
In all these estimates the inverse aspect ratio

=r/R is considered to be a small quantity.
 
1 .
46

0 .
46
  f t f t only depends on the aspect ratio.
PhD Network, Garching, 28.9.2010
R. Dux

The bounce movement together with the vertical torus drifts leads to orbits with a banana shape in the poloidal cross section.
The trapped particles show larger excursions from the magnetic surface, since the vertical drifts act very long at the banana-tips.
On the outer branch of the banana the current carried by the particle is always in the direction of the plasma current (co).
PhD Network, Garching, 28.9.2010
R. Dux

Conservation of canonical toroidal momentum p

 m a
Rv

 e a
  const yields for low aspect ratio an estimate for the radial width of the banana on the low-field side
2 m a
Rv

 e a
  v

 v
||
  v
T

2 m a
Rv

 e a
RB p w b

0 w b
  v
T e a
B p m a
   p
The width scales with the poloidal gyro radius (= Larmor radius evaluated with the poloidal field).
PhD Network, Garching, 28.9.2010
w b
R. Dux

v
||, t
  v
T n t n
  w b
  v
T e a
B p m a
Consider a radial density gradient.
• On the low-field side, there are more co-moving trapped particles than counter moving particles, leading to a co-current density
• effect is similar to the diamagnetic current n t u
||
 v
||, t w b dn t dr
  v
T
 v
T eB p m
 dn dr
 
3 / 2
1 eB p dp dr
The banana current is in the co-direction for negative radial pressure gradient: dp/dr < 0.
Collisions try to cancel the anisotropy in the velocity distribution.
PhD Network, Garching, 28.9.2010
R. Dux

The velocity vector is turned by pitch angle scattering.
The collision frequency is the characteristic value for an angle turn of

1:
 a
  b
 ab
To scatter a particle out of the trapped region it needs on average only an angle

. Due to the diffusive nature of the angle change by collisions the effective collision frequency is:
 a , eff


 a
 
2


 a
The distance from LFS to HFS along the field line is: L
 qR
A passing particle with thermal velocity v
Ta needs a transit time:
A trapped particle has lower parallel velocity and needs the longer bounce time:

B


T

 qR
 v
Ta

T
 qR v
Ta
PhD Network, Garching, 28.9.2010
R. Dux

The collisionality is the ratio of the effective collision frequency to the bounce frequency

* a

 a , eff
 b


 a qR
0
 v
Ta

 a qR
0 v
Ta
 
3 / 2  qR
0
 mfp , a
 
3 / 2

1
 a
*
*  a
 
1

* a

 

3 / 2

3 / 2 low : banana medium : plateau high : Pfirsch Schlüter
 a
* 

3 (
4
4 .
9
4

0


)
10

2
24
R
0 q
 
3 / 2 e a
2
 
B
2
R
0

T
  q

 

3

2
/ 2
Z
2 a m a
1 m a
 b
 b m ab m ab ln ln
 ab e b
2 n b
 ab
Z b
2 n b
• The summation includes a.
• higher collisionality for high-Z.
• strong T-dependence
PhD Network, Garching, 28.9.2010
e, H @ center e, H @ edge
Imp @ center
Imp @ edge banana plateau plateau
PS
R. Dux

If the collisionality is in the banana regime, we can estimate the diffusion coefficient. The diffusion is due to the trapped particles.
D
BP
 n t
 eff n
 
2 n t
 eff n





 r
 w b
   p
 q


D
BP
 



 q




2
 q 2

3 / 2
D
CL
In the banana regime the transport of trapped particles dominates by a large factor. This banana-plateau contribution becomes small at high collisionalities.
This estimate works only if the step length (banana width) is small against the gradient length.
PhD Network, Garching, 28.9.2010
R. Dux


Simple model for banana regime:
The loss of trapped particles into the passing domain creates a force density onto the passing particles
F t
 p
  eff m a n t u
|| a , t
 m a

 a

3 / 2
1 dp a eB p dr
The passing particles loose momentum to the trapped particles in a fraction n t
/n of all collisions
F p
 t
   a m a n a u
|| a
F

F t
 p

F p
 t
   a m a n a
1 en a
B p dp a dr
 u
|| a
  a
1 en a
B p dp a dr
 u
|| a
In the fluid equations, this is the contribution of the viscous forces to the parallel momentum balance. The contribution increases with the collision frequency in the banana regime and decreases with 1/
 in the PS regime.
PhD Network, Garching, 28.9.2010
R. Dux

 u
(
||, a
0 ) 
1 e a n a
 p a
 
RB t



1
B

B
B 2



 e
||
 u
ˆ a
B
B 2
 e
||

 a
  
1 e a
RB t
 b
 a
F ab , ||
B
This integration constant û of the parallel fluid velocity is calculated from the flux surface averaged parallel momentum balance.
B

   ˆ a

||

BF a ||
The PS flow drops out and one gets a system of equations for the û
(here it is written for the shifted Maxwellian approach):
 a

 ˆ a

RB t
1 e a n a
 p a
 

   b
 a m a n a
 ab
 u
ˆ b
 ˆ a

Thu û are functions of the viscosity coefficients, collision frequencies and the pressure gradients. Once a solution has been obtained, one can calculate the banana-plateau contribution to the radial transport.
 a
  
1 e a
RB t
B
2 b

 a m a n a
 ab
 u
ˆ b
 u
ˆ a

PhD Network, Garching, 28.9.2010
R. Dux

We calculate the û for a Hydrogen plasma using the simple viscosity estimate in the case of low collisionality.
   ee
  ei


 u
ˆ e

RB t en
 p
  e


  ei
 u
ˆ i
 u
ˆ e

  ei

 u
ˆ e

RB t en
 p e
 


  ei
 u
ˆ i
 u
ˆ e

   ii
  ie


 u
ˆ i

RB t en u
ˆ i
 ˆ e

1



RB t en
 p i
 


  ie
 u
ˆ e
 u
ˆ i


 p e

  p i


 u
ˆ i

RB t en
 ei
  ee
 p
  i



0
 ii
  ee m e m i
 ie
  ei m e m i
 e
 
BP

1 e
RB t
B 2 m e n
 ei
 u
ˆ i
 u
ˆ e


1



  t
2
B 2 m e
 ei e 2
 p
 
This flux has the same form as the classical hydrogen flux enhanced by a rather large geometrical factor: g
BP

B
2

R
 
2
B
2 p t
2
B
2



2 q 2

 q 2
3 / 2
This is just the same estimate, we got with our random walk arguments.
For large collisionalities the viscosity decreases with collision frequency and the banana-plateau flux becomes small.
PhD Network, Garching, 28.9.2010
R. Dux

The difference of the û for a Hydrogen plasma from the simple viscosity estimate yields a parallel current.
j
||
 en
 u
ˆ i
 u
ˆ e
 B
B
2 u
ˆ i
 u
ˆ e

1



RB t en

 p e

  p i
 j
||

ˆ j B
B
2

1



RB t
B
B
2
1
RB p
 p
 r


B p
 p
 r
This is the a very rough estimate for the bootstrap current density. It is a factor of 1/
 larger, than the banana current which is initiating the bootstrap current of the passing particles. j
||, banana
 en t u
||, t
 
3 / 2
1 dp
B p dr
A better expression correct to order
 j bs


B p
2 .
44 k
B

T e

T i

 n
 r

0 .
69 nk
B

T e
 r

0 .
42 nk
B

T i
 r
Finally, a dependence on the collisionality has to enter .
PhD Network, Garching, 28.9.2010
R. Dux

Trapped particles do not carry any current.
Only the force on the passing particles generates a current.
n

 
 p
 n 1
Momentum is lost by collisions with ions or by collisions with trapped particles.
du
|| dt
   ei u
||
   ee u
||
These two effects lead to a neo-classical correction on the Spitzer conductivity due to the trapped particles.
  
SP


1

1


C

*


2
The corrections disappear for high collisionality of the electrons.
PhD Network, Garching, 28.9.2010
R. Dux

Conservation of canonical toroidal momentum p

 mRv

 e a
  const
At the banana tips, the toroidal velocity is zero. All turning points of the banana are on a surface with
  const
The movement of this surface of const.
flux yields a radial movement of the banana orbit.
d
 dt

 
 t

 v

   
RE t induced electric field

 v

RB p
    ware
(

*
) f t n
E t
B p
The Ware pinch is much larger than the classical pinch: v
E

E t
B p
B 2
PhD Network, Garching, 28.9.2010
• co: acceleration
• counter: de-acceleration
• no equal stay above/below equator
• radial drifts do not cancel
R. Dux

The total radial flux induced by collisions is a sum of three contributions: classical(CL) , PfirschSchlüter(PS) and banana-plateau (BP) flux.
    x

 
CL, PS, BP b
 a
D ab x





 n
 a

Diffusion
 e a

 e b  n
1

 n

 b

H
   
Drift ab x
1

T


 n a



 
 temperature screening
For low collisionalities the BP-term dominates at high collisionalities the
PS-term.
For each term the drifts increase with the charge ratio times the diffusion coefficient.
There are numerical codes available to calculate the different contributions
(NCLASS by W. Houlberg, NEOART by A. Peeters).
PhD Network, Garching, 28.9.2010
R. Dux

D coll

D
CL

D
PS

D
BP
D a
CL

 a
2
 a
2
D
BP

 q
2
3 / 2
D
CL
D
PS
 q
2
D
CL
BP contribution decreases in plateau regime and is zero in
PS regime:
D
BP at

*=1 is roughly equal to D
PS at

*=

-3/2
Thus, there is a collisionality region with roughly constant D (plateau regime).
PhD Network, Garching, 28.9.2010
R. Dux

change of collisionality by change of T at a fixed position n
He , Si
 n e
T n e


 n
0 .
D

05
1

 20
10
50 m
 keV

3 q

2 .
5
ε 
0 .
24
B t

2 .
5 T f trap

0 .
62
PhD Network, Garching, 28.9.2010
R. Dux

ITER-FDR (old)
R

8 .
45 m n e

1

10
20 m
T ( 0 )

32 keV

3 q
95
B t


3
5 .
7 T
ASDEX Upgrade
R

1 .
65 m n e

1

T ( 0 )

10
20
2 .
5 m

3 keV q
95
B t


3 .
3
2 .
5 T
PhD Network, Garching, 28.9.2010
R. Dux

• near the axis the banana width is assumed to be small against the radial distance to the axis
• for very strong gradients, with gradient length smaller than the banana width
• for high-Z impurities in strongly rotating plasmas, with toroidal Mach numbers >> 1
- leads to asymmetries of the density on the flux surface
• ...
PhD Network, Garching, 28.9.2010
R. Dux

PhD Network, Garching, 28.9.2010
R. Dux

(Neo-)classical transport can be explained by the combination of particle orbits and
Coulomb collisions
The particle density in phase space is given by a velocity distribution d
6
N
 f a
  x ,
 v , t
 d
3 x d
3 v
The kinetic equation is the Fokker-Planck equation
 f
 t a

 v
 f

 a x
 e a m a
 
E

 v


B
  f

 a v
  b
C ab
 f a
, f b

Collision operator the time derivative along the particle orbit prescribed macroscopic fields
The electric and magnetic fields are static and only fluctuations with a length scale smaller than the Debye length are considered. These fluctuations are considered within the collision operator.
PhD Network, Garching, 28.9.2010
R. Dux