Pauli–Lubanski pseudovector

For the notation, see Ricci calculus.

Quantum field theory
Feynman diagram
History
Background Field theory Gauge theory Poincaré symmetry Quantum mechanics Spontaneous symmetry breaking
Symmetries Charge conjugation Crossing Parity Time reversal Symmetry in quantum mechanics
Tools Anomaly Effective field theory Expectation value Faddeev–Popov ghosts Feynman diagram Lattice gauge theory LSZ reduction formula Partition function Propagator Quantization Regularization Renormalization Vacuum state Wick's theorem Wightman axioms
Equations Dirac equation Klein–Gordon equation Proca equations Wheeler–DeWitt equation Bargmann–Wigner equations
Standard Model Electroweak interaction Higgs mechanism Quantum chromodynamics Quantum electrodynamics Yang–Mills theory
Incomplete theories Quantum gravity String theory Supersymmetry Technicolor Theory of everything
Scientists C. D. Anderson P. W. Anderson Bethe Bjorken Bogoliubov Brout Callan Coleman DeWitt Dirac Dyson Englert Fermi Feynman Fierz Fock Fröhlich Glashow Gell-Mann Gross Guralnik Heisenberg Higgs Haag Hagen 't Hooft Jordan Kendall Kibble Lamb Landau Lee Majorana Mills Nambu Nishijima Parisi Polyakov Salam Schwinger Skyrme Sudarshan Tomonaga Veltman Ward Weinberg Weyl Wilczek Wilson Yang Yukawa Weisskopf

In physics, specifically in relativistic quantum mechanics and quantum field theory, the Pauli–Lubanski pseudovector named after Wolfgang Pauli and Józef Lubański^[1] is an operator defined from the momentum and angular momentum, used in the quantum-relativistic description of angular momentum. It is the generator of the little group of the Lorentz group, that is the maximal subgroup (with four generators) leaving the eigenvalues of the four-momentum vector $P μ$ invariant.^[2]

Definition

It is usually denoted by $W$ (or less often by $S$ ) and defined by:^[3]^[4]^[5]

$W_{\mu} \stackrel{\mathrm{def}}{=} ~ \tfrac{1}{2}\varepsilon_{\mu \nu \rho \sigma} J^{\nu \rho} P^\sigma ,$

where

$\varepsilon_{\mu \nu \rho \sigma}$ is the four-dimensional totally antisymmetric Levi-Civita symbol
$J^{\nu \rho}$ is the relativistic angular momentum tensor operator
$P^{\sigma}$ is the four-momentum.

In the language of exterior algebra, it can be written as the Hodge dual of a trivector,^[6]

\mathbf{W} = \star(\mathbf{J}\wedge\mathbf{p}).

$W μ$ evidently satisfies

P^{\mu}W_{\mu}=0,

as well as the following commutator relations,

\left[P^{\mu},W^{\nu}\right]=0,

\left[J^{\mu \nu},W^{\rho}\right]=i \left( g^{\rho \nu} W^{\mu} - g^{\rho \mu} W^{\nu}\right),

Consequently,

\left[W_{\mu},W_{\nu}\right]=-i \epsilon_{\mu \nu \rho \sigma} W^{\rho} P^{\sigma}.

The scalar $W μ W μ$ is a Lorentz invariant operator, and commutes with the four-momentum, and can thus serve as a label for irreducible representations of the Lorentz group. That is, it can serve as the label for the spin, a feature of the spacetime structure of the representation, over and above the label ( $P μ P μ$ ) for the mass of states in a representation.

Massive fields

In quantum field theory, in the case of a massive field, the Casimir invariant $W μ W μ$ describes the total spin of the particle, with eigenvalues

W^2=W_{\mu}W^{\mu}=-m^2 s(s+1),

where $s$ is the spin quantum number of the particle and $m$ is its rest mass.

It is straightforward to see this in the rest frame of the particle, where $W \to = mJ \to$ and $W 0 = 0$ , so that the little group amounts to the rotation group,

W_{\mu}W^{\mu}=-m^2 \vec{J}\cdot\vec{J}.

Since this is a Lorentz invariant quantity, it will be the same in all other reference frames. It is also customary to take $W 3$ to describe the spin projection along the third direction in the rest frame.

In moving frames, decomposing $W = (W 0, W \to)$ into components $(W 1, W 2, W 3)$ , with $W 1$ and $W 2$ orthogonal to $P \to$ , and $W 3$ parallel to $P \to$ , the Pauli–Lubanski vector may be expressed in terms of the spin vector $S \to$ = $(S 1, S 2, S 3)$ (similarly decomposed) as

W_0 = P S_3, \qquad W_1 = m S_1, \qquad W_2 = m S_2, \qquad W_3 = \frac{E}{c^2} S_3,

where

E^2 = P^2 c^2 + m^2 c^4

is the energy–momentum relation.

The transverse components $W 1, W 2$ , along with $S 3$ , satisfy the following commutator relations (which apply generally, not just to non-zero mass representations),

[W_1, W_2] = \tfrac{ih}{2\pi} ((E/c^2)^2 - (P/c)^2) S_3, \qquad [W_2, S_3] = \tfrac{ih}{2\pi} W_1, \qquad [S_3, W_1] = \tfrac{ih}{2\pi} W_2.

For particles with non-zero mass, and the fields associated with such particles,

[W_1, W_2] = \tfrac{ih}{2\pi} m^2 S_3.

Massless fields

In general, in the case of non-massive representations, two cases may be distinguished. For massless particles,

W^2=W_{\mu}W^{\mu}=- E^{2}((K_{2}-J_{1})^{2} + (K_{1}+J_{2})^{2})\stackrel{\mathrm{def}}{=} - E^{2}(A^{2} + B^{2}) .

So, mathematically, $P$ ² = 0 does not imply $W$ ² = 0.

In the more general case, the components of $W \to$ transverse to $P \to$ may be non-zero, thus yielding the family of representations referred to as the cylindrical luxons, their identifying property being that the components of $W \to$ form a Lie subalgebra isomorphic to the 2-dimensional Euclidean group $ISO(2)$ , with the longitudinal component of $W \to$ playing the role of the rotation generator, and the transverse components the role of translation generators. This amounts to a group contraction of $SO(3)$ , and leads to what are known as the continuous spin representations. However, there are no known physical cases of fundamental particles or fields in this family.

In a special case, $W \to$ is parallel to $P \to$ ; or equivalently $W \to \times P \to = 0 \to$ . For non-zero $W \to$ , this constraint can only be consistently imposed for luxons, since the commutator of the two transverse components of $W \to$ is proportional to $m 2$ $J \to \cdot P \to$ .

For this family, the helicity operator

W^0/P,

represents an invariant, where

W^0 = -\vec{J}\cdot\vec{P}.

All particles that interact with the Weak Nuclear Force, for instance, fall into this family, since the definition of weak nuclear charge ( weak isospin) involves helicity, which, by above, must be an invariant. The appearance of non-zero mass in such cases must then be explained by other means, such as the Higgs mechanism. Even after accounting for such mass-generating mechanisms, however, the photon (and therefore the electromagnetic field) continues to fall into this class, although the other mass eigenstates of the carriers of the electroweak force (the $W$ particle and anti-particle and $Z$ particle) acquire non-zero mass.

Neutrinos were formerly considered to fall into this class as well. However, through neutrino oscillations, it is now known that at least two of the three mass eigenstates of the left-helicity neutrino and right-helicity anti-neutrino each must have non-zero mass.

References

Notes

↑ Lubański, J. K. (1942). "Sur la theorie des particules élémentaires de spin quelconque. I". Physica 9 (3): 310–324. doi:10.1016/S0031-8914(42)90113-7. ; Lubanski, J. K. (1942). "Sur la théorie des particules élémentaires de spin quelconque. II". Physica 9 (3): 325–338. doi:10.1016/S0031-8914(42)90114-9.
↑ Wigner, Eugene (1939). "On unitary representations of the inhomogeneous Lorentz group". The Annals of Mathematics 40 (1): 149–204. doi:10.2307/1968551.
↑ L.H. Ryder (1996). Quantum Field Theory (2nd ed.). Cambridge University Press. p. 62. ISBN 0-52147-8146.
↑ N.N. Bogolubov (1989). General Principles of Quantum Field Theory (2nd ed.). Springer. p. 273. ISBN 0-7923-0540-X.
↑ T. Ohlsson (2011). Relativistic Quantum Physics: From Advanced Quantum Mechanics to Introductory Quantum Field Theory. Cambridge University Press. p. 11. ISBN 1-13950-4320.
↑ R. Penrose (2005). The Road to Reality. Vintage books. p. 568. ISBN 978-00994-40680.

Other

Sergeĭ Mikhaĭlovich Troshin, Nikolaĭ Evgenʹevich Ti͡urin (1994). Spin phenomena in particle interactions. World Scientific. ISBN 9-81021-6920.