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November 1, 2020

Octonions and the Standard Model (Part 6)

Posted by John Baez

One of the most interesting functions on the exceptional Jordan algebra is the determinant. The linear transformations that preserve this form the exceptional Lie group E 6\mathrm{E}_6. And today I’ll show you how to compute this determinant in terms of 10-dimensional spacetime geometry: that is, scalars, vectors and spinors in 10d Minkowski spacetime.

The exceptional Jordan algebra 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) consists of 3×33 \times 3 self-adjoint matrices of octonions. The diagonal entries are forced to be their own conjugate, hence real:

𝔥 3(𝕆)={(α z y * z * β x y x * γ):x,y,z𝕆,α,β,γ} \mathfrak{h}_3(\mathbb{O}) = \left\{ \left( \begin{array}{ccc} \alpha & z & y^\ast \\ z^\ast & \beta & x \\ y & x^\ast & \gamma \end{array} \right) : \; x,y,z \in \mathbb{O}, \alpha, \beta, \gamma \in \mathbb{R} \right\}

Thus, 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) is 27-dimensional.

𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) is a Jordan algebra with product

ab=12(ab+ba) a \circ b = \frac{1}{2}( a b + b a )

where at right we’re just doing ordinary matrix multiplication. The group of linear transformations that preserve this product is 52-dimensional and it’s called F 4\mathrm{F}_4: it’s one of the five exceptional compact simple groups, and everyone should learn to love it.

F 4\mathrm{F}_4 is not just coincidentally connected to the exceptional Jordan algebra. It’s deeply connected. For example, its smallest nontrivial representation is 26-dimensional! Why 26 and not 27? Because it acts on 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) in a way that preserves the identity, and also the inner product

a,b=tr(a,b) \langle a, b \rangle = \mathrm{tr}(a,b)

so it preserves the 26-dimensional space of elements orthogonal to the identity: the traceless self-adjoint 3×33 \times 3 self-adjoint matrices of octonions, 𝔰𝔥 3(𝕆)\mathfrak{sh}_3(\mathbb{O}).

But the exceptional Jordan algebra also has another nice structure: the determinant. You might worry that the determinant of a matrix of octonions is ill-defined, since the octonions are noncommutative and nonassociative. And that’s true in general. But there’s a nice way to define it for a 3×33 \times 3 self-adjoint matrix of octonions:

det(α z y * z * β x y x * γ)=αβγ(α|x| 2+β|y| 2+γ|z| 2)+2Re(xyz) \mathrm{det} \left( \begin{array}{ccc} \alpha & z & y^\ast \\ z^\ast & \beta & x \\ y & x^\ast & \gamma \end{array} \right) = \alpha \beta \gamma - (\alpha |x|^2 + \beta |y|^2 + \gamma |z|^2) + 2 Re(x y z)

See? This is beautiful. It’s even better when you know that |x| 2=xx *=x *|x|^2 = x x^\ast = x^\ast, and that Re(xyz)Re(x y z) is invariant under cyclic permutations of x,y,zx,y,z, so we could rewrite this formula in a number of ways and get the same thing.

The transformations in F 4\mathrm{F}_4 preserve this determinant, but many others do too. There is a 78-dimensional group of linear transformations of 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) that preserve the determinant. It’s called E 6\mathrm{E}_6, it’s a noncompact exceptional simple Lie group, and again you should learn to love it. It’s deeply connected to 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}): for example, this space is its smallest nontrivial representation.

Actually this group is called E 6(26)\mathrm{E}_{6(-26)}, since E 6\mathrm{E}_6 has a number of different noncompact real forms, and this particular one has F 4\mathrm{F}_4 as its maximal compact subgroup, so it has

26=7852 26 = 78 - 52

extra noncompact directions. Indeed, as a manifold — though not as a Lie group — we have

E 6(26)F 4× 26 \mathrm{E}_{6(-26)} \cong \mathrm{F}_4 \times \mathbb{R}^{26}

But I don’t plan to talk about any other real form of E 6\mathrm{E}_6 anytime soon, so for now I’ll just call this one E 6\mathrm{E}_6.

By the way, note that 26, 52 and 78 are all multiples of 26. This is part of the spooky numerology that you learn when you get into exceptional Lie groups. That 26\mathbb{R}^{26} you see above is really 𝔰𝔥 3(𝕆)\mathfrak{sh}_3(\mathbb{O}): the 26-dimensional space of traceless elements of 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}).

But I’m getting ahead of myself!

Last time I explained how the exceptional Jordan algebra could be chopped into three parts, which correspond to scalars, vectors and left-handed spinors in 10d Minkowski spacetime. This time I’ll say how the determinant can be expressed in terms of these parts.

In the end we’ll have a formula for the determinant in terms of various operations involving scalars, vectors and spinors in 10d spacetime. The most exciting of these describes how a spin-1/2 fermion (described by a spinor of one handedness) can absorb a spin-1 boson (described by a vector) and turn into another spin-1/2 fermion (described by a spinor of the other handedness):

All these operations will be invariant under the group Spin(9,1)\mathrm{Spin}(9,1). As an immediate consequence we get an inclusion

Spin(9,1)E 6 \mathrm{Spin}(9,1) \subseteq \mathrm{E}_6

This has a nice meaning! As we saw last time, 𝔥 2(𝕆)\mathfrak{h}_2(\mathbb{O}) is 10d Minkowski spacetime. The group SO(9,1)\mathrm{SO}(9,1) acts as symmetries. We can think of 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) as an ‘exceptional’ 27-dimensional spacetime containing 10d Minkowski spacetime, with symmetry group E 6\mathrm{E}_6. A point in this larger spacetime consists of a point in 10d Minkowski spacetime — that is, a vector — together with a scalar and a left-handed spinor. While SO(9,1)\mathrm{SO}(9,1) acts on vectors, only its double cover Spin(9,1)\mathrm{Spin}(9,1) acts on spinors. So we get an inclusion of Spin(9,1)\mathrm{Spin}(9,1), not SO(9,1)\mathrm{SO}(9,1), in E 6\mathrm{E}_6.

I hope to continue developing the theme of 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) as a funny sort of ‘exceptional spacetime’ later. But we need to start by understanding the main structures on 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}). For this I want to express the determinant on 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) in terms of invariant operations on scalars, vectors and spinors in 10d Minkowski spacetime.

Intertwining operators

We might as well get our money’s worth and let 𝕂\mathbb{K} be any normed division algebra ,,\mathbb{R}, \mathbb{C}, \mathbb{H} or 𝕆\mathbb{O}. We’ll let nn stand for its dimension: 1, 2, 4, or 8. Last time I described representations of Spin(n+1,1)\mathrm{Spin}(n+1, 1) on

  • scalars: \mathbb{R}

  • vectors: V=𝔥 2(𝕂)V = \mathfrak{h}_2(\mathbb{K})

  • right-handed spinors S +=𝕂 2S_+ = \mathbb{K}^2

  • left-handed spinors S =𝕂 2S_- = \mathbb{K}^2

Now let’s describe some equivariant maps that relate these representations. Another name for an equivariant map between group representations is an ‘intertwining operator’— that’s what all my old books say, but it seems to be a bit old-fashioned: some of my students have never even heard of it!

By the way, a lot of these maps exist quite generally for scalars, vectors, and spinors in Minkowski spacetimes of any dimension — so this stuff is good to learn if you care about physics at all. But we get nice formulas for them using division algebras in Minkowski spacetimes of dimensions n+2=3,4,6n+ 2 = 3, 4, 6 and 1010.

Here they are:

1) An invariant pairing, our friend the Minkowski metric

g:VV g \colon V \otimes V \to \mathbb{R}

given by

g(v,w)=12Retr(vw˜) g(v,w) = \frac{1}{2} \mathrm{Re} \, \mathrm{tr}(v \tilde{w})

where the tilde stands for trace reversal:

v˜=vtrv1 \tilde{v} = v - \mathrm{tr}{v} 1

which, as we saw last time, has the geometrical meaning of time reversal.

2) An invariant pairing between right- and left-handed spinors:

,:S +S \langle -, - \rangle \colon S_+ \otimes S_- \to \mathbb{R}

given by

ψ,ϕ=Re(ψ ϕ) \langle \psi, \phi \rangle = Re(\psi^\dagger \phi)

where the dagger stands for conjugate transpose. Here I’m thinking of ϕ,ψ𝕂 2\phi , \psi \in \mathbb{K}^2 as column vectors, so ψ \psi^\dagger is a row vector and the product ψ ϕ\psi^\dagger \phi is an element of 𝕂\mathbb{K}. This pairing is nondegenerate, so

S + *S S_+^\ast \cong S_-

as representations of Spin(n+1,1)\mathrm{Spin}(n+1,1).

3) An action of vectors on right-handed spinors that turns them into left-handed spinors:

γ:VS +S \gamma \colon V \otimes S_+ \to S_-

given by

γ(vψ)=vψ \gamma(v \otimes \psi) = v \psi

where in vψv \psi we’re multiplying a matrix and a column vector.

4) An action of vectors on left-handed spinors that turns them into right-handed spinors:

γ˜:VS S + \tilde{\gamma} \colon V \otimes S_- \to S_+

given by

γ˜(vψ)=v˜ψ \tilde{\gamma}(v \otimes \psi) = \tilde{v} \psi

In physics, maps 3) and 4) are used to describe how a spin-1/2 particle can absorb a gauge boson and turn into another spin-1/2 particle:

We saw last time that they also give rise to the action of the spin group Spin(n+1,1)Spin(n+1,1) on spinors of either handedness.

These maps give others using duality: we can turn inputs into outputs, or vice versa, by taking their duals. For example, our map VS S +V \otimes S_- \to S_+ also gives a map S S + *V *S_- \otimes S_+^\ast \to V^\ast, but using our invariant pairings we can re-express this as a map S S VS_- \otimes S_- \to V. We can get a map S +S +VS_+ \otimes S_+ \to V in the same way. It’s worth having formulas for these maps:

5) An equivariant map that turns two left-handed spinors into a vector:

[,]:S S V [-,-] \colon S_- \otimes S_- \to V

given by

[ψ,ϕ]=ψϕ +ϕψ [\psi, \phi] = \psi \phi^\dagger + \phi \psi^\dagger

Here we are multiplying column vectors by row vectors and getting 2×22 \times 2 matrices, and when we add those up the end result is self-adjoint.

6) An equivariant map that turns two right-handed spinors into a vector:

[,]:S +S +V [-,-] \colon S_+ \otimes S_+ \to V

given by

[ψ,ϕ]=ψϕ +ϕψ ˜ [\psi, \phi] = \widetilde{\psi \phi^\dagger + \phi \psi^\dagger}

where the impressively long tilde stands for trace reversal.

To see proofs that maps 1)–6) are intertwining operators, see Section 3 here:

  • John C. Baez, John Huerta, Division algebras and supersymmetry I, in Superstrings, Geometry, Topology, and C *{}^\ast-algebras, eds. R. Doran, G. Friedman and J. Rosenberg, Proc. Symp. Pure Math. 81, AMS, Providence, 2010, pp. 65–80.

I’m trying to make these blog articles self-contained, but you can just pop over there for the details.

The determinant

As we’ve seen, the determinant of

a=(α z y * z * β x y x * γ)𝔥 3(𝕆) a = \left( \begin{array}{ccc} \alpha & z & y^\ast \\ z^\ast & \beta & x \\ y & x^\ast & \gamma \end{array} \right) \in \mathfrak{h}_3(\mathbb{O})


det(a)=αβγ(α|x| 2+β|y| 2+γ|z| 2)+2Re(xyz) \mathrm{det}(a) = \alpha \beta \gamma - (\alpha |x|^2 + \beta |y|^2 + \gamma |z|^2) + 2 Re(x y z)

But we can break aa up into its scalar, vector and spinor parts:

a=(α ψ ψ v) a = \left( \begin{array}{cc} \alpha & \psi^\dagger \\ \psi & v \end{array} \right)


α,v=(β x x * γ)V,ψ=(z * y)S \alpha \in \mathbb{R}, \qquad v = \left( \begin{array}{cc} \beta & x \\ x^\ast & \gamma \end{array} \right) \in V , \qquad \psi = \left( \begin{array}{cc} z^\ast \\ y \end{array} \right) \in S_-

Then we have:

Theorem 8. For any a𝔥 3(𝕂)a \in \mathfrak{h}_3(\mathbb{K}) we have

det(a)=αg(v,v)+g(v,[ψ,ψ]) \mathrm{det}(a) = - \alpha g(v,v) + g(v, [\psi, \psi])

Proof. Start with the definition

det(a)=αβγ(α|x| 2+β|y| 2+γ|z| 2)+2Re(xyz) det(a) = \alpha \beta \gamma - (\alpha |x|^2 + \beta |y|^2 + \gamma |z|^2) + 2 Re(x y z)

You can see the determinant of the 2×22 \times 2 block

det(v)=det(β x x * γ)=βγ|x| 2 det(v) = det \left( \begin{array}{cc} \beta & x \\ x^\ast & \gamma \end{array} \right) = \beta \gamma - |x|^2

hiding in this expression, and as I mentioned last time, det(v)=g(v,v)det(v) = -g(v,v), so

det(a)=αg(v,v)β|y| 2γ|z| 2+2Re(xyz) det(a) = - \alpha g(v,v) - \beta |y|^2 - \gamma |z|^2 + 2 Re(x y z)

Thus to prove the theorem we just need to show

g(v,[ψ,ψ])=β|y| 2γ|z| 2+2Re(xyz) g(v,[\psi,\psi]) = - \beta |y|^2 - \gamma |z|^2 + 2 Re(x y z)

So, let’s compute the left-hand side! We have

[ψ,ψ] = 2ψψ = 2(z * y)(z y *) = 2(|z| 2 z *y * yz |y| 2) \begin{array}{ccl} [\psi,\psi] &=& 2 \psi \psi^\dagger \\ &=& 2 \left( \begin{array}{c} z^\ast \\ y \end{array} \right) \left( \begin{array}{cc} z & y^\ast \end{array} \right) \\ &=& 2 \left( \begin{array}{cc} |z|^2 & z^\ast y^\ast \\ y z & |y|^2 \end{array} \right) \end{array}

and thus

g(v,[ψ,ψ]) = 12Retr(v˜[ψ,ψ]) = Retr((β x x * γ)˜(|z| 2 z *y * yz |y| 2)) = Retr((γ x x * β)(|z| 2 z *y * yz |y| 2)) \begin{array}{ccl} g(v,[\psi,\psi]) &=& \frac{1}{2} \mathrm{Re} \, \mathrm{tr}( \tilde v [\psi, \psi]) \\ &=& \mathrm{Re} \, \mathrm{tr} \left( \widetilde{\left( \begin{array}{cc} \beta & x \\ x^\ast & \gamma \end{array} \right)} \left( \begin{array}{cc} |z|^2 & z^\ast y^\ast \\ y z & |y|^2 \end{array} \right) \right) \\ &=& \mathrm{Re} \, \mathrm{tr} \left( \left( \begin{array}{cc} -\gamma & x \\ x^\ast & -\beta \end{array} \right) \left( \begin{array}{cc} |z|^2 & z^\ast y^\ast \\ y z & |y|^2 \end{array} \right) \right) \end{array}

Multiplying the damned matrices and taking the real part of their trace, we get

g(v,[ψ,ψ])=Re(γ|z| 2+xyz+x *z *y *β|y| 2) g(v,[\psi,\psi]) = Re\left( - \gamma |z|^2 + x y z + x^\ast z^\ast y^\ast - \beta |y|^2 \right)

which is close to what we want. The first and last terms in the parentheses are already real and match what we’re shooting for, so we just need to show

Re(xyz+x *z *y *)=2Re(xyz) \mathrm{Re}(x y z + x^\ast z^\ast y^\ast) = 2 \mathrm{Re} (x y z)

For this we use two normed division algebras facts: the cyclic property of the real part, and its invariance under conjugation:

Re(x *z *y *)=Re((yzx) *)=Re(yzx)=Re(xyz) \mathrm{Re}(x^\ast z^\ast y^\ast) = \mathrm{Re}((y z x)^\ast) = \mathrm{Re} (y z x) = \mathrm{Re}(x y z)

So we’re done!   █

Some spinoffs

It follows from the theorem that the group of determinant-preserving transformations of 𝔥 3(𝕂)\mathfrak{h}_3(\mathbb{K}) contains Spin(n+1,n)\mathrm{Spin}(n+1,n). In the case we care about most, this gives an inclusion of Lie groups

Spin(9,1)E 6 \mathrm{Spin}(9,1) \subseteq \mathrm{E}_6

and thus an inclusion of Lie algebras

𝔰𝔬(9,1)𝔢 6 \mathfrak{so}(9,1) \subseteq \mathfrak{e}_6

Now the dimension of 𝔢 6\mathfrak{e}_6 is 78 — or so I’ve claimed without proof. The dimension of 𝔰𝔬(9,1)\mathfrak{so}(9,1) is the triangular number 109/2=4510 \cdot 9 / 2 = 45. Since

dim(𝔢 6)dim(𝔰𝔬(9,1))=7845=33 \mathrm{dim}(\mathfrak{e}_6) - \mathrm{dim}( \mathfrak{so}(9,1)) = 78 - 45 = 33

we could look for an interesting 33-dimensional space whose direct sum with 𝔰𝔬(9,1)\mathfrak{so}(9,1) gives 𝔢 6\mathfrak{e}_6 — as vector spaces, not as Lie algebras. And indeed we have one, since S +S_+ and S S_- are 16-dimensional. It’s S +S S_+ \oplus S_- \oplus \mathbb{R}!

And in fact, there’s a nice way to put a Lie bracket on 𝔰𝔬(9,1)S +S \mathfrak{so}(9,1) \oplus S_+ \oplus S_- \oplus \mathbb{R} to get an isomorphism of Lie algebras

𝔢 6𝔰𝔬(9,1)S +S \mathfrak{e}_6 \cong \mathfrak{so}(9,1) \oplus S_+ \oplus S_- \oplus \mathbb{R}

By ‘nice’, I mean it’s geometrically well-motivated. So we get a description of 𝔢 6\mathfrak{e}_6 in terms of 10-dimensional spacetime geometry!

We can also try this game with division algebras that are less glamorous than the octonions. It’s worth doing, even if we only care about the exceptional case, just to get some analogues that are easier to understand. If we take \mathbb{R}, the same argument winds up showing that

so(2,1)𝔰𝔩(3,) \mathrm{so}(2,1) \subseteq \mathfrak{sl}(3,\mathbb{R})

We then count:

dim(𝔰𝔩(3,))dim(𝔰𝔬(2,1))=83=5 \mathrm{dim}(\mathfrak{sl}(3,\mathbb{R})) - \mathrm{dim}( \mathfrak{so}(2,1)) = 8 - 3 = 5

We should try to copy what worked before. In this case S +=S = 2S_+ = S_- = \mathbb{R}^2 as vector spaces, so S +S S_+ \oplus S_- \oplus \mathbb{R} is 5-dimensional! And indeed we get a nice isomorphism

𝔰𝔩(3,)𝔰𝔬(2,1)S +S \mathfrak{sl}(3,\mathbb{R}) \cong \mathfrak{so}(2,1) \oplus S_+ \oplus S_- \oplus \mathbb{R}

where again ‘nice’ means that it’s motivated by the geometry.

If we use \mathbb{C}, we get

so(3,1)𝔰𝔩(3,) \mathrm{so}(3,1) \subseteq \mathfrak{sl}(3,\mathbb{C})

We then count:

dim(𝔰𝔩(3,))dim(𝔰𝔬(3,1))=166=10 \mathrm{dim}(\mathfrak{sl}(3,\mathbb{C})) - \mathrm{dim}( \mathfrak{so}(3,1)) = 16 - 6 = 10

In this case S +=S = 2S_+ = S_- = \mathbb{C}^2 as vector spaces, so S +S S_+ \oplus S_- \oplus \mathbb{R} is just 9-dimensional as a real vector space. So close and yet so far! But it turns out that everything is okay: we have a nice isomorphism

𝔰𝔩(3,))𝔰𝔬(3,1)S +S \mathfrak{sl}(3,\mathbb{C})) \cong \mathfrak{so}(3,1) \oplus S_+ \oplus S_- \oplus \mathbb{C}

Finally, we can move to the quaternionic case and try the same trick. We get

so(5,1)𝔰𝔩(3,) \mathrm{so}(5,1) \subseteq \mathfrak{sl}(3,\mathbb{H})

The determinant of a quaternionic matrix is a tricky thing, but it’s real valued, so while GL(3,)\mathrm{GL}(3,\mathbb{H}) has real dimension 3×3×4=363 \times 3 \times 4 = 36, it has a Lie subgroup SL(3,)\mathrm{SL}(3,\mathbb{H}) of dimension just one less, namely 3535.

We then count:

dim(𝔰𝔩(3,))dim(𝔰𝔬(5,1))=3515=20 \mathrm{dim}(\mathfrak{sl}(3,\mathbb{H})) - \mathrm{dim}( \mathfrak{so}(5,1)) = 35 - 15 = 20

In this case S +S_+ and S S_- are 8-dimensional, so S +S S_+ \oplus S_- \oplus \mathbb{H} has dimension 20. So I’m willing to guess… but I’m not completely sure… that we get a nice isomorphism

𝔰𝔩(3,)𝔰𝔬(5,1)S +S \mathfrak{sl}(3,\mathbb{H}) \cong \mathfrak{so}(5,1) \oplus S_+ \oplus S_- \oplus \mathbb{H}

I should check this someday.

  • Part 1. How to define octonion multiplication using complex scalars and vectors, much as quaternion multiplication can be defined using real scalars and vectors. This description requires singling out a specific unit imaginary octonion, and it shows that octonion multiplication is invariant under SU(3)\mathrm{SU}(3).
  • Part 2. A more polished way to think about octonion multiplication in terms of complex scalars and vectors, and a similar-looking way to describe it using the cross product in 7 dimensions.
  • Part 3. How a lepton and a quark fit together into an octonion — at least if we only consider them as representations of SU(3)\mathrm{SU}(3), the gauge group of the strong force. Proof that the symmetries of the octonions fixing an imaginary octonion form precisely the group SU(3)\mathrm{SU}(3).
  • Part 4. Introducing the exceptional Jordan algebra 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}): the 3×33 \times 3 self-adjoint octonionic matrices. A result of Dubois-Violette and Todorov: the symmetries of the exceptional Jordan algebra preserving their splitting into complex scalar and vector parts and preserving a copy of the 2×22 \times 2 adjoint octonionic matrices form precisely the Standard Model gauge group.
  • Part 5. How to think of 2×22 \times 2 self-adjoint octonionic matrices as vectors in 10d Minkowski spacetime, and pairs of octonions as left- or right-handed spinors.
  • Part 6. The linear transformations of the exceptional Jordan algebra that preserve the determinant form the exceptional Lie group E 6\mathrm{E}_6. How to compute this determinant in terms of 10-dimensional spacetime geometry: that is, scalars, vectors and left-handed spinors in 10d Minkowski spacetime.
  • Part 7. How to describe the Lie group E 6\mathrm{E}_6 using 10-dimensional spacetime geometry. This group is built from the double cover of the Lorentz group, left-handed and right-handed spinors, and scalars in 10d Minkowski spacetime.
  • Part 8. A geometrical way to see how E 6\mathrm{E}_6 is connected to 10d spacetime, based on the octonionic projective plane.
  • Part 9. Duality in projective plane geometry, and how it lets us break the Lie group E 6\mathrm{E}_6 into the Lorentz group, left-handed and right-handed spinors, and scalars in 10d Minkowski spacetime.
  • Part 10. Jordan algebras, their symmetry groups, their invariant structures — and how they connect quantum mechanics, special relativity and projective geometry.
Posted at November 1, 2020 8:08 PM UTC

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Re: Octonions and the Standard Model (Part 6)

for literature references, isn’t 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) called an Albert Algebra?

Posted by: RodMcGuire on November 2, 2020 12:48 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

Over any field kk we can define the concept of an octonion algebra or Cayley algebra, which is an 8-dimensional nonassociative unital algebra equipped with a nondegenerate quadratic form NN such that N(xy)=N(x)N(y)N(x y) = N(x) N(y). There are many such algebras: for example if k=k = \mathbb{R} there are two, the octonions and the split octonions, and if k=k = \mathbb{C} there is one, the bioctonions. Over finite fields there may be more.

An Albert algebra is defined to be any 27-dimensional Jordan algebra that is ‘exceptional’, meaning the Jordan product is not defined via ab=ab+baa \circ b = a b + b a starting from some (possibly larger) associative algebra. When k=k = \mathbb{R} there are three, one of which is 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}). Only this one is ‘formally real’, meaning that

a 1a 1++a na n=0a 1,,a n=0 a_1 \circ a_1 + \cdots + a_n \circ a_n = 0 \implies a_1, \dots, a_n = 0

But when people, especially physicists, speak of the exceptional Jordan algebra, they usually mean 𝔥 3(𝕆)\mathfrak{h}_3(\mathbb{O}) — and that’s how I’m using the term here.

Posted by: John Baez on November 2, 2020 4:34 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

This is fascinating; thanks for putting it all together. Could

(cf the subsection

Relation to octonionic 3×33\times 3 matrix algebra)

be part of this picture?

Posted by: jackjohnson on November 5, 2020 1:26 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

It’s possible — but as the nLab article points out, it’s just a hope at this point. Since G 3G_3 is not a compact Lie group, it will probably take some delicate homotopy-theoretic work to unearth any further facts about it. That’s how all the information about it has been gotten so far, it seems. I’ve got a lot more to say about E 6,F 4\mathrm{E}_6, \mathrm{F}_4 and the exceptional Lie algebra, but it’s all of a much simpler nature (it seems to me).

Posted by: John Baez on November 5, 2020 4:55 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

Thanks for this great series of posts. Do you have a reference for the Lie bracket you refer to in the last section?

Posted by: anon on November 6, 2020 5:05 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

I’ll describe that Lie bracket in the post I’m writing now. Greg Egan figured it out in a project we did with John Huerta back in November 2015. Someone probably knew it already, but we wanted to work everything out ourselves. Now I want to make all our discoveries public.

Posted by: John Baez on November 6, 2020 8:06 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

Of course everyone knows what you mean, but I would prefer to change “one of the five exceptional compact simple groups” to “one of the five exceptional [connected] simply connected compact simple groups” (since there are also the adjoint quotients of E 6\mathsf E_6 and E 7\mathsf E_7).

Posted by: L Spice on November 6, 2020 7:32 PM | Permalink | Reply to this

Re: Octonions and the Standard Model (Part 6)

Yes, the extra qualifications you need are required for a precise theorem statement. I should also have said five isomorphism classes of…

Occasionally one wants to make an offhand remark that’s not cluttered with fine print. But thanks for reminding everyone about these nonisomorphic Lie groups with isomorphic Lie algebras! Such issues can be really important in physics.

Posted by: John Baez on November 6, 2020 8:04 PM | Permalink | Reply to this

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