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twistor space

Contents

Idea

Twistor space in the original sense of (Penrose 67) is a complex manifold whose complex geometry is usefully related to the conformal geometry of (conformally compactified complexified) 4-dimensional Minkowski spacetime. The Penrose transform from twistor space to this spacetime yields powerful computational tools for studying certain quantum field theories, in particular 4d Yang-Mills theory. Notably it sends ordinary cohomology classes on twistor space to self-dual Yang-Mills fields on spacetime (Ward 77, Ward-Wells 90). Morever, when twistor space is taken as a target space for twistor string theory, then it serves to compute the MHV amplitudes in super Yang-Mills theory (Witten 03).

This Penrose transform is exhibited by a correspondence of coset spaces/flag varieties/Grassmannians which is a special case of general such correspondences as they are studied in Schubert calculus, geometric representation theory, parabolic geometry. Therefore one can consider “generalized twistors” to be elements of certain flag varieties and “generalized Penrose transforms” to be those induced by the relevant correspondences. (Baston-Eastwood 89, Cap 01).

In this generality given a semisimple Lie group GG and two parabolic subgroups P 1P_1 and P 2P_2 with intersection P 1P 2P_1 \cap P_2, then the twistor correspondence is the correspondence (see also at Schubert calculus – Correspondences and at horocycle correspondence) of the form

G/(P 1P 2) p 1 p 2 G/P 1 G/P 2 \array{ && G/(P_1 \cap P_2) \\ & {}^{\mathllap{p_1}}\swarrow && \searrow^{\mathrlap{p_2}} \\ G/P_1 && && G/P_2 }

given by the projections onto the two coset spaces/flag varieties and a Penrose transform is an integral transform/pull-push (p 1) !(p 1) *(p_1)_! \circ (p_1)^\ast through this correspondence.

In particular there are higher twistor spaces corresponding to higher dimensional Minkowski spacetimes which are useful for describing higher dimensional quantum field theory, notably there are twistor spaces for 6-dimensional spacetime useful for the study of the 6d (2,0)-superconformal QFT on the worldvolume of the M5-brane (MREIC 11) with its self-dual higher gauge field, the B-field .

The original twistor correspondence (Penrose 67) is the correspondence

( Gr 1,2( 4) P 3 Gr 2( 4))( SL (4)/SL (2) SL (4)/SL (3) SL (4)/(SL (2)×SL (2))), \left( \array{ && Gr_{1,2}(\mathbb{C}^4) \\ & \swarrow && \searrow \\ \mathbb{C}P^3 && && Gr_2(\mathbb{C}^4) } \right) \;\;\;\;\; \simeq \;\;\;\;\; \left( \array{ && SL_\mathbb{C}(4)/SL_{\mathbb{C}}(2) \\ & \swarrow && \searrow \\ SL_{\mathbb{C}}(4)/SL_{\mathbb{C}}(3) && && SL_{\mathbb{C}}(4)/(SL_{\mathbb{C}}(2)\times SL_{\mathbb{C}}(2)) } \right) \,,

where

  • the Grassmannian G 2( 4)G_2(\mathbb{C}^4) of planes in complexified 4d Minkowski spacetime;

  • the twistor space is the complex projective space P 3=Gr 1( 4)\mathbb{C}P^3 = Gr_1(\mathbb{C}^4);

  • the correspondence space Gr 1,2( 4)Gr_{1, 2}(\mathbb{C}^4) is the space of lines in planes in 4\mathbb{C}^4.

(e.g. Ward-Wells 90)

Details

Twistors for 4d Minkowski space

We discuss the original twistors for the description of physics in 4d Minkowski spacetime. In summary, twistor space of 4d Minkowski space is the space of pairs consisting of a momentum vector and an angular momentum tensor subject to the constraint that the momentum is lightlike and of definite helicity.

The formulation is all motivated from the form that basic quantities of special relativistic physics take when vectors are expressed in spinor coordinates via the exceptional spin isomorphism

Spin(3,1)SL(2,). Spin(3,1) \simeq SL(2,\mathbb{C}) \,.

Under this identification a chiral spinor κ\kappa is represented just by a pair of complex numbers ξ,η\xi, \eta \in \mathbb{C} and one may write the spinor as

(κ α)=(ξ η) 2. \left( \kappa^\alpha \right) = \left( \array{ \xi \\ \eta } \right) \in \;\; \mathbb{C}^2 \,.

Moreover, via the non-degenerate bilinear pairing

Γ:SSV \Gamma \;\colon\; S \otimes S \longrightarrow V

given by the Clifford algebra (see at spin representation for details) one can express vectors

(x i)=(x 0,x 1,x 2,x 3) (x^i) = (x^0, x^1, x^2, x^3)

in Minkowski spacetime as “bi-spinors” given by 2x2 Hermitean matrices

(x αβ) (x iγ i αβ) =12(x 0+x 3 x 1+ix 2 x 1ix 2 x 0x 3)Mat 2(), \begin{aligned} \left(x^{\alpha \beta}\right) & \coloneqq (x^i \gamma_i^{\alpha \beta}) \\ & = \tfrac{1}{\sqrt{2}} \left( \array{ x^0 + x^3 & x^1 + i x^2 \\ x^1 - i x^2 & x^0 - x^3 } \right) \;\; \in Mat_{2}(\mathbb{C}) \end{aligned} \,,

where γ i\gamma_i denote the generators of the Clifford algebra given by the Pauli matrices.

This is such that the Lorentz metric norm is just the determinant of this matrix

(x i)=2det((x αβ)). \Vert \left(x^i\right) \Vert = 2 det\left(\left(x^{\alpha \beta} \right)\right) \,.

This spinorial re-expression of vectors turns out to yield very efficient expressions particularly for those kinds of terms that appear in the observed physics of massless chiral particles, such as they appear in the standard model of particle physics.

For instance a skew rank-2 tensor (2-from) (F ij)(F_{i j}) with F ij=F jiF_{i j} = - F_{j i} (for instance the field strength of an electromagnetic field) has spinorial expression of the simple form

F α 1β 1α 2β 2 F i 1i 2γ α 1β 1 i 1γ α 2β 2 i 2 =ϕ α 1α 2ϵ β 1β 2+ψ β 1β 2ϵ α 1α 2 \begin{aligned} F_{\alpha_1 \beta_1 \alpha_2 \beta_2} & \coloneqq F_{i_1 i_2} \gamma^{i_1}_{\alpha_1 \beta_1} \gamma^{i_2}_{\alpha_2 \beta_2} \\ & = \phi_{\alpha_1 \alpha_2} \epsilon_{\beta_1 \beta_2} + \psi_{\beta_1 \beta_2} \epsilon_{\alpha_1 \alpha_2} \end{aligned}

for complex numbers (ϕ α 1α 2)(\phi_{\alpha_1 \alpha_2}) and (ψ β 1β 2)(\psi_{\beta_1 \beta_2}). Here if FF itself is real-number valued, then ψ\psi is the complex conjugate of ϕ\phi and hence any real 2-form is encoded equivalently by a bispinor ϕ\phi via

F α 1β 1α 2β 2ϕ α 1α 2ϵ β 1β 2+ϕ¯ β 1β 2ϵ α 1α 2 F_{\alpha_1 \beta_1 \alpha_2 \beta_2} \coloneqq \phi_{\alpha_1 \alpha_2} \epsilon_{\beta_1 \beta_2} + \overline{\phi}_{\beta_1 \beta_2} \epsilon_{\alpha_1 \alpha_2}

Crucially the Hodge dual of a 2-form has then the simple expression

(F) α 1β 1α 2β 2=iϕ α 1α 2ϵ β 1β 2+iψ β 1β 2ϵ α 1α 2, (\star F)_{\alpha_1 \beta_1 \alpha_2 \beta_2} = - i \phi_{\alpha_1 \alpha_2} \epsilon_{\beta_1 \beta_2} + i \psi_{\beta_1 \beta_2} \epsilon_{\alpha_1 \alpha_2} \,,

which is the first sign that self-dual Yang-Mills theory has a simpler expression in terms of such spinorial coordinates.

Now characterizing an elementary particle is (by the discussion at unitary representation of the Poincaré group) the momentum 4-vector (p i)(p^i) and its angular momentum tensor (M ij)(M^{i j}). A twistor is effectively a pair of spinorial coordinates expression this data for massless and chiral particles.

Here chiral means this: from combining the momentum and angular momentum one obtains the Pauli-Lubanski vector

S i12(M) ijp j S_i \coloneqq \tfrac{1}{2} (\star M)_{i j} p^j

and chiral particles satisfy

S i=sp i S_i = s p_i

for some constant ss.

A twistor is a set of spinorial coordinates for encoding tensors ((p i),(M ij))\left(\left(p^i\right), \left(M^{i j}\right)\right) which satisfy

  1. masslessness: p ip i=0p^i p_i = 0

  2. chirality S i=sp iS_i = s p_i.

By the discussion at celestial sphere we have that the first condition means equivalently that there is a single spinor (π α)(\pi_\alpha) such that the spinorial expression for the momentum is

p αβ=π απ¯ β. p_{\alpha \beta} = \pi_\alpha \overline{\pi}_\beta \,.

By the above discussion of 2-forms we know moreover that M ijM^{i j} is encoded by a bispinor μ αβ\mu_{\alpha \beta} and imposing the chirality constraint one finds, using the above formula for the Hodge dual, that its solutions are parameterized precisely by another spinor (ω α)(\omega_\alpha) via

μ¯ αβ=iω (απ¯ β) \overline{\mu}_{\alpha \beta} = i \omega_{(\alpha} \overline{\pi}_{\beta)}

(where the parenthesis denote symmetrization of indices).

In summary then the possible momentum and angular momentum (p i,M ij)(p^i, M^{i j}) of massless chiral particles in 4d Minkowski spacetime is parameterized precisely by pair of spinors

Z=((ω α),(π β)) 4. Z = \left( (\omega^\alpha), (\pi_\beta) \right) \;\; \in \mathbb{C}^4 \,.

The image of this under modding out by a global complex factor is a Penrose twistor

ZP 3, Z \in \mathbb{C}P^3 \,,

an element of the 3-dimensional complex projective space, called twistor space.

Twistor space

To discuss twistor space for Minkowski spacetime, it is useful to work more generally with dd-dimensional Minkowski spacetime for d{3,4,6,10}d \in \{3,4,6,10\}. If we also use the corresponding irreducible real spin representation then by the discussion there, these are equivalently 2-component vectors over the real normed division algebras 𝕂{,,,𝕆}\mathbb{K} \in \{\mathbb{R}, \mathbb{C}, \mathbb{H}, \mathbb{O}\}, respectively. (See also at supersymmetry and division algebra, we follow Bengtsson-Cederwall 88).

With this, the vector space underlying dd-dimensional Minkowski spacetime d1,1\mathbb{R}^{d-1,1} is identified with the space of 2×22 \times 2 hermitian matrices with entries in 𝕂\mathbb{K}

d1,1 linearMat 2×2 hermitian(𝕂) \mathbb{R}^{d-1,1} \simeq_{linear} Mat_{2 \times 2}^{hermitian}(\mathbb{K})

and the Minkowski metric norm-square is then identified with the determinant of matrices:

η(v,v)=det(v)v d1,1 linearMat 2×2 hermitian(𝕂). \eta(v,v) = det(v) \;\;\; v\in \mathbb{R}^{d-1,1} \simeq_{linear} Mat_{2 \times 2}^{hermitian}(\mathbb{K}) \,.

A choice of linear basis for this space is provided by the Pauli matrices with coefficients in 𝕂\mathbb{K}, namely the matrices

(Γ 0 α˙α)[1 0 0 1],(Γ 1 α˙α)[1 0 0 1],(Γ n+1 α˙α)[0 e n e¯ n 0] (\Gamma_0^{\dot \alpha \alpha}) \coloneqq \left[ \array{ 1 & 0 \\ 0 & -1 } \right] \;\;\,, \;\;\;\; (\Gamma_1^{\dot \alpha \alpha}) \coloneqq \left[ \array{ 1 & 0 \\ 0 & 1 } \right] \;\;\,, \;\;\;\; (\Gamma_{n+1}^{\dot \alpha \alpha}) \coloneqq \left[ \array{ 0 & e_n \\ \overline{e}_n & 0 } \right]

where {e n} n=2 d\{e_n\}_{n = 2}^{d} denotes an orthonormal basis for the elements of 𝕂\mathbb{K}. Here we write

()¯:𝕂𝕂 \overline{(-)} \;\colon\; \mathbb{K} \longrightarrow \mathbb{K}

for the operation of complex conjugation in 𝕂\mathbb{K}, i.e. the \mathbb{R}-linear operation which sends the unit 11 to itself, and sends imaginary elements to their negative.

In terms of this basis then a dd-component vector (X μ) d1,1(X^\mu) \in \mathbb{R}^{d-1,1} is identified with the hermitian 2×22 \times 2 matrix

(X α˙α)(X μΓ μ α˙α)=[x 0+x 1 x ne n x ne¯ n x 0x 1]. (X^{\dot \alpha \alpha}) \;\coloneqq\; (X^\mu \Gamma_\mu^{\dot \alpha \alpha}) \;=\; \left[ \array{ x^0 + x^1 & x^{n} e_n \\ x^n \overline{e}_n & x^0 - x^1 } \right] \,.

This presentation of Minkowski spacetime by 2×22 \times 2 hermitian matrices with coefficients in 𝕂\mathbb{K} makes it very natural to consider also its “𝕂\mathbb{K}-ification” (hence complexification in the case that d=4d = 4 and 𝕂=\mathbb{K} = \mathbb{C}), namely the space of all 2×22 \times 2 matrices with entries in 𝕂\mathbb{K}:

𝕂 d1,1Mat 2×2(𝕂). \mathbb{K}\mathbb{R}^{d-1,1} \coloneqq Mat_{2\times 2}(\mathbb{K}) \,.

This space carries the operation of Hermitian conjugation

XX X \mapsto X^\dagger

as an involution, and ordinary dd-dimensional Minkowski spacetime is hence the fixed point set of this involution.

By the discussion there, the Spin-invariant pairing of two real spinors ψ,ϕ𝕂 2\psi, \phi \in \mathbb{K}^2 to a vector ψ¯ΓϕMat 2×2 hermitian(𝕂)\overline{\psi} \Gamma \phi \in Mat_{2\times 2}^{hermitian}(\mathbb{K}) is given by (prop.)

(ψ¯Γϕ)ψϕ +ϕψ . (\overline{\psi}\Gamma \phi) \coloneqq \psi \phi^\dagger + \phi \psi^\dagger \,.

In particular the pairing of a spinor ψ=(ψ α˙)\psi = (\psi_{\dot \alpha}) with itself is

(ψψ ) αα˙=2ψ¯ αψ α˙. (\psi \psi^\dagger)_{\alpha \dot\alpha} = 2 \overline{\psi}_\alpha \psi_{\dot \alpha} \,.

Since, as hermitian matrices, the 2×22 \times 2 matrices arising this way are manifestly precisely the hermitian projection operators on 1-dimensional linear subspaces of 𝕂 2\mathbb{K}^2, these are precisely the 2×22 \times 2 hermitian matrices with vanishing determinant. Hence the future-oriented lightlike vectors in Minkowski spacetime in d={3,4,6,10}d = \{3,4,6,10\} are precisely those that arise as the pairing of a chiral spinor with itself.

The above formula shows that as we rescale ψkψ\psi \mapsto k \psi with k𝕂k \in \mathbb{K}, then the corresponding lightlike vector is sent to itself, rescaled by the real number kk¯k \overline{k} \in \mathbb{R}. Hence the direction of lightlike vectors is parameterized by the projective space 𝕂P 1\mathbb{K}P^1. At least for 𝕂=\mathbb{K} = \mathbb{C} (the complex numbers) this is called the celestial sphere (in this case: the Riemann sphere P 1\mathbb{C}P^1).

Lightlike vectors in d1,1\mathbb{R}^{d-1,1} up to scale are equivalently loci of lightlike geodesics through the origin. A general lightlike geodesic in d1,1\mathbb{R}^{d-1,1} is instead parameterized by

τ(X α˙α+τψ αψ¯ α˙) \tau \mapsto (X^{\dot \alpha \alpha} + \tau {\psi}^\alpha \overline{\psi}^{\dot \alpha})

for some offset (X α˙α)(X^{\dot \alpha \alpha}). To encode this offset into spinors, consider the image of ψ\psi under the Clifford action with XX:

ω αψ α˙X α˙α. \omega^\alpha \coloneqq \psi_{\dot \alpha} X^{\dot \alpha \alpha} \,.

This relation bewteen ω\omega and ψ\psi is called the incidence relation in this context.

The locus of the lightlike geodesic does not change as we rescale ψ\psi by elements k𝕂k \in \mathbb{K}, and then ω\omega gets rescaled accordingly. Hence the pair (ω α,ψ α˙)(\omega^\alpha, \psi_{\dot \alpha}) regarded as encoding lightlike geodesics in Minkowski spacetime should be thought of as an element of the projective space

𝕂P 3{(Z a)=(ω α,ψ α˙)𝕂 4} ((Z a)(kZ a)|k𝕂). \mathbb{K}P^3 \coloneqq \{ (Z^{a}) = (\omega^\alpha,\psi_{\dot \alpha}) \in \mathbb{K}^4 \}_{( (Z^a) \sim (k Z^a) \vert k \in \mathbb{K} )}.

This is the twistor space corresponding to the given Minkowski spacetime.

However, by the above definition of ω α\omega^\alpha, not every element of this space corresponds to a lighlike geodesic. Rather (for d{3,4,6}d \in \{3,4,6\}) it is only those satisfying

ω αψ¯ α=ψ α˙ω¯ α˙ \omega^\alpha \overline{\psi}_\alpha = \psi_{\dot \alpha} \overline{\omega}^{\dot \alpha}

reflecting the fact that (X α˙α)(X^{\dot \alpha \alpha}) is a hermitian matrix, instead of a general 2×22\times 2 matrix. (For d=10d = 10 there is no elegant statement like this, due to the non-associativity of the octonions 𝕂=𝕆\mathbb{K} = \mathbb{O}).

Hence the subspace inclusion

d1,1𝕂 d1,1 \mathbb{R}^{d-1,1} \hookrightarrow \mathbb{K}\mathbb{R}^{d-1,1}

of Minkowski-spacetime into its 𝕂\mathbb{K}-ification, corresponds to a subspace

𝒩𝕂P 3 \mathcal{N} \hookrightarrow \mathbb{K}P^3

of twistor space. This is called the space of null twistors, or the spin shell.

If we consider the metric on 𝕂 4\mathbb{K}^4 given in component by

[0 δ α β δ β˙ α˙ 0] \left[ \array{ 0 & \delta^\beta_\alpha \\ - \delta^{\dot \alpha}_{\dot \beta} & 0 } \right]

then this subspace is the quadric given by the equation

Z aZ¯ a=0. Z^a \overline{Z}_a = 0 \,.

Now conversely, given Z a=(ω α,ψ α˙)Z^a = (\omega^\alpha, \psi_{\dot\alpha}) not equal to zero and satisfying this condition in that there is a hermitian X α˙αX^{\dot \alpha \alpha} with ω α=ψ α˙X α˙α\omega^{\alpha} = \psi_{\dot \alpha} X^{\dot \alpha \alpha}, then also every hermitian matrix of the form

X α˙α+τψ α˙ψ α X^{\dot \alpha \alpha} + \tau \psi^{\dot \alpha}\psi^\alpha

(for τ\tau \in \mathbb{R}, hence every point on the lightlike geodesic through XX in the direction of ψψ \psi \psi^\dagger) satisfies the relation (since the spinor index is raised with (ϵ α˙β˙)(\epsilon^{\dot \alpha \dot \beta}), which is skew symmetric). This way non-zero points in 𝒩𝕂P 3\mathcal{N} \hookrightarrow \mathbb{K}P^3 correspond to lightlike geodesics in Minkowski spacetime.

(graphics from Adamo 13)

This correspondence extends also to the 0-point in 𝒩\mathcal{N} if one passes to “compactified Minkowski spacetime”, given by the Grassmannian Gr 2( 4)Gr_2(\mathbb{C}^4) of complex planes in 4\mathbb{C}^4 (review includes Fioresi-Lledo-Varadarajan 07, section 2).

References

General

The notion originates in

  • Roger Penrose, Twistor algebra, Journal of Mathematical Physics 8 (2): 345–366, (1967)

  • Roger Penrose, The twistor programme, Reports on Mathematical Physics 12 (1): 65–76 (1977)

Key developments concerning scattering amplitudes are due to

The relation to self-dual Yang-Mills theory is due to

  • R. S. Ward, On Selfdual gauge fields, Phys. Lett. A61 (1977) 81-82.

Introductions and surveys include

Review of the application in super Yang-Mills theory includes

See also

Relation to geometric representation theory and parabolic geometry

A discussion in the general context of geometric representation theory is in

  • R. J. Baston, M. G. Eastwood, The Penrose Transform Its Interaction with Representation Theory Oxford Science Publications, Clarendon Press, 1989

and the further generalization to Cartan geometry/parabolic geometry is discussed in

Application to quantum field theory

More on traditional applications to quantum field theory is in

  • R.S. Ward, R.O. Wells, Twistor geometry and field theory, Cambridge Univ. Press 1990.

The relation of twistor geometry to MHV amplitudes in 4d Yang-Mills theory and twistor string theory is due to

Surveys of the resulting modern application of twistors in field theory include

  • David Skinner, The geometry of scattering amplitudes, talk notes, November 2009 (pdf)

Twistors in higher dimensions

Discussion of twistors in dimensions 3,4,6 and 10 using the normed division algebras (as in supersymmetry and division algebras) is in

Application to the 6d self-dual 2-form field

A general discussion of Penrose-Ward-type transforms sending circle 2-bundles (holomorphic line 2-bundles) on some twistor space to circle 2-bundles with connection and self-dual curvature 3-form on spacestime (expected to play a role in the description of the 6d (2,0)-superconformal QFT) is in

  • David Chatterjee, sections 4 and 8 of On Gerbs, 1998 (pdf)

  • L. J. Mason, R. A. Reid-Edwards, A. Taghavi-Chabert, appendix of Conformal Field Theories in Six-Dimensional Twistor Space, J. Geom. Phys. 62 (2012), no. 12, 2353-2375 (arXiv:1111.2585)

More generally, there are arguments that the worldvolume theory of several coincident M5-branes carries not just an abelian but a nonabelian higher gauge field given by a principal 2-bundle principal 2-connection.

The idea of generalizing the Penrose-Ward transform to one that takes nonabelian principal 2-bundles to self-dual principal 2-connections is explored in

Revised on October 18, 2016 15:42:02 by Urs Schreiber (89.204.135.226)