On Non-Relativistic Supersymmetry and its Spontaneous Breaking

TL;DR

This paper investigates non-relativistic supersymmetric field theories, analyzing their spontaneous supersymmetry breaking, spectrum, and quantum corrections, revealing preserved supersymmetry but broken scale invariance and IR freedom.

Contribution

It provides a detailed analysis of spontaneous supersymmetry breaking and quantum corrections in non-relativistic supersymmetric theories across various dimensions.

Findings

Supersymmetry remains unbroken at the vacua.

Scale invariance is broken despite supersymmetry preservation.

The theories are IR free with quantum corrections calculated.

Abstract

We study non-relativistic supersymmetric field theories in diverse dimensions. The theories consist of scalars and fermions and possess two, four or eight real supercharges. We analyze their spontaneous supersymmetry breaking structure and calculate the gapless spectrum. We calculate the perturbative quantum corrections at the supersymmetric vacua and show that while supersymmetry is preserved, scale invariance is broken and the theories are IR free.

Tables

Table 1. Table 1 : The internal symmetries of the Lagrangian ( 4 ).

Group	Transformation
$U{\left(1\right)}_{𝕄}$	${\varphi }_1\to e^{-i\alpha /2}{\varphi }_1,{\varphi }_2\to e^{-i\alpha /2}{\varphi }_2,{\psi }_1\to e^{-i\alpha /2}{\psi }_1,{\psi }_2\to e^{-i\alpha /2}{\psi }_2.$
$U\left(1\right)$	${\varphi }_1\to {\varphi }_1,{\varphi }_2\to {\varphi }_2,{\psi }_1\to e^{i\alpha /2}{\psi }_1,{\psi }_2\to e^{i\alpha /2}{\psi }_2$.
$SU{\left(2\right)}_{ℱ}$	${\sigma }_x:{\psi }_1\to \cos \left({\theta }_1/2\right){\psi }_1+i\sin \left({\theta }_1/2\right){\psi }_2,{\psi }_2\to \cos \left({\theta }_1/2\right){\psi }_2+i\sin \left({\theta }_1/2\right){\psi }_1.$
	${\sigma }_y:{\psi }_1\to \cos \left({\theta }_2/2\right){\psi }_1+\sin \left({\theta }_2/2\right){\psi }_2,{\psi }_2\to \cos \left({\theta }_2/2\right){\psi }_2-\sin \left({\theta }_2/2\right){\psi }_1.$
	${\sigma }_z:{\psi }_1\to e^{i{\theta }_3/2}{\psi }_1,{\psi }_2\to e^{-i{\theta }_3/2}{\psi }_2.$
$SU{\left(2\right)}_{ℬ}$	${\sigma }_x:{\varphi }_1\to \cos \left({\theta }_1/2\right){\varphi }_1+i\sin \left({\theta }_1/2\right){\varphi }_2,{\varphi }_2\to \cos \left({\theta }_1/2\right){\varphi }_2+i\sin \left({\theta }_1/2\right){\varphi }_1.$
	${\sigma }_y:{\varphi }_1\to \cos \left({\theta }_2/2\right){\varphi }_1+\sin \left({\theta }_2/2\right){\varphi }_2,{\varphi }_2\to \cos \left({\theta }_2/2\right){\varphi }_2-\sin \left({\theta }_2/2\right){\varphi }_1.$
	${\sigma }_z:{\varphi }_1\to e^{i{\theta }_3/2}{\varphi }_1,{\varphi }_2\to e^{-i{\theta }_3/2}{\varphi }_2.$

Equations

$${\mathcal{L}}_0$$

$${\partial }_{\nu }\to D_{\nu }={\partial }_{\nu }-i\mu c{\delta }_{\nu }^0,\text{where}{\partial }_0=\frac{1}{c}{\partial }_t,$$

$${\psi }_1\to \sqrt{c}{\psi }_1,{\psi }_2\to \frac{1}{\sqrt{c}}{\psi }_2,$$

$${\mathcal{L}}_0$$

$${\mathcal{L}}_1=\frac{g^{-2}q{c}^{-2}}{4}\int d^2\theta d^2\bar{\theta }{\Phi }_1^{\ast }\left(x\right){\Phi }_1\left(x\right){\Phi }_2^{\ast }\left(x\right){\Phi }_2\left(x\right),$$

$${\mathcal{L}}_2=\frac{g^{-2}\lambda c^{-2}}{4}\int d^2\theta d^2\bar{\theta }{\Phi }_1^{\ast }\left(x\right){\Phi }_1\left(x\right){\Phi }_1^{\ast }\left(x\right){\Phi }_1\left(x\right),$$

$${\mathcal{L}}_1=\frac{q}{4}({\varphi }_1{\varphi }_1^{\ast }+{\varphi }_2{\varphi }_2^{\ast }+{\psi }^{\ast }\psi {)}^2,$$

$${\mathcal{L}}_2$$

$$+2{\varphi }_1{{\varphi }_1}^{\ast }{\psi }^{\ast }\psi +{\psi }_2{\psi }_1{\psi }_1^{\ast }{\psi }_2^{\ast }+{\varphi }_1{{\varphi }_1}^{\ast }{\varphi }_2{{\varphi }_2}^{\ast }).$$

$$\delta {\varphi }_1={ϵ}_{[2}{\psi }_{1]},\delta {\varphi }_2=\psi {\epsilon }^{\ast },$$

$$\delta {\psi }_1={ϵ}_1{\varphi }_2-{ϵ}_2^{\ast }{\varphi }_1,\delta {\psi }_2={ϵ}_2{\varphi }_2+{ϵ}_1^{\ast }{\varphi }_1,$$

$$Q_1=\int d^{d}x\left(i{\varphi }_1^{\ast }{\psi }_1-i{\varphi }_2{\psi }_2^{\ast }\right),Q_2=\int d^{d}x\left(i{\varphi }_1^{\ast }{\psi }_2+i{\varphi }_2{\psi }_1^{\ast }\right),$$

$$\delta {\varphi }_1={ϵ}_{[2}{\psi }_{1]},\delta {\varphi }_2=-\psi {\epsilon }^{\ast },$$

$$\delta {\psi }_1=-{ϵ}_1{\varphi }_2-{ϵ}_2^{\ast }{\varphi }_1,\delta {\psi }_2=-{ϵ}_2{\varphi }_2+{ϵ}_1^{\ast }{\varphi }_1.$$

$${\Theta }_1=\int d^{d}x\left(i{\varphi }_1^{\ast }{\psi }_1+i{\varphi }_2{\psi }_2^{\ast }\right),{\Theta }_2=\int d^{d}x\left(i{\varphi }_1^{\ast }{\psi }_2-i{\varphi }_2{\psi }_1^{\ast }\right),$$

$$\mathbb{M}=\int d^{d}x\left({\varphi }_1^{\ast }{\varphi }_1+{\varphi }_2^{\ast }{\varphi }_2+{\psi }^{\ast }\psi \right).$$

$$C=-\int d^{d}x\left({\psi }^{\ast }\psi \right).$$

$${\mathcal{J}}_F^1=\int d^{d}x\left({\psi }_1^{\ast }{\psi }_2+{\psi }_2^{\ast }{\psi }_1\right),$$

$${\mathcal{J}}_F^2=i\int d^{d}x\left(-{\psi }_1^{\ast }{\psi }_2+{\psi }_2^{\ast }{\psi }_1\right),$$

$${\mathcal{J}}_F^3=\int d^{d}x\left({\psi }_1^{\ast }{\psi }_1-{\psi }_2^{\ast }{\psi }_2\right),$$

$$\left\{Q_a,Q_b^{\ast }\right\}=\left\{{\Theta }_a,{\Theta }_b^{\ast }\right\}=\mathbb{M}{\delta }_{ab}.$$

$$\mathcal{V}=-m^2\left({\varphi }_1{\varphi }_1^{\ast }+{\varphi }_2^{\ast }{\varphi }_2+{\psi }^{\ast }\psi \right)+\frac{q}{4}{\left({\varphi }_1{\varphi }_1^{\ast }+{\varphi }_2{\varphi }_2^{\ast }+{\psi }^{\ast }\psi \right)}^2,$$

$${\varphi }_1{\varphi }_1^{\ast }+{\varphi }_2{\varphi }_2^{\ast }+{\psi }^{\ast }\psi =\frac{2m^2}{q},$$

$$\mathcal{L}$$

$$-\frac{q}{2}\sqrt{\frac{2m^2}{q}}\left({\varphi }_1{\varphi }_1^{\ast }+{\varphi }_2{\varphi }_2^{\ast }+{\psi }^{\ast }\psi \right)\left({\varphi }_1+{\varphi }_1^{\ast }\right).$$

$${\mathcal{L}}_{quad}$$

$$+i\left({\varphi }_2^{\ast }{\partial }_t{\varphi }_2-{\varphi }_2{\partial }_t{\varphi }_2^{\ast }\right)-g{\varphi }_2^{\ast }{\nabla }^2{\varphi }_2$$

$$-i\left({\partial }_t{\psi }^{\ast }\psi -{\psi }^{\ast }{\partial }_t\psi \right)-g{\psi }^{\ast }{\nabla }^2\psi ].$$

$${\mathcal{L}}_{quad}$$

$$\mathcal{V}$$

$$+\lambda ({\varphi }_1{{\varphi }_1}^{\ast }{\varphi }_1{{\varphi }_1}^{\ast }-{\psi }_1^{\ast }{\psi }_2^{\ast }{\varphi }_1{\varphi }_2-{\psi }_2{\psi }_1{\varphi }_2^{\ast }{{\varphi }_1}^{\ast }$$

$$+2{\varphi }_1{{\varphi }_1}^{\ast }{\psi }^{\ast }\psi +{\psi }_2{\psi }_1{\psi }_1^{\ast }{\psi }_2^{\ast }+{\varphi }_1{{\varphi }_1}^{\ast }{\varphi }_2{{\varphi }_2}^{\ast }),$$

$$\mathcal{L}$$

$$\begin{array}[]{l}{\phi_{1}}=\sqrt{{Z_{{\phi_{1}}}}}{\phi_{1}}^{r},\qquad{\phi_{2}}=\sqrt{{Z_{{\phi_{2}}}}}{\phi_{2}}^{r},\qquad\psi=\sqrt{{Z_{\psi}}}{\psi^{r}},\\ {\delta_{z{\phi_{1}}}}={Z_{{\phi_{1}}}}-1,\qquad{\delta_{z{\phi_{2}}}}={Z_{{\phi_{2}}}}-1,\qquad{\delta_{z\psi}}={Z_{\psi}}-1,\\ {\delta_{{g}}}=g_{0}-{g},\qquad{\delta_{{m^{2}}}}={m_{0}}^{2}-{m^{2}},\qquad{\delta_{q}}={q_{0}}-q\ .\end{array}$$

Full text

1 Introduction

Relativistic supersymmetry is the unique extension of the space-time Poincaré symmetry algebra. It includes spinor generators $Q$ that map bosonic degrees of freedom to fermionic ones. Relativistic supersymmetric quantum field theories have been studied for several decades. They posses many attractive features that made them leading candidates for an extension of the Standard Model of particle physics (for a review see e.g. Martin:1997ns ). To date, supersymmetry has not been discovered at high energy experiments. On the other hand, there is an accumulated theoretical evidence that emergent supersymmetry may play a role in certain low energy condensed matter systems (see e.g. CMsusy ; CMsusy2 ; aff for some recent work).

The aim of this paper is to study non-relativistic supersymmetric field theories. Such theories are potentially relevant in nature, for instance, to the descriptions of low energy systems. Non-relativistic supersymmetric models can be obtained as limits of relativistic supersymmetry ones when the speed of light is taken to infinity Clark:1983ne . They can also be constructed directly in the non-relativistic regime with no relativistic completion. The non-relativistic field theories may possess non-relativistic boost invariance (Galilean field theories) or not (Lifshitz field theories).

There are significant differences between relativistic supersymmetry and the non-relativistic one. First, relativistic supersymmetry is an extension of space-time symmetry, i.e. the anticommutator $\{Q,Q\}$ yields the bosonic space-time translations. This is not necessarily the case in non-relativistic supersymmetry. The non-relativistic supersymmetry which will be studied in this paper is an internal symmetry. $\{Q,Q\}\sim\mathbb{M}$, where $\mathbb{M}$ is the generator of particle number symmetry which is conserved in non-relativistic field theories 111See, however, Chapman:2015wha for other non-relativistic supersymmetry algebras.. Thus, when this non-relativistic supersymmetry is spontaneously broken, the particle number symmetry must be spontaneously broken too. Second, there is no spin-statistics theorem for non-relativistic field theories. The fermionic generators that we will consider are scalars under the space rotation group and are distinguished from the bosonic scalar generators by their statistics. This allows us to write non-relativistic supersymmetric theories with the same field content in general space dimension $d$.

Non-relativistic field theories may possess the standard non-relativistic scale invariance $t\rightarrow e^{2\sigma}t,\vec{x}\rightarrow e^{\sigma}\vec{x}$, or a more general scale invariance characterized by a dynamical exponent $z$, $t\rightarrow e^{z\sigma}t,\vec{x}\rightarrow e^{\sigma}\vec{x}$. We will consider the standard as well as the general case with even z.

The paper is organized as follows. In section two we will construct the non-relativistic supersymmetric models and the supersymmetry algebra. In section three we will analyze the spontaneous breaking of the non-relativistic models and calculate the spectrum of Nambu-Goldstone (NG) bosons and fermions. In section four we will calculate the quantum corrections at the supersymmetry preserving vacua to all orders in perturbation theory. The last section is devoted to a discussion and outlook. Details of the calculations are outlined in the appendices.

2 The Non-Relativistic Supersymmetric Theory

2.1 A Non-Relativistic Supersymmetry Limit

In the following we will take the non-relativistic limit of $\mathcal{N}=2$ (eight real supercharges) relativistic supersymmetric hypermultiplet Lagrangian in $(3+1)$-dimensional flat spacetime. Relativistic massless fields propagate at the speed of light and do not have a non-relativistic limit with propagating fields. Thus, one has to add a relativistic mass before taking the limit. The $\mathcal{N}=2$ hypermultiplet consists of a chiral and an anti-chiral $\mathcal{N}=1$ multiplets denoted by $\Phi_{1}$ and $\Phi^{*}_{2}$, respectively (we use the notation of Martin:1997ns ). The free field Lagrangian reads:

[TABLE]

where $\mu$ is a mass parameter and $c$ is the speed of light. In order to take the non-relativistic limit deAzcarraga:1991fa ; Jensen:2014wha , we introduce a chemical potential

[TABLE]

rescale the fermionic fields

[TABLE]

use the equation of motion for $\psi_{2}$ and take the limit $c\rightarrow\infty$. One obtains:

[TABLE]

where we redefined $\phi_{1}\rightarrow\phi_{1}^{*},\psi\rightarrow i\psi^{*}$, the fields have been rescaled by appropriate factors of $\mu$, and we denoted $g\equiv\frac{1}{\mu}$. Note, that the non-relativistic fermions $\psi_{a},a=1,2$ are not spinors but rather scalars and the index $a$ enumerates them. We defined the contraction of indices: $\psi^{*}\psi\equiv\sum\limits_{a=1}^{2}{\psi^{*}_{a}\psi_{a}}$.

Next, we will add interactions. The free field Lagrangian (1) possesses a global $U(1)$ symmetry $(\Phi_{1}(\theta),\Phi_{2}(\theta))\rightarrow(e^{i\alpha}\Phi_{1}(\theta),e^{-i\alpha}\Phi_{2}(\theta))$, which we will maintain. The simplest interaction terms contain four superfields:

[TABLE]

and

[TABLE]

where $\lambda$ and $q$ are coupling constant. While $\mathcal{L}_{1}$ preserves the $\mathcal{N}=2$ supersymmetry, $\mathcal{L}_{2}$ breaks it to $\mathcal{N}=1$. All other interactions with four superfields lead to the same non-relativistic interaction terms that read:

[TABLE]

and

[TABLE]

The resulting $(3+1)$-dimensional non-relativistic Lagrangians can be studied in arbitrary number of spacetime dimensions $d+1$ without spoiling any symmetries, since the non-relativistic fermions are singlets under spatial rotations. Also, the non-relativistic supersymmetric model could have been constructed without taking the non-relativistic limit, by directly employing non-relativistic supersymmetry transformations.

2.2 Non-relativistic Supersymmetry

The space-time symmetries of (4) form the Schrödinger algebra, which is the non-relativistic limit of the relativistic conformal algebra Hagen:1972pd ; Niederer:1972zz . It includes space-time translations, spatial rotations, Galilean (non-relativistic) boosts, dilatation and one special conformal transformation. Dilatation $t\rightarrow e^{2\sigma}t,\vec{x}\rightarrow e^{\sigma}\vec{x}$, acts on the fields by $(\phi_{i},\psi)\rightarrow e^{-\frac{d}{2}\sigma}(\phi_{i},\psi)$. As we will see, unlike relativistic supersymmetry, the non-relativistic supersymmetry commutes with space-time symmetries, and is an internal symmetry generated by fermionic charges Clark:1983ne .

${\cal L}_{0}$ is invariant under eight real supersymmetric transformations. Four real supersymmetries are:

[TABLE]

where $\epsilon$ is the infinitesimal fermionic parameter of the supersymmetric transformation. $\psi^{*}\epsilon$ is defined by $\psi^{*}\varepsilon\equiv\sum\limits_{a=1}^{2}{\psi^{*}_{a}\varepsilon_{a}}=-\varepsilon\psi^{*}$, and we denote $\epsilon_{[a}\psi_{b]}=\epsilon_{a}\psi_{b}-\epsilon_{b}\psi_{a}$. The supercharges associated with the supersymmetry transformation (9) are

[TABLE]

and their complex conjugates $Q^{*}$. The other four real supersymmetry transformation symmetries of (4) read

[TABLE]

The supercharges corresponding to (11) are

[TABLE]

and their complex conjugates $\Theta^{*}$. The Lagrangian (4) possesses $SU(2)^{2}\times U(1)^{2}$ internal symmetries listed in table 1. The charge associated with $U(1)_{\mathbb{M}}$ is

[TABLE]

$\mathbb{M}$ is the particle number generator and is a central extension of the symmetry algebra. It appears in the commutator of the space translations $P_{i}$ and Galilean boosts $K_{j}$, $[P_{i},K_{j}]=-i\mathbb{M}\delta_{ij}$. The charge of the second $U(1)$ transformation reads

[TABLE]

The subscripts $\mathcal{B},\mathcal{F}$ of $SU(2)_{\mathcal{B}},\ SU(2)_{\mathcal{F}}$ denote the type of particles which transform non-trivially under the symmetries, where $\mathcal{B}$ refers to bosons and $\mathcal{F}$ refers to fermions. The generators of the two $SU(2)$ symmetries read :

[TABLE]

The supersymmetry algebra takes the form (see also Clark:1983ne ):

[TABLE]

The complete algebra including all the global symmetries is given in appendix A.

The Lagrangian (4) can generalized to the case of an even dynamical exponent $z$, i.e. invariance under the Lifshitz scaling. The internal symmetries in table 1, including the supersymmetry transformations (9), (11) remain the same as well as the algebra in appendix A. The space-time symmetries form now the Lifshitz algebra that includes space and time translations, spatial rotations and Lifshitz scaling. Note, that when $z=d$ the two interactions (7) 222Since $\mathbb{M}$ is a central extension of the supersymmetry algebra, any power of (13) preserves all the supersymmetries and global symmetries. and (8) are marginal and preserve eight and four real supersymmetries, respectively (see also DeFranceschi:1979af ).

3 Spontaneous Breaking of Non-Relativistic Superymmetry

In this section we will analyze the pattern of non-relativistic spontaneous supersymmetry breaking. The supersymmetry algebra (16) dictates that the $U(1)_{\mathbb{M}}$ symmetry must be spontaneously broken too. We will consider potentials with eight and four supersymmetries. In appendix (B) we give an example with two supersymmetries.

3.1 Eight Supersymmetries Broken to Four

Consider the free field Lagrangian (4) with the addition of a potential term

[TABLE]

where $q>0,m^{2}>0$. The analysis of this case has been performed in Clark:1983ne , however, our results for the spectrum of NG bosons and fermions are different. The potential has a moduli space of minima at

[TABLE]

with value $\mathcal{V}_{min}=-\frac{m^{4}}{q}<0$. Expanding the Lagrangian $\mathcal{L}=\mathcal{L}_{0}-\mathcal{V}_{1}$, where $\mathcal{L}_{0}$ is the free field Lagrangian (4), around a mimimum of (18) $\phi_{1}=\sqrt{\frac{2m^{2}}{q}},\phi_{2}=0$ one has

[TABLE]

The gapless spectrum is read from the quadratic part of (19). Define $a=\frac{i}{2}\left(\phi_{1}^{*}-\phi_{1}\right)$, and $b=\frac{1}{2}\left(\phi_{1}^{*}+\phi_{1}\right)$, one gets

[TABLE]

The $b$ field is gapped and can be integrated out, leading to

[TABLE]

The low energy spectrum contains two NG bosons and two NG fermions. The NG boson ($a$) has a linear dispersion relation $\omega\sim k$ (type A). It is associated with the spontaneously broken $U(1)_{\mathbb{M}}$ symmetry. The NG boson ($\phi_{2}$) and the two NG fermions ($\psi$) have a quadratic dispersion relation $\omega\sim k^{2}$ (type B). $\phi_{2}$ is associated with the breaking of $SU(2)_{\mathcal{B}}$ to a $U(1)$ symmetry (see table 1). The two NG fermions are associated with the breaking of four supersymmetry generators. The counting is consistent with the non-relativistic analysis of Watanabe:2011ec ; Watanabe:2012hr , where the number of type A NG particles plus twice the number of type B NG particles is equal to seven, which is the number of broken generators. Note, that there are no additional NG bosons associated with the spontaneous breaking of the Galilean boosts as expected by the inverse Higgs constraints Brauner:2014aha . Similar analysis holds when $z\neq 2$, with the linear dispersion relation replaced by $\omega\sim k^{z/2}$ and the quadratic one by $\omega\sim k^{z}$.

3.2 Four Supersymmetries Broken to Zero

Consider the potential

[TABLE]

where $q>0,m^{2}>0$. We distinguish two cases: $\lambda>0$ and $\lambda<0,q+4\lambda>0$. The case $\lambda=0$ reduces to (17), and in all other cases there are no supersymmetry breaking minima.

When $\lambda>0$, the field that acquires a vev is $\phi_{2}$, $\phi_{2}=\sqrt{\frac{2m^{2}}{q}}$, and the value of the potential is $\mathcal{V}=-\frac{m^{4}}{q}<0$. Expanding the Lagrangian around the mimimum one gets the quadratic part:

[TABLE]

There is one type A NG boson associated with the spontaneous breaking of $U\left(1\right)_{\mathbb{M}}$, and two type B NG fermions associated with the breaking of the four supersymmetries. Unlike the previous case, here there is no $SU\left(2\right)_{\mathcal{B}}$ symmetry that is spontaneously broken. The case $\lambda<0,q+4\lambda>0$ is similar to the previous one with the exchange of the two bosonic fields. $\phi_{1}$ takes the value $\phi_{1}=\sqrt{\frac{2m^{2}}{(q+4\lambda)}}$ at the minimum and the value of the potential $\mathcal{V}=-\frac{M^{4}}{\left(q+4\lambda\right)}<0$. Expanding the Lagrangian around the minimum one gets the quadratic part

[TABLE]

The spectrum is as for $\lambda>0$ with $\phi_{1}$ replaced by $\phi_{2}$.

4 Quantum Corrections

In this section we will calculate the the quantum corrections to the non-relativistic supersymmetric field theories when supersymmetry is not spontaneously broken. We will consider the interactions (7) and (8) with a mass term satisfying $m^{2}<0$ so that there is no spontaneous breaking of supersymmetry.

We will separate the two cases: $z=d=2$ where all integrals can be calculated and even $z=d\neq 2$. We will see that supersymmetry is preserved quantum mechanically while scale invariance is broken. When $d<z$, the interaction terms in (7) and (8) are relevant and the quantum corrections are not divergent. When $d>z$ the interactions are irrelevant and the quantum corrections diverge polynomially.

The propagators for the free field Lagrangian for a general even value of critical exponent $z$ are read from (4) with the replacement $\nabla^{2}\to(\nabla^{2})^{\frac{z}{2}}$. They are given in figure 1, where $(\omega,\vec{k})$ are the frequency and momentum.

The quantum corrections for the model with eight supersymmetries (7) are given in section 4.1. The details of calculation, including the Feynman rules, expressions for the diagrams and results of the scattering amplitudes can be found in appendix C.2. The quantum corrections to the model with four supersymetries are given in section 4.2, where the details of calculation can be found in appendix C.3. We also refer the reader to appendix C.1, where we show that there are $\Lambda^{d}$ divergent corrections to the propagators, where $\Lambda$ is the spatial momentum UV cutoff. However, these corrections, which appear at the one-loop order only, are independent of the external momentum, and as pointed out in Bergman:1991hf can be removed by normal ordering.

4.1 Eight Supersymmetries

In this subsection we study the quantum corrections to the eight real supersymmetries interactions with $z=d$ (7). We show that supersymmetry is preserved to all orders in perturbation theory, while scale invariance is broken. The different sectors of supersymmetry particles do not mix with each other, as shown in figure 2.

Denote :

[TABLE]

There are no external momentum dependent quantum corrections to the propagators of the particles $\phi_{1}$, $\phi_{2}$ and $\psi$. One way to see this is by observing that in these diagrams both propagators have poles only on one side of the integration contour. Since the integrals over the loop frequency converge, one can close the integration contour in the region which does not contain poles Bergman:1991hf ; Fitzpatrick:2012ww ). Therefore,

[TABLE]

to all orders in perturbation theory. Up to constant shifts in the bare mass constants (see appendix C.1), we write the renormalized Lagrangian

[TABLE]

The relevant Feynman rules and details of calculation are given in appendix C.2. The corrections to the vertices are depicted in figure 2.

When $z=d=2$, the summation of the diagrams in figure 2(a) and the tree level value yields

[TABLE]

where $(\omega,p)$ are the total frequency and momentum of the bosonic external legs (see Bergman:1991hf for the calculation with a single self-interacting non-relativistic boson field). The calculation of all diagrams depicted in figure 2 is detailed in appendix C.2.1. The correction to the coupling $q$ reads

[TABLE]

where $\mu$ is an arbitrary physical energy scale. This follows from the requirement that when the external momentum and frequency dependence $gp^{2}-4\omega$ equals the physical energy scale $4\mu^{2}$ the total amplitude for each process takes the tree level value. The $\beta$-function is positive and reads Bergman:1991hf

[TABLE]

Thus scale invariance is broken in perturbation theory and the theory is IR free. The fact that the independent corrections to the different interactions can all be reabsorbed by the same correction $\delta_{q}$ at any order in perturbation theory implies that supersymmetry is preserved in perturbation theory. The $\beta$-function for general $z=d$ is

[TABLE]

In appendix C.2 we detail the relations between the scattering amplitudes in the general $z=d$ case with even $z$. Supersymmetry is preserved in perturbation theory, while scale invariance is broken (31).

4.2 Four Supersymmetries

The renormalized interaction reads

[TABLE]

with $\delta_{\lambda}$ and $\lambda$ defined as $\delta_{\lambda}=\lambda_{0}-\lambda$, and $\lambda_{0}$ is the bare coupling. The details of calculation, including the Feynman rules, expressions for the diagrams and scattering amplitudes are in appendix C.3.

For the $z=d=2$ case one has

[TABLE]

The $\beta$-function reads

[TABLE]

and for a general even value of $z=d$

[TABLE]

The $\beta$-function is positive and scale invariance is broken quantum mechanically. The fact that the independent corrections to the different interactions in (32) can all be reabsorbed by the same correction $\delta_{\lambda}$ at any order in perturbation theory implies that supersymmetry is preserved prerturbatively.

5 Summary and Outlook

We studied the pattern of supersymmetry breaking and the quantum structure of non-relativistic supersymmetric models with diverse number of supercharges. Supersymmetry is an internal fermionic symmetry in these models and the structure of its breaking is compatible with the spontaneous symmetry breaking pattern of global symmetries in non-relativistic field theories. The quantum analysis of the model at the supersymmetry preserving vacua indicates that while supersymmetry is preserved in perturbation theory, scale invariance is broken. The perturbative $\beta$-functions are positive, implying that the theories are IR free and require a UV completion.

There are various interesting directions to follow. While relativistic supersymmetry algebras are classified, this is not so in the non-relativistic case where supersymmetry can be an internal or spacetime symmetry. Such a classification is clearly desirable. Another natural direction to follow is to generalize the basic models studied in this work and consider other possible supersymmetric multiplets and interactions.

The fermions in the models that we studied are grassmann variables that are singlets under the space rotation group. This follows from the fact that the spin-statistics theorem does not hold in non-relativistic theories. For our analysis, however, other representation for the fermions could have been chosen. The question that naturally arises is, what distinguishes the different cases. This can have potential applications to low energy systems where non-relativistic supersymmetry may arise as an emergent symmetry. One can, for instance, couple the non-relativistic theory to non-singlet external sources such as gauge fields (see e.g. Alexandre:2013wua ; Festuccia:2016caf ) that can distinguish the various representations. It would be interesting to explore this and construct observable effects.

We studied the models at the supersymmetry preserving vacuum. The quantum analysis at the supersymmetry breaking vacua is challenging and the issue of UV completion deserves further study. While there is a natural UV completion by a relativistic supersymmetric field theory, there may be other, perhaps non-relativistic, interesting completions.

Finally, in our models scale invariance is broken quantum mechanically, and it would be interesting to construct scale invariant non-relativistic supersymmetric theories. Here one expects a rich structure of scale anomalies Jensen:2014hqa ; Arav:2016xjc .

**Acknowledgment **

We would like to thank Igal Arav for valuable discussions and Carlos Hoyos for a discussion on spontaneous symmetry breaking in the model with four supersymmetries. This work is supported in part by the I-CORE program of Planning and Budgeting Committee (grant number 1937/12), the US-Israel Binational Science Foundation, GIF and the ISF Center of Excellence. A.R.M gratefully acknowledges the support of the Adams Fellowship Program of the Israel Academy of Sciences and Humanities.

Appendix A The Supersymmetry Algebra

The non-vanishing commutaion relations of the supersymmetry algebra written in table 1 are:

[TABLE]

$a,b=1,2$, $i,j,k=1,2,3$, $\varepsilon_{ijk}$ is the Levi-Civita tensor $\varepsilon_{123}=1$, and the Pauli matrices ${{\sigma^{i}}_{a}}^{b}$ are:

[TABLE]

Appendix B A Model with Two Supercharges

Consider the Lagrangian

[TABLE]

where $\phi$ is a complex bosonic field, $\psi$ is a complex one component Grassmann field and $z$ is an even integer. The Lagrangian is invariant under the supersymmetry transformation

[TABLE]

The corresponding two supercharges are given by

[TABLE]

and its complex conjugate. The supersymmetric anti-commutations relation reads

[TABLE]

where $\mathbb{M}$ is the central extension given by

[TABLE]

The supersymmetry invariant mass term is

[TABLE]

and four-fields supersymmetry invariant interaction reads :

[TABLE]

Note, that since the fermion is a one component complex Grassman field, terms containing four fermions vanish. Consider the Lagrangian

[TABLE]

where we assume $q>0$. Similar to the analysis made in section 3, when $m^{2}\leqslant 0$ there is no SSB. When $m^{2}>0$ $\phi$ acquires a vev $\left\langle\phi\right\rangle=\sqrt{\frac{2m^{2}}{q}}$. Expanding the Lagrangian around the classical minimum one finds

[TABLE]

The massless NG fields are one type A ($\phi_{1}$) boson with a dispersion relation $\omega\sim k^{z/2}$ associated with the broken $U(1)_{\mathbb{M}}$ symmetry, and one type B fermion ($\psi$) with dispersion relation $\omega\sim k^{z}$ associated with the breaking of supersymmetry.

Appendix C Derivation of the Scattering Amplitudes and Quantum Corrections

In this appendix we outline the details of the calculation of the quantum corrections in section 4. In appendix C.1, we show that there are $\Lambda^{d}$ divergent corrections to the propagators which do not cancel by supersymmetry. In sections C.2 and C.3 the details of calculations of the quantum corrections to the models with eight and four supersymmetries are given.

C.1 The Divergent $\Lambda^{d}$ Correction

When considering the field theory of each of the individual sectors alone ($\phi_{1}$, $\phi_{2}$, $\psi_{1}$, $\psi_{2}$ ), with a four-fields self interaction, one finds that there are $\Lambda^{d}$ divergences in the corrections to the propagators which arise only at the one-loop order. However, all $\Lambda^{d}$ divergences, which arise from diagrams such as those depicted in figure 3, do not depend on external momenta and can be absorbed by a re-definition of the mass term. As pointed out in Bergman:1991hf , they can be removed by normal ordering.

These divergences do not cancel by supersymmetry, unlike e.g. the supersymmetric models studied in Chapman:2015wha . For instance, for the interaction written in (7), the corrections to the bosonic propagator for $z=d$ (figure 3) read

[TABLE]

where $\Lambda$ is a spatial momentum UV cutoff.

C.2 Quantum Corrections and Scattering Amplitudes for the Eight Supercharges Model

The Feynman rules for the vertices correspond to the model in (27) are given by figure 4.

C.2.1 The $z=d=2$ Case

In the case of $z=2$ the integrals can be calculated. In order to evaluate the different amplitudes for the diagrams drawn in figure 2 we briefly review the derivation of the first diagram on the right hand side of the equality mark (one loop) in figure 2(a). This was already calculated in Bergman:1991hf . The expression for the diagram is given by the following

[TABLE]

where $(\omega,p)$ are the frequency and momentum of the external bosonic leg of the diagram. Preforming the integral over the frequency while closing the contour on the lower half plane, after a change of variables $l=k+\frac{1}{2}p$ we get

[TABLE]

and

[TABLE]

Summing the tree level diagram $iq$ and the diagrams in figure 2(a) gives Bergman:1991hf

[TABLE]

The amplitude for the scattering process containing two external legs of $\phi_{2}$ and two of $\phi^{*}_{2}$ is the same as the result (69), that is

[TABLE]

The amplitude for the process containing four external legs of $\phi_{1}$, $\phi_{2}$, $\phi_{1}^{*}$ and $\phi_{2}^{*}$ is given by

[TABLE]

The diagrams in figure 2(b) together with the tree level diagram in 4(c) give

[TABLE]

The diagrams in figure 2(d) together with the tree level 4(e) (or with $\phi_{1}$ and $\phi_{1}^{*}$ replaced by $\phi_{2}$ and $\phi_{2}^{*}$) result in

[TABLE]

C.2.2 A General $z=d$ Case

In the case of $d=z$ where $z$ is an even integer, the value of the integral $\mathcal{BL}$ changes. We are interested only in the UV divergent part extracted from the general expression for $\mathcal{BL}$, which allows us to deduce the $\beta$-function. In this case we have

[TABLE]

Picking up the pole in the lower half plane one finds

[TABLE]

where we used spherical symmetry. The UV divergent part reads

[TABLE]

where we have neglected the terms which are finite in the UV, which agrees with the UV divergent part of (68) when $d=z=2$. The $\beta$-function of the coupling $q$ is

[TABLE]

The quantum corrections remain the same as those depicted in figure 2, and the scattering amplitudes as in section C.2.1 with $\mathcal{BL}$ replaced by the expression for a general value of $z=d$ in equation (77). The relations between the scattering amplitudes remain unchanged and supersymmetry preserved. Scale invariance breaks down as implied by the nonzero $\beta$-function (78).

C.3 Quantum Corrections and Scattering Amplitudes for the Four Supercharges Model

The Feynman rules for the interaction in (32) are depicted in figure 5.

C.3.1 The $z=d=2$ Case

The quantum corrections to the vertex in figure 5(a) are of the same form as those depicted in figure 2(a), with the replacement $iq\to 4i\lambda$. The amplitude of the scattering process is therefore as in (69) with the replacement $iq\to 4i\lambda$,

[TABLE]

Similarly, the vertex in figure 5(c) receive the same quantum corrections as in figure 2(d) with the same replacement $iq\to 4i\lambda$. Therefore, the amplitude is again as in equation (74) with the appropriate replacement,

[TABLE]

The relations between the amplitudes (79) and (80) are the same relations between the amplitudes (69) and (74) and are compatible with supersymmetry. However, there is still a need to verify the relations between the other vertices in this model and their quantum corrections.

The quantum corrections to the four fermions vertex are depicted in figure 6(c). The resulting amplitude together with the tree-level in figure 5(b) is given by

[TABLE]

The quantum corrections to the vertex in 5(d) are depicted in figure 6(b). The resulting amplitude together with the tree-level 5(d) is given by

[TABLE]

The quantum corrections to the vertex in 5(c) are depicted in figure 6(a). The resulting amplitude together with the tree-level 5(c) is given by

[TABLE]

Similar to the same definition used in section 4.1, we define that when the external momentum and frequency dependence $gp^{2}-4\omega$ equals the physical energy scale $4\mu^{2}$ the total amplitude for each process equals the tree level value of the same coupling. This is obtained for all the amplitudes (79)-(83) by choosing the following counter term

[TABLE]

which will keep the structure of the original vertices at the energy scale $\mu$. Similarly to the model in 4.1, this theory also possesses a positive beta function (34).

C.3.2 A General $z=d$ Case

As in section C.2.2, the UV divergent part of the quantum corrections for the theory in (32) are the same as those of section C.3.1, with $\mathcal{BL}$ replaced by the expression for a general $z=d$ (77). Again the relations between the scattering amplitudes in section C.3.1 remain the same and supersymmetry is preserved. The resulting $\beta$-function is 35.