text:
\section{S1. Microscopic theory}
In this section, we derive a quasiclassical framework and the Bogoliubov--de Gennes (BdG) equation from an interacting neutron system via zero-range attractive ${}^{3}P_{2}$ force. The derivation can be also referred to our previous paper\cite{Masaki:2019rsz}. The starting microscopic Hamiltonian $H$ is composed of the one-body terms $H_{1}$ and the interaction term $H_{2}$ given, respectively, in the following:
\begin{align}
H_{1} = \int d \bm{r} \sum_{\sigma,\sigma^{\prime}=\uparrow,\downarrow}
\psi_{\sigma}^{\dagger}(\bm{r})[h_{0}(-\mathrm{i} \bm{\nabla})\delta_{\sigma,\sigma^{\prime}} + U_{\sigma\sigma^{\prime}}]\psi_{\sigma^{\prime}}(\bm{r}),~~~~~
H_{2} = - \int d \bm{r} \sum_{\alpha\beta= x,y,z}\dfrac{g}{2}T_{\alpha\beta}^{\dagger}(\bm{r})T_{\alpha\beta}(\bm{r}),
\end{align}
where $H_{1}$ consists of the kinetic energy $h_{0}(-\mathrm{i} \bm{\nabla}) = (-\nabla^{2}/2m - \mu)$ measured from the chemical potential $\mu$, and the Zeeman energy $\hat{U}(\bm{r}) = -V_{\mathrm{Z}}\hat{\sigma}_{z}$ along the $z$ axis; $\hat{\cdot}$ denotes a 2 $\times$ 2 matrix in the spin space. The $^{3}P_{2}$ force with coupling strength $g > 0$ is represented by $H_{2}$, and the pair creation and annihilation operators $T^{\dagger}$ and $T$ are defined, respectively, by
\begin{align}
\hat{T}_{\alpha\beta}^{\dagger}(\bm{r}) = \sum_{\sigma,\sigma^{\prime}}
\psi_{\sigma}^{\dagger}(\bm{r})[t_{\alpha\beta,\sigma\sigma^{\prime}}^{*} (\mathrm{i} \bar{\bm{\nabla}})\psi_{\sigma^{\prime}}^{\dagger}(\bm{r})],~~\text{and}~~~
T_{\alpha\beta}(\bm{r}) = \sum_{\sigma\sigma^{\prime}}[t_{\alpha\beta,\sigma\sigma^{\prime}}(-\mathrm{i} \bar{\bm{\nabla}})\psi_{\sigma^{\prime}}(\bm{r})]\psi_{\sigma}(\bm{r}).
\end{align}
We have introduced a spin-momentum coupling in the pair force via the 2 $\times$ 2 matrix in spin space $\hat{t}_{\alpha\beta}$ defined by
\begin{align}
\hat{t}_{\alpha\beta}(-\mathrm{i} \bar{\bm{\nabla}})
=\hat{t}_{\alpha\beta}(-\mathrm{i} \bm{\nabla}/k_{\mathrm{F}})
=\mathrm{i} \hat{\sigma}_{y}\left\{\dfrac{1}{2\sqrt{2}}\left[
\hat{\sigma}_{\alpha}(-\mathrm{i} \bar{\nabla}_{\beta})
+ \hat{\sigma}_{\beta}(-\mathrm{i}\bar{\nabla}_{\alpha})\right]
-\dfrac{1}{3\sqrt{2}}\delta_{\alpha\beta}\hat{\bm{\sigma}}\cdot(-\mathrm{i} \bar{\bm{\nabla}})
\right\}
=[\hat{t}_{\alpha\beta}^{*}(\mathrm{i}\bar{\bm{\nabla}})]^{*}.
\end{align}
Following Ref.~\cite{Masaki:2019rsz}, we obtain the quasiclassical transport equation called the Eilenberger equation:
\begin{align}
0 = \mathrm{i} \bm{v}_{\mathrm{F}} \cdot \bm{\nabla}\check{g} + [\mathrm{i} \omega_{n}\check{\tau}_{z} + \check{u} + \check{\sigma}_{\Delta},\check{g}],
\end{align}
where $\check{\cdot}$ is a 4 $\times$ 4 matrix in the spin and Nambu space, $\check{\tau}_{z} = \mathrm{diag}(1,1, -1, -1)$ is the third component of the  Pauli matrices in the Nambu space, $\check{u} = V_{\mathrm{Z}}\mathrm{diag}(\hat{\sigma}_{z},\hat{\sigma}_{z}^{\mathrm{tr}})$ denotes the Zeeman field. The quasiclassical propagator $\check{g}$ is defined by
\begin{align}
\check{g}(\bm{k}_{\mathrm{F}},\bm{R};\mathrm{i}\omega_{n})
&= \begin{bmatrix}\hat{g} & \hat{f} \\ -\hat{\bar{f}} & \hat{\bar{g}}\end{bmatrix}
= \oint_{C_{\mathrm{qc}}}\dfrac{d\xi}{ \mathrm{i} \pi}\check{G}(\bm{k},\bm{R};\mathrm{i} \omega_{n}),\\
\check{G}(\bm{k},\bm{R};\mathrm{i}\omega_{n})
&= \int_{0}^{\beta}d \tau e^{\mathrm{i}\omega_{n} \tau}
\int d (\bm{r}_{1} - \bm{r}_{2})e^{-\mathrm{i} \bm{k}\cdot(\bm{r}_{1} - \bm{r}_{2})}
\check{\tau}_{z}\braket{\mathcal{T}_{\tau}\vec{\Psi}(\bm{r}_{1},\tau)\vec{\Psi}^{\dagger}(\bm{r}_{2})}
\end{align}
In the first line, the integral with respect to the energy $\xi = k^{2}/2m - \mu$ is performed along the contour $C_{\mathrm{qc}}$, which consists of the counterclockwise contour in the half upper $\xi$ plane and the clockwise contour in the half lower $\xi$ plane. Here, $\bm{R} = (\bm{r}_{1} + \bm{r}_{2})/2$ is a coordinate to describe the spatial inhomogeneity of the superfluid order parameter,
$\mathcal{T}_{\tau}$ is an imaginary time ordered operator, and the Nambu spinor $\vec{\Psi}$ has been introduced as $\vec{\Psi}(\bm{r},\tau)
=(\psi_{\uparrow}(\bm{r},\tau),\psi_{\downarrow}(\bm{r},\tau),\psi_{\uparrow}^{\dagger}(\bm{r},\tau),\psi_{\downarrow}^{\dagger}(\bm{r},\tau))$ with $\psi_{\sigma}^{(\dagger)}(\bm{r},\tau) = e^{H\tau}\psi_{\sigma}^{(\dagger)}(\bm{r})e^{-H\tau}$. The order parameter matrix is defined by
\begin{align}
\check{\sigma}_{\Delta}(\bm{k}_{\mathrm{F}},\bm{R}) =  \begin{bmatrix}\hat{0} & \hat{\Delta} \\  -\hat{\Delta}^{\dagger} & \hat{0}\end{bmatrix},~~~
\hat{\Delta}(\bm{k}_{\mathrm{F}},\bm{R})
= \sum_{\alpha\beta}\mathcal{A}_{\alpha\beta}(\bm{R})\hat{\sigma}_{\alpha}\mathrm{i} \hat{\sigma}_{y}\bar{k}_{\mathrm{F},\beta},
\end{align}
where $\mathcal{A}_{\alpha\beta}$ is a 3 $\times$ 3 order parameter tensor of a spin-triplet $p$-wave superfluid, and $\bar{\bm{k}}_{\mathrm{F}} \equiv \bm{k}_{\mathrm{F}}/k_{\mathrm{F}}$ is a normalized Fermi momentum parametrized as $(\cos\alpha\sin\chi, \sin\alpha\sin\chi, \cos\chi)$. The order parameter tensor $\mathcal{A}$ is connected to the anomalous quasiclassical propagator $\hat{f}$ by the gap equation
\begin{align}
\mathcal{A}_{\alpha\beta}
&= -\dfrac{\Delta_{\alpha\beta}(\bm{R}) + \Delta_{\beta\alpha}(\bm{R})}{2\sqrt{2}} + \dfrac{\sum_{\gamma}\Delta_{\gamma\gamma}(\bm{R})}{3\sqrt{2}}, \\
\Delta_{\alpha\beta}(\bm{R}) &= g\nu_{\mathrm{n}} \mathrm{i} \pi T\sum_{n: |\omega_{n}| \le \omega_{\mathrm{c}}}\braket{\mathrm{Tr} \hat{t}_{\alpha\beta}(\bar{\bm{k}}_{\mathrm{F}})\hat{f}(\bm{k}_{\mathrm{F}},\bm{R};\mathrm{i}\omega_{n})}_{\mathrm{F}},
\end{align}
where $g$ is the strength of the coupling constant and $\nu_{\mathrm{n}}$ is the density of state for the normal state at the Fermi energy, and $\braket{\cdots}_{\mathrm{F}}$ denotes the Fermi surface average defined by $\int d \alpha \int d \cos \chi/(4\pi) [\cdots]$. The cut-off energy of the Matsubara summation is denoted by $\omega_{\mathrm{c}}$ and related to $g\nu_{\mathrm{n}}$ as
\begin{align}
\dfrac{3}{g\nu_{\mathrm{n}}} = \log \dfrac{T}{T_{\mathrm{c}}} +  \sum_{n: |\omega_{n}| < \omega_{\mathrm{c}}}\dfrac{\pi}{\omega_{n}}.
\end{align}
An order parameter profile with a vortex is determined by
self-consistently  solving the Eilenberger equation and the gap equations with the boundary condition explained below. In order to study the interaction energy of the HQVs, we utilize the Luttinger--Ward energy functional:
\begin{align}
\mathcal{J}_{\mathrm{sn}}
= \dfrac{\nu_{\mathrm{n}}}{2}
\int_{0}^{1}d \lambda \mathrm{Sp}\left[\check{\sigma}_{\Delta}\left(\check{g}_{\lambda} - \dfrac{1}{2}\check{g}\right)\right],
\end{align}
where $\mathrm{Sp}[\cdots] = \mathrm{i} \pi T \sum_{n} \int d \bm{R} \braket{\mathrm{Tr}[\cdots]}_{\mathrm{F}}$, and $\check{g}_{\lambda}$ is the solution to the equation $[\mathrm{i} \omega_{n} \check{\tau}_{z} + \check{u} + \lambda\check{\sigma}_{\Delta},\check{g}_{\lambda}] + \mathrm{i} \bm{v}_{\mathrm{F}}\cdot\bm{\nabla}\check{g}_{\lambda} = 0$.

The Bogoliubov--de Gennes (BdG) equation also can be derived following Ref.~\cite{Masaki:2019rsz} as,
\begin{align}
&\check{\mathcal{H}}_{\mathrm{BdG}}(\bm{R})\vec{u}_{\nu}(\bm{R}) = \epsilon_{\nu} \vec{u}_{\nu}(\bm{R}),\\
&\check{\mathcal{H}}_{\mathrm{BdG}}(\bm{R}) =
\begin{pmatrix}
h_{0}(-\mathrm{i} \bm{\nabla})\hat{1} + \hat{U} & \hat{\Delta}(\bm{R}) \\
-\hat{\Delta}^{*}(\bm{R}) & -h_{0}(\mathrm{i} \bm{\nabla})\hat{1} - \hat{U}^{\mathrm{tr}}
\end{pmatrix},
\label{eq:bdg}
\end{align}
where $\hat{1}$ is the 2 $\times$ 2 identity matrix, and the gap matrix is given, using the anticommutator $\{a,b\}_{+} = ab + ba$, by
\begin{align}
\hat{\Delta}(\bm{R}) = \dfrac{\hat{\sigma}_{\alpha}\hat{\sigma}_{y}}{2k_{\mathrm{F}}}\left\{\mathcal{A}_{\alpha\beta}(\bm{R}),\nabla_{\beta}\right\}_{+}.
\end{align}

\section{S2. Boundary Condition and Basis Tensor of $\mathcal{A}$.}
\label{sec:bc}

In this section, we detail the boundary conditions for isolated HQVs and a pair of HQVs.
For this purpose, it is convenient to expand the order parameter tensor $\mathcal{A}_{\alpha\beta}$ with respect to the $z$-component of the total angular momentum as $\mathcal{A}_{\alpha\beta}(\bm{R}) = \sum_{M = -2}^{2}\gamma_{M}(\bm{R})\Gamma_{M,\alpha\beta}$, where
$\Gamma_{M}$ is the 3 $\times$ 3 basis tensor with the angular momentum $M$ such that $J_{z} \Gamma_{M} = M \Gamma_{M}$, and $\gamma_{M}(\bm{R})$ is a complex scalar function and denotes the projected order parameter to the sector $M$. The operation $J_{z}$ on a tensor $\mathcal{A}$
is written down as $[J_{z}\mathcal{A}]_{\alpha\beta} = \mathcal{A}_{\alpha\gamma}\mathrm{i}\epsilon_{z \gamma \beta} - \mathrm{i} \epsilon_{z\alpha\gamma} \mathcal{A}_{\gamma\beta}$ with antisymmetric tensor $\epsilon_{\alpha\beta\gamma}$.
A representation of $\Gamma_{M}$ is given by
\begin{align}
\Gamma_{\pm2} = \dfrac{1}{2}
\begin{pmatrix}
1 & \pm \mathrm{i} & 0 \\
\pm \mathrm{i} & - 1 & 0\\
0 & 0 & 0
\end{pmatrix},~~
\Gamma_{\pm1} = \dfrac{1}{2}
\begin{pmatrix}
0 & 0 & \mp 1\\
0 & 0 & -\mathrm{i} \\
\mp 1 & -\mathrm{i} & 0
\end{pmatrix},~~
\Gamma_{0} = \dfrac{1}{\sqrt{6}}
\begin{pmatrix}
-1 & 0 & 0\\
0 & -1 & 0 \\
0 & 0 & 2
\end{pmatrix}.\end{align}
The $D_{4}$-BN state with point node along the $z$ axis is represented for this basis set as $|\gamma_{2}| = |\gamma_{-2}|$ and $\gamma_{0,\pm1} = 0$. In the following, we consider asymptotic forms of vortices, which give boundary conditions for the above equation set.
An integer vortex for such a $D_{4}$-BN state has an asymptotic form:
\begin{align}
\mathcal{A}_{\alpha\beta}(\theta) = \sum_{M=\pm2}e^{ \mathrm{i} \kappa \theta}\gamma_{M}\Gamma_{M,\alpha\beta}~~(\kappa = \pm1).
\end{align}
This boundary condition breaks the axial symmetry
which is described by a form $\mathcal{A} = \sum_{M}e^{\mathrm{i} (\kappa - M)\theta}\gamma_{M}\Gamma_{M,\alpha\beta}$.
In addition to such a non-axisymmetric integer vortex, a HQV is topologically allowed in the $D_{4}$-BN state. Its asymptotic form is given by
\begin{align}
\mathcal{A}_{\alpha\beta}(\theta) = \sum_{M=\pm2}e^{ \mathrm{i} (\kappa - n M) \theta}\gamma_{M}\Gamma_{M,\alpha\beta}~~(\kappa = \pm 1/2, n = \pm1/4),  \label{eq:bc-hqv}
\end{align}
which indicates that there are two kinds of HQVs in terms of the relative sign between $\kappa$ and $n$. Without loss of generality, we set $\kappa = 1/2$ in the main text and in the following. It is proposed that an integer vortex with $\kappa = 1$ can split into two HQVs with $(\kappa,n) = (1/2, 1/4)$ and $(\kappa,n) = (1/2, -1/4)$\cite{Masuda:2016vak}. Such a configuration is schematically given as follows: Let a vortex center with $n=-1/4$ ($n=1/4$) be $\bm{R}_{1}$ $(\bm{R}_{2})$, and define the polar angle measured from its center as $\theta_{1}$ ($\theta_{2}$). An asymptotic form of two HQVs which is equivalent to that of a single integer vortex is given by
\begin{align}
\mathcal{A} = \sum_{M=\pm2} e^{\mathrm{i} (\kappa + nM)\theta_{1} + \mathrm{i} (\kappa - nM)\theta_{2}}\gamma_{M}\Gamma_{M,\alpha\beta}~~(\kappa = 1/2, n = 1/4), \label{eq:bc-twohqvs}
\end{align}
 where the phase behaves as $2 \kappa \theta$ for $|\bm{R}| \to \infty (\theta_{1,2} \to \theta)$.

\begin{figure}
\includegraphics[width=\hsize]{gap_v1.pdf}
\caption{HQV with $(\kappa,n) =(1/2, -1/4)$.
	     (a) Total intensities $[\sum_{M}|\gamma_{M}|^{2}]^{1/2}$.
	     (b) Schematic image of the boundary condition.
	     (c), (e), (g) Amplitudes $|\gamma_{M}|$ for $M = -2$, $0$ ,and $2$.
	     (d), (f), (h) Phases $\tan^{-1}(\gamma_{M})$ for $M = -2$, $0$ ,and $2$.
	 	}
\label{fig:-1/4}
\end{figure}
\begin{figure}
\includegraphics[width=\hsize]{gap_v3.pdf}
\caption{HQV with $(\kappa,n) =(1/2, 1/4)$.
	     (a) Total intensities $[\sum_{M}|\gamma_{M}|^{2}]^{1/2}$.
	     (b) Schematic image of the boundary condition.
	     (c), (e), (g) Amplitudes $|\gamma_{M}|$ for $M = -2$, $0$ ,and $2$.
	     (d), (f), (h) Phases $\tan^{-1}(\gamma_{M})$ for $M = -2$, $0$ ,and $2$.}
\label{fig:1/4}
\end{figure}

\section{S3. Isolated Half Quantum Vortices}
\label{sec:hqv}

In this section, we present self-consistent solutions of isolated HQVs. As mentioned in the previous section and in the main text,
there are two kinds of HQVs characterized by $n = \pm 1/4$ implying two possible rotational directions of the triad relative to the vorticity.
In Fig.~\ref{fig:-1/4}, a HQV solution with $(n,\kappa) = (1/2, -1/4)$ is shown. The relative phase of $\gamma_{2}$ and $\gamma_{-2}$ is set to zero in Eq.~\eqref{eq:bc-hqv}, and the schematic image of the boundary condition is shown in panel (b). In panel (b), $\theta$ denotes the azimuthal angle in the real space and the red dashed line implies the branch cut. The colored arrows in each circle object represent the direction of the $d$ vectors, whose color bar is identical to those of panels (b), (f), and (h). The cyan and the magenta lines in each object stand for the directions of the eigenvalues $1$ and $-1$ of $\mathcal{A}_{\alpha\beta}(\bm{R})$, respectively. Panel (a) shows the total amplitude defined by $\{\frac{3}{2}\mathrm{Tr}\braket{[\hat{\Delta}(\bm{k}_{\mathrm{F}},\bm{R})]^{\dagger}\hat{\Delta}(\bm{k}_{\mathrm{F}},\bm{R})}_{\mathrm{F}}\}^{1/2} = [\sum_{M}|\gamma_{M}(\bm{R})|^{2}]^{1/2}$. Panels (c), (e), and (g) show $|\gamma_{-2}|$, $|\gamma_{0}|$, and $|\gamma_{2}|$, respectively, while panels (d), (f), and (h) show the corresponding phase $\arg (\gamma_{M})$. As expected from the boundary condition, the sector $M = -2$ has a single winding, while the sector $M = 2$ has no winding, which results in an almost uniform amplitude profile. It is remarkable that the amplitude of induced component $M=0$ seem three fold. Its phase winding around the core is single but opposite to the winding in $M=-2$. Although the phase change along the loop around the core is non linear, the opposite single winding can be understood as an analogy to a vortex in a spinless chiral $p$-wave superconductor. The gap matrices contributed from the sectors $M = - 2$ and $M=0$ are given, respectively, by
\begin{align}
\hat{\Delta}_{-2} = \gamma_{-2}(\bm{R})
\begin{pmatrix}
0 & 0 \\
0 & \bar{k}_{x} - \mathrm{i} \bar{k}_{y}
\end{pmatrix},~~
\hat{\Delta}_{0} = \dfrac{\gamma_{0}(\bm{R})}{\sqrt{6}}
\begin{pmatrix}
\bar{k}_{x} - \mathrm{i} \bar{k}_{y} & 0 \\
0 & - (\bar{k}_{x} + \mathrm{i} \bar{k}_{y})
\end{pmatrix}, \label{eq:gap-matrix:-1/4}
\end{align}
where we set $\bar{k}_{z} = 0$ for simplicity. In the case of an axisymmetric vortex in a spinless chiral $p$-wave superconductor,
the induced component has the opposite chirality against the component which has non-zero order parameter far from the vortex core \cite{Heeb1999,MatsumotoHeeb2001}. Here we call the latter component the {\it bulk component}. In this case, the vorticity of the induced component is determined such that a simultaneous rotation in the real space and the momentum space gives the same phase change between the bulk component and the induced component. In more details, let $\kappa_{\mathrm{b}}$ ($\kappa_{\mathrm{i}}$) and $\chi_{\mathrm{b}}$ ($\chi_{\mathrm{i}}$) be the vorticity and  chirality of the bulk component (the induced component), respectively. The chirality is defined so that $\bar{k}_{x} + \mathrm{i} \chi \bar{k}_{y} = e^{\mathrm{i} \chi \alpha}$, and it takes either $1$ or $-1$, and $\chi_{\mathrm{i}} = -\chi_{\mathrm{b}}$. The phase factor is given by $\kappa_{\mathrm{b}} \theta + \chi_{\mathrm{b}}\alpha$ and $\kappa_{\mathrm{i}} \theta + \chi_{\mathrm{i}}\alpha$, and the simultaneous rotation by angle $\Delta \theta$ gives the phase change $(\kappa_{\mathrm{b}} + \chi_{\mathrm{b}})\Delta \theta$ and $(\kappa_{\mathrm{i}} + \chi_{\mathrm{i}})\Delta \theta$, respectively. Therefore, the vorticity for the induced component is determined as
$\kappa_{\mathrm{i}} = \kappa_{\mathrm{b}} + \chi_{\mathrm{b}} - \chi_{\mathrm{i}} = \kappa_{\mathrm{b}} + 2 \chi_{\mathrm{b}} \equiv (\kappa_{\mathrm{b}} + \chi_{\mathrm{b}}) + \chi_{\mathrm{b}}$, where $\kappa_{\mathrm{b}} + \chi_{\mathrm{b}}$ is the sum of the vorticity and  chirality, characterizing two inequivalent vortices in chiral $p$-wave superconductors.
By applying this argument to the present HQV case, the winding of the induced component is obtained as follows: From Eqs.~\eqref{eq:gap-matrix:-1/4} and \eqref{eq:bc-hqv}, $\kappa_{\mathrm{b}} = 1$ and $\chi_{\mathrm{b}} = -1$ for $M = -2$, and thus we obtain $\kappa_{\mathrm{i}} = - 1$. This is consistent with the opposite single winding indicated by panel (f). Again we remark that the phase change is non linear and the amplitude does not enjoy the axial symmetry in the present case. In terms of the spin sectors, the winding in the bulk component appears only in the spin down sector as seen from Eq.~\eqref{eq:gap-matrix:-1/4}.

Next, we present a self-consistent solution of the other isolated HQV. In order to describe the HQV in the left hand side of a pair of the HQVs, we shift the phase of $\gamma_{-2}$ by $\pi$ in Eq.~\eqref{eq:bc-hqv}, as seen from Eq.~\eqref{eq:bc-twohqvs} by setting $\theta_{1} = \pi$ for $\bm{R}_{2} = (0,0)$ and $\bm{R}_{1}=(\infty, 0)$. The numerical solution of this HQV is shown in Fig.~\ref{fig:1/4}. The meaning of each panel is the same as in Fig.~\ref{fig:-1/4}. The boundary condition schematically shown in panel (b) stands for the opposite rotation compared with Fig.~\ref{fig:-1/4}(b).
Correspondingly, the sector with $M = -2$ has no winding, while that with $M=2$ has a single winding. The gap matrix contributed from the sector $M=2$ is written down as
\begin{align}
\hat{\Delta}_{2} = -\gamma_{2}(\bm{R})
\begin{pmatrix}
\bar{k}_{x} + \mathrm{i} \bar{k}_{y} & 0 \\  0 & 0
\end{pmatrix}.\label{eq:gap-matrix:1/4}
\end{align}
It can be seen that only the spin-up sector in the bulk component has the winding in this case,
in contrast to Eq.~(\ref{eq:gap-matrix:-1/4}) for the spin-down sector in the previous case.
 The winding of the induced component can be understood by applying the above argument. In the present case, it follows from Eqs.~\eqref{eq:bc-hqv} and \eqref{eq:gap-matrix:1/4} that $\kappa_{\mathrm{b}} = 1$ and $\chi_{\mathrm{b}}= 1$ for $M=2$, while $\chi_{\mathrm{i}} = -1$ for the spin-up sector of $M=0$ as seen from Eq.~\eqref{eq:gap-matrix:-1/4}.
Therefore, we obtain $\kappa_{\mathrm{i}} = 3$, which is consistent with the winding indicated by Fig.~\ref{fig:1/4}(f). We note that its change is nonlinear as well as the previous HQV. Correspondingly, the amplitude $|\gamma_{0}|$ is five fold,
in contrast to a three-fold symmetry in the previous case.

\section{S4. Mass Current and Spin Current for a Pair of HQVs}
\begin{figure}
\includegraphics[width=0.9\hsize]{spin_current.pdf}
\caption{(a) Mass current $j_{\mathrm{m}}$ and (b) spin current $j_{\mathrm{s}}^{z}$ for the $z$ component for a pair of HQVs.
            In each panel, the direction of the in-plane current is indicated by the colors and the directions of the arrows,
            while its intensity is indicated by the lengths of the arrows and the colormap behind the arrows.
            }
\label{fig:current}
\end{figure}
In this section, we show the spatial profiles of the mass current density $j_{\mathrm{m}}$ and the spin current density with spin along the $z$ axis $j_{\mathrm{s}}^{z}$ for a pair of HQVs.
Within the quasiclassical theory, these currents are calculated by
\begin{align}
\bm{j}_{\mathrm{m}}(\bm{R})
&= \dfrac{\mathrm{i} \pi T \nu_{\mathrm{n}}}{2m}\sum_{n:|\omega_{n}|\le \omega_{\mathrm{c}}}\mathrm{Tr}\left[\braket{{\bm{k}}_{\mathrm{F}}\check{\tau}_{z}\check{g}^{M}(\bm{k}_{\mathrm{F}},\bm{R};\mathrm{i}\omega_{n})}_{\mathrm{F}}\right],
\\
j_{\mathrm{s}}^{z}(\bm{R})
&= \dfrac{\mathrm{i} \pi T \nu_{\mathrm{n}}}{2m}\sum_{n:|\omega_{n}|\le \omega_{\mathrm{c}}}\mathrm{Tr}\left[\braket{{\bm{k}}_{\mathrm{F}}\check{\tau}_{z}\check{g}^{M}(\bm{k}_{\mathrm{F}},\bm{R};\mathrm{i}\omega_{n})\check{S}_{z}}_{\mathrm{F}}\right],
\end{align}
where $\check{S}_{\mu = x,y,z} = \mathrm{diag}(\hat{\sigma}_{\mu},\hat{\sigma}_{\mu}^{\mathrm{tr}})/2$. The summations over the Matsubara frequency are cut-off by $\omega_{\mathrm{c}}$ which is used for the above gap equation, and it is (at least) qualitatively correct. In Fig.~\ref{fig:current}, we show the in-plane components of $j_{\mathrm{m}}$ in panel (a) and $j_{\mathrm{s}}^{z}$ in panel (b). The currents along the $z$ axis is zero, and the spin currents for $\mu = x$ and $y$ are zero as well. In each panel, the colored arrows show the direction of the current and its intensity, and the colormap behind the arrows also indicates the intensity of the current. The mass current reflects the vorticity of the two HQVs, and it rotates in the same sense around the two cores. In the region far from the core, it gradually decays in a way similar to one for a single integer vortex. Between the two cores, the mass currents contributed from the two cores cancel out. The spin current has an opposite behavior against the mass current: it rotates in the opposite sense between the cores because the localized states contributing to the current have opposite spins. As a result, the contributions far from the cores vanishes, while the region between the cores have rather strong flows.

\section{S5. Symmetry and topology of vortex-bound states in the $D_{4}$-BN phase}

Here we discuss the symmetry and topology of zero-energy states bound at a molecule of non-Abelian HQVs in the $D_{4}$-BN state. For comparison, we also show the axisymmetric $o$-vortex in the $D_{4}$-BN state, which is the most symmetric vortex with normal core, hosting multiple Majorana zero modes. In Ref.~\cite{Masaki:2019rsz}, we demonstrated that under constraints of the axial symmetry of vortices, the $\varv$ vortex with the uniaxial-nematic superfluid core is thermodynamically stable in low magnetic fields, while the $o$ vortex becomes stable as the magnetic field increases. We also found that the $o$ vortex has topologically-protected zero-energy modes, while the axisymmetric $\varv$ vortex has a finite excitation gap in the low-lying quasiparticle spectrum. In this work, we investigate the stability and microscopic structure of non-Abelian HQVs without assuming axial symmetry. As mentioned in the main text, the low-lying quasiparticle structure in the HQV is distinct from those of the $o$ vortex and $\varv$ vortex, since a single zero energy state appears at each core of HQVs. Below, we uncover the robustness and non-Abelian anyonic nature of the zero-energy states bound at a molecule of non-Abelian HQVs on the basis of symmetry and topology.

\subsection{S5.1. Symmetry classification}

To unveil the symmetry and topology of vortices, following Refs.~\cite{tsutsumiPRB15,mizushimaJPSJ16,shiozakiPRB14}, we start with the semiclassical approximation where the Hamiltonian varies slowly in the real-space coordinate. The Bogoliubov quasiparticle structure is governed by the BdG Hamiltonian in Eq.~\eqref{eq:bdg}. The $^{3}P_{2}$ order parameter in the BdG Hamiltonian has the spatial modulation due to a vortex line. In the semiclassical approximation, the spatial modulation is considered as adiabatic changes as a function of the real-space coordinate surrounding the defect with an angle $\theta$, where we introduce the cylindrical coordinate ${\bm R}=(\rho,\theta,z)$. Then, the BdG Hamiltonian in the base space, $(\bm{k},\theta)$ is obtained from Eq.~\eqref{eq:bdg}, as
\begin{align}
\check{\mathcal{H}}({\bm k},\theta)
= \begin{pmatrix}
{h}_0({\bm k})\hat{1}+\hat{U} & \hat{\Delta}({\bm k},\theta) \\
\hat{\Delta}^{\dag}({\bm k},\theta) & -h_{0}({\bm k})\hat{1} - \hat{U}^{\mathrm{tr}}
\end{pmatrix},
\label{eq:bdg2}
\end{align}
where $\hat{U}$ is the Zeeman energy due to a magnetic field ${\bm H}$, and the $2\times 2$ spin matrix of the $^{3}P_{2}$ pair potential is given by
\begin{align}
\hat{\Delta}({\bm k},\theta) = i \hat{\sigma}_{\mu}\mathcal{A}_{\mu i}(\theta) k_i/k_{\mathrm{F}} \hat{\sigma}_{y}.
\end{align}
Here we consider the $D_{4}$-BN phase of  $^{3}P_{2}$ superfluids. The asymptotic form of the order parameter with an isolated vortex satisfies the boundary condition
\begin{align}
\mathcal{A}_{\mu i}(\theta) = \Delta_0 e^{i\kappa\theta}R_n(\theta)
\begin{pmatrix}
1 & 0 & 0 \\ 0 & -1 & 0 \\ 0 & 0 & 0
\end{pmatrix}R^{\mathrm{tr}}_{n}(\theta),
\label{eq:bc}
\end{align}
where $R^{(z)}_n(\theta)\in \mathrm{SO}(2)$ is the rotation matrix about $z$ axis by angle $n\theta$
\begin{align}
R^{(z)}_n(\theta) = \begin{pmatrix}
\cos(n\theta)  & -\sin(n\theta) & 0 \\ \sin(n\theta) & \cos(n\theta) & 0 \\ 0 & 0 & 1
\end{pmatrix}.
\end{align}
We assume the spatial uniformity of the order parameter along the vortex line, i.e., the $z$-axis. The parameters $\kappa$ and $n$ in Eq.~\eqref{eq:bc} represents the $\mathrm{U}(1)$ phase winding and the $n$-fold texture of the $D_{4}$-BN order along the azimuthal angle $\theta$, respectively (see Fig.~1 in the main text).

\begin{table*}[t!]
\caption{\label{table1}Classification of vortices for the $D_{4}$-BN phase in terms of the vorticity $\kappa$, the $n$-fold rotation of the $D_{4}$-BN order, the mirror ($M_{xy}$) and $P_{3}$ (magnetic $\pi$ rotation) symmetries, and topological invariants $\mathrm{Ch}_{2}\in 2\mathbb{Z}$, $\nu_{\lambda}\in\mathbb{Z}_{2}$, and $w_{\mathrm{1d}}\in\mathbb{Z}$, where $\lambda=\pm i$ is the eigenvalue of $M_{xy}$. The column ``Core states'' corresponds to the superfluid components which may be induced around the vortex core (also see the discussion below Eq.~\eqref{eq:p3tr}), and ``non-Abelian'' is the existence of the zero-energy state (ZES) which has the nature of a non-Abelian anyon. We numerically confirmed the self-consistent solutions of axisymmetric $o$- and $\varv$-vortices in addition to HQVs, while no stable solutions of $u$, $w$, and $u \varv w$ vortices have been found with assuming  the axial symmetry.}
\begin{ruledtabular}
\begin{tabular}{cccccccccccccc}
& & Symmetry & $M_{xy}$ & $\kappa$ & $n$ & Core states & $\mathrm{Ch}_{2}$ & $(\nu_{\lambda=+i},\nu_{\lambda=-i})$ & $|w_{\mathrm{1d}}|$ & ZES & Non-Abelian anyon \\
\hline
&$o$ vortex & $P_{1},P_{2},P_{3}$  & $\surd$   & $\mathbb{Z}$ & $\mathbb{Z}$ & Re$\gamma_{0}$ & 0 & $(1,-1)$ & 2 & Yes & Yes  & \\
&$u$ vortex & $P_{1}$ & --- & $\mathbb{Z}$ & $\mathbb{Z}$ & $\gamma_0$  &   &  &  &  & & \\
&$\varv$ vortex & $P_{2}$ & --- & $\mathbb{Z}$ & $\mathbb{Z}$ & $\mathrm{Re}\gamma_{\pm 1}$, $\mathrm{Re}\gamma_0$  & 0  & --- & --- & No & & \\
&$w$ vortex & $P_{3}$ & --- & $\mathbb{Z}$ & $\mathbb{Z}$ & $\mathrm{Im}\gamma_{\pm 1}$, $\mathrm{Re}\gamma_0$  &   &  &  & & & \\
&$u \varv w$ vortex & --- & --- & $\mathbb{Z}$ & $\mathbb{Z}$ & $\gamma_{0,\pm 1}$  &   &  &  &  &  & \\
& HQV       & $P_{3}$ & $\surd$ & $\mathbb{Z}+ 1/2$ & $\mathbb{Z}\pm 1/4$ & $\mathrm{Re}\gamma_0$ &  0 &  $(1,0)$ or $(0,-1)$ & 1 & Yes & Yes & \\
\end{tabular}
\end{ruledtabular}
\label{table:critical_exponents}
\end{table*}

Let us consider systems invariant under a $\mathrm{U}(1)$ gauge transformation and an $\mathrm{SO}(3)$ spin-momentum rotation. The continuous symmetry group, $G=\mathrm{U}(1)\times \mathrm{SO}(3)$, acts on the the $3\times 3$ traceless symmetric tensor, $\mathcal{A}_{\mu i}$, as
$\mathcal{A} \rightarrow e^{i\varphi}g\mathcal{A}g^{\mathrm{tr}}$, where $e^{i\varphi}\in \mathrm{U}(1)$ and $g\in\mathrm{SO}(3)$ are elements associated with a gauge transformation and simultaneous spin-orbit rotation, respectively. The $D_{4}$-BN order, $\mathcal{A}_{\mu i}^{\mathrm{BN}}$, is invariant under the dihedral-four ($D_{4}$) group, whose elements $(e^{i\alpha},g)$ are
\begin{align}
D_{4} = \{ (1,{\bm 1}), (-1,R^{z}_{4}),  (1, I^{z}), (-1,I^{z}R_{4}^{z}), (1, I^{x}), (1, I^{y})\},
\label{eq:D4}
\end{align}
where $I^{j}$ and $R^z_4$ represent $\pi$ rotations around the $j$-axis ($j=x,y,z$) and $\pi/2$ ($n=4$) rotations around the $z$ axis, respectively, and ${\bm 1}$ is the $3\times 3$ unit matrix. The OP manifold in the $D_{4}$-BN state is then characterized by the broken symmetry, $R=[\mathrm{U}(1)\times \mathrm{SO}(3)]/D_{4}$. The topological charges of line defects are characterized by the first homotopy group
\begin{align}
\pi_{1}(R) = \mathbb{Z}\times_{h} D_{4}^{\ast}
\end{align}
where $\times_{h}$ denotes a product
defined in Ref.~\cite{Kobayashi:2011xb}.
This ensures two different classes of topological line defects: Vortices with commutative topological charges and vortices with non-commutative topological charges. The former includes the $o$ and $\varv$ vortices, while an example of the latter is the non-Abelian HQV. Integer vortices are characterized by $\kappa \in \mathbb{Z}$ and $n\in\mathbb{Z}$ in Eq.~\eqref{eq:bc}. The HQV has a half integer of vorticity, $\kappa \in \mathbb{Z}+1/2$, which is accompanied by the $\pi$ jump in the $\mathrm{U}(1)$ phase, $e^{\pm i\theta/2}$. In the $D_{4}$-BN state, however, as the order parameter tensor has the $D_{4}$ symmetry as in Eq.~\eqref{eq:D4},
$R^z_4 \mathcal{A}^{\mathrm{BN}} R^{z\mathrm{tr}}_4 = - \mathcal{A}^{\mathrm{BN}} $,
the discontinuity is compensated by the 4-fold rotation with $n \in \mathbb{Z} \pm 1/4$. For $\kappa>0$, the choice of $n=+1/4$ ($-1/4$) corresponds to the clockwise (counterclockwise) texture of the $D_{4}$-BN gap structure along the azimuthal direction.

It is convenient to expand $\mathcal{A}_{\mu\nu}$ in terms of the eigenstate of the total angular momentum $J_{z}$, $\Gamma_{M}$, as in Sec.~S2. In this basis, the $D_{4}$-BN order parameter is composed of the equal contributions of the $M=+2$ and $M=-2$ components, where the former (latter) corresponds to the Cooper pairing with angular momentum $L_{z}=+1$ ($-1$) and spin angular momentum $S_{z}=+1$ ($-1$).
On the basis of $\Gamma_{M}$, the vortex state can be expressed as
\begin{align}
\mathcal{A}_{\mu\nu}(\rho,\theta) = \sum_{M=-2}^{2} \gamma_{M}(\rho,\theta) \Gamma_{M,\mu\nu}.
\label{eq:ansatz}
\end{align}
Particularly, the asymptotic form of an isolated HQV at $\rho \rightarrow \infty$ is obtained from Eq.~\eqref{eq:bc} as
\begin{align}
\mathcal{A}_{\mu\nu}(\theta) = \sum_{M=-2,2} \gamma_{M} e^{i \kappa_{M} \theta} \Gamma_{M,\mu\nu}.
\end{align}
The winding number of Cooper pairs with $J_{z}=M$, $\kappa_{M}$, must be an integer, $\kappa_{M}\in\mathbb{Z}$, and is represented by $\kappa_{M} = \kappa \theta - \varphi$. An isolated HQV is characterized by the vorticity $\kappa = 1/2$ and the rotation angle of the triad $\varphi = n\theta = + \theta/4$ ($\varphi = -\theta/4$).
The combinations of $(\kappa,n)$ in the other vortices are summarized in Table~\ref{table1}. On the basis of the eigenstate $\Gamma_{M}$, as mentioned above, the asymptotic form of the HQV is recast into the superposition of the $ L_{z}=S_{z}=+1$ Copper pairs with vorticity $\kappa _{M=+2} =0$ ($1$) and the $L_{z}=S_{z}=-1$ Copper pairs with vorticity $\kappa _{M=-2} =1$ ($0$), i.e., $(k_{x}+ik_{y})\ket{\uparrow\uparrow}+e^{i\theta}(k_{x}-ik_{y})\ket{\downarrow\downarrow}$ for $(\kappa,n)=(1/2,1/4)$. As mentioned in Sec.~S3 and the main text, however, the superfluid component $\gamma_{M=0}$ appears around the vortex core within the length scale of $\xi$.

Let us now summarize the symmetries of the BdG Hamiltonian in Eq.~\eqref{eq:bdg}. The BdG Hamiltonian with line defects in three-dimensional system belongs to the class D in the ten-fold way of the Altland-Zrinbauer symmetry classes~\cite{Schnyder:2008tya}. The Hamiltonian breaks the time-reversal symmetry but holds the particle-hole symmetry
\begin{align}
\check{\mathcal{C}} \check{\mathcal{H}}({\bm k},\theta) \check{\mathcal{C}}^{-1} = -\check{\mathcal{H}}(-{\bm k},\theta),
\label{eq:phs}
\end{align}
where $\check{\mathcal{C}} = \check{\tau}_{x} K$ ($K$ is the complex conjugation operator).

In addition to the particle-hole symmetry, three different types of discrete symmetries, $\{P_{1},P_{2},P_{3}\}$, are relevant to vortices. These symmetry operators are composed of discrete elements of the symmetry group $G$, such as the time-reversal operator $\hat{\mathcal{T}}=-i\hat{\sigma}_{y}K$, the spatial inversion ${P}$, the discrete phase rotation $U_{\pi}=e^{i(\kappa+1)\pi}$, and the joint $\pi$-rotation about an axis perpendicular to the vortex line (e.g., the $x$ axis), $\hat{C}_{2,x}=e^{-i\hat{J}_{x}\pi}$. The elements of such symmetry are given by
\begin{align}
\hat{P}_{1}=PU_{\pi}\hat{1}, ~ \hat{P}_{3} = \hat{\mathcal{T}}\hat{C}_{2,x},
\end{align}
and $\hat{P}_{2}=\hat{P}_{1}\hat{P}_{3}$. For a vortex preserving these symmetries, the BdG Hamiltonian in Eq.~\eqref{eq:bdg2} obeys
\begin{align}
\check{\mathcal{P}}_{1} \check{\mathcal{H}}(k_{x},k_{y},k_{z},\theta) \check{\mathcal{P}}_{1}^{-1} &= \check{\mathcal{H}}(-k_{x},-k_{y},-k_{z},\theta+\pi), \\
\check{\mathcal{P}}_{3} \check{\mathcal{H}}(k_{x},k_{y},k_{z},\theta) \check{\mathcal{P}}_{3}^{-1} &= \check{\mathcal{H}}(-k_{x},k_{y},k_{z},-\theta)
\end{align}
where $\check{\mathcal{P}}_{3} \equiv \mathrm{diag}(\hat{P}_{1},\hat{P}_{1}^{\ast})$ and $\check{\mathcal{P}}_{3} \equiv \mathrm{diag}(\hat{P}_{3},\hat{P}_{3}^{\ast})=\mathrm{diag}(i \hat{\sigma}_{z}, -i \hat{\sigma}_{z})K$
 are the $P_{1,2,3}$ operators extended to the Nambu space. The $o$ vortex is the most symmetric vortex preserving all discrete symmetries, $\{P_{1},P_{2},P_{3}\}$.
The $P_{3}$ operator composed of the $\pi$-rotation about the $x$ axis and $\mathcal{T}$ flips the momentum and spin as ${\bm k}\rightarrow (-k_{x},k_{y},k_{z})$ and ${\bm \sigma}\rightarrow (\sigma_{x},-\sigma_{y}-\sigma_{z})$ and changes the azimuthal angle $\theta\rightarrow -\theta$. The $^{3}P_{2}$ order parameter is transformed as
\begin{align}
P_{3}:~\mathcal{A}(\theta) \rightarrow \begin{pmatrix}
 \mathcal{A}^{\ast}_{xx}(-\theta) & -\mathcal{A}^{\ast}_{xy}(-\theta) & -\mathcal{A}^{\ast}_{xz}(-\theta) \\
-\mathcal{A}^{\ast}_{xy}(-\theta) &  \mathcal{A}^{\ast}_{yy}(-\theta) &  \mathcal{A}^{\ast}_{yz}(-\theta) \\
-\mathcal{A}^{\ast}_{xz}(-\theta) &  \mathcal{A}^{\ast}_{yz}(-\theta) &  \mathcal{A}^{\ast}_{zz}(-\theta)
\end{pmatrix}, \label{eq:p3tr}
\end{align}
corresponding to $\gamma_{M}(\rho,\theta) \rightarrow (-1)^{M}\gamma^{\ast}_{M}(\rho,-\theta)$. In the $D_{4}$-BN state, an axisymmetric vortex represented by Eq.~\eqref{eq:ansatz} with $\gamma_{M}(\rho,\theta)=\gamma_{M}e^{i(\kappa - M )\theta}$ maintains the $P_{3}$ symmetry when $\mathrm{Re}\gamma_{\pm 1}(\rho)=0$.
The $P_{1}$ symmetry requires the order parameters to satisfy the relations, $\gamma_{M}(\rho, \theta) = -\gamma_{M}(\rho,\theta+\pi)$. For axisymmetric vortices, this implies that nonvanishing $\gamma_{\pm 1}$ or an even $\kappa_{M}$ breaks the $P_{1}$ symmetry.
In the same manner, the $P_{2}$ symmetry leas to the relations $\gamma_{M}(\rho,\theta) \rightarrow -(-1)^{M}\gamma^{\ast}_{M}(\rho,-\theta+\pi)$. For axisymmetric vortices with an odd $\kappa$, the $P_{2} $ symmetry is preserved if $\mathrm{Im}\gamma_{M}(\rho)=0$.
The vortex state preserving only the $P_{2}$ ($P_{3}$) symmetry is referred to as the $\varv$-vortex ($w$-vortex) state. As discussed in Sec.~S3 and Figs.~S2 and S3, the nonvanishing $\gamma_0$ component induced around the core breaks the axial symmetry but satisfies $\gamma_0(\rho,\theta) = \gamma^{\ast}_0(\rho,-\theta)$. In addition, no $\gamma_{\pm 1}$ components are induced. Hence, the HQV maintains the $P_{3}$ symmetry. Table~\ref{table1} summarizes the possible classes of vortices in terms of these discrete symmetries. In the previous work~\cite{Masaki:2019rsz}, we demonstrated that only $o$ vortex and $\varv$ vortex are the stable solution of the self-consistent equations, while the no stable solutions of the $u$-, $w$, and $u \varv w$ vortex are obtained in the $D_{4}$-BN state with the constraints of the axial symmetry.

The mirror reflection with respect to the $xy$-plane is defined as the following transformation of the real-space, the momentum, and the spin variables: $(x,y,z)\rightarrow (x,y,-z)$, $(k_{x},k_{y},k_{z})\rightarrow (k_{x},k_{y},-k_{z})$, and $(\sigma_{x},\sigma_{y},\sigma_{z})\rightarrow (-\sigma_{x},-\sigma_{y},\sigma_{z})$. For systems with spatial uniformity along the $z$-axis, only the momentum and spin variables transform under the mirror reflection since the BdG Hamiltonian does not depend on $z$. The mirror reflection operator in the spin space, $M_{xy}$, is simply given by $\hat{M}_{xy}=i\hat{\sigma}_{z}$.
When the $^{3}P_{2}$ superfluid order parameter is invariant under the mirror reflection symmetry, the operator acts as
\begin{align}
\hat{M}_{xy} \hat{\Delta}({\bm k},\theta) \hat{M}_{xy}^{\mathrm{tr}} = \eta\hat{\Delta}(k_{x},k_{y},-k_{z},\theta).
\end{align}
As the parity under the mirror reflection, $\eta=\pm$, is compensated by the discrete $\mathrm{U}(1)$ rotation, the mirror operator in the Nambu space is given as
$\check{\mathcal{M}}^{\eta}_{xy} = \mathrm{diag}(\hat{M}_{xy},\eta \hat{M}^{\ast}_{xy})$.
The BdG Hamiltonian \eqref{eq:bdg} is invariant under mirror reflection symmetry, i.e.,
\begin{align}
\check{\mathcal{M}}^{\eta}_{xy}\check{\mathcal{H}}({\bm k},\theta) \check{\mathcal{M}}^{\eta \dag}_{xy} = \check{\mathcal{H}}(k_{x},k_{y},-k_{z},\theta).
\label{eq:mirrorBdG}
\end{align}
The mirror reflection operator thus acts on the symmetric traceless tensor $\mathcal{A}_{\mu i}$ as
\begin{align}
M_{xy}: ~ \mathcal{A}_{\mu i} \rightarrow \begin{pmatrix}
-\mathcal{A}_{xx} & -\mathcal{A}_{xy} & \mathcal{A}_{xz} \\
-\mathcal{A}_{xy} & -\mathcal{A}_{yy} & \mathcal{A}_{yz} \\
\mathcal{A}_{xz} & \mathcal{A}_{yz} & -\mathcal{A}_{zz}
\end{pmatrix}.
\label{eq:mirror}
\end{align}
Therefore, the BdG Hamiltonian is invariant under the mirror reflection if $\mathcal{A}_{xz} = \mathcal{A}_{yz}=0$, i.e., $\gamma_{M=\pm 1} = 0$. This condition can be satisfied by the $o$ vortex and the non-Abelian HQVs. In Table~\ref{table1}, we summarize the symmetry and topology of the several classes of topological line defects in the $D_{4}$-BN states.

\subsection{S5.2. Topological invariants for vortex-bound states}

One of the topological invariants appropriate for line defects in the Altland-Zrinbauer symmetry class D is the second Chern number~\cite{teo,tsutsumiPRB15}. Consider the BdG Hamiltonian at an infinite point from a vortex, $\check{\mathcal{H}}({\bm k},\theta)$, which is obtained from Eq.~\eqref{eq:bdg} on the four-dimensional space $({\bm k},\theta)$ as $\check{\mathcal{H}}({\bm k},\theta)=\lim _{\rho \rightarrow \infty}\check{\mathcal{H}}({\bm k},{\bm R})$. The second Chern number is given by
\begin{align}
\mathrm{Ch}_{2} = \frac{1}{8\pi^{2}} \int _{S^{3}\times S^{1}} \mathrm{tr}\left[
\mathcal{F}\wedge \mathcal{F}
\right],
\end{align}
where $\mathcal{F} = d{A} + {A}\wedge {A}$ is the non-Abelian field strength in the four-dimensional base space. Let $\ket{u_n({\bm k},\theta)}$ be the $n$th occupied eigenstate of $\check{\mathcal{H}}({\bm k},\theta)$. The non-Abelian Berry's connection, $A_{nm}^{\alpha}$, is defined with the eigenstates as
\begin{align}
A^{\alpha}_{nm} = -i\braket{u_{n}({\bm k},\theta)| \partial _{\alpha} u_{m}({\bm k},\theta)}.
\end{align}
Here we introduce $(\partial_{1},\partial_{2},\partial_{3},\partial_{4}) \equiv (\partial_{k_{x}},\partial_{k_{y}},\partial_{k_{z}}, \partial_{\theta})$ with $\alpha = 1, 2,3,4$. Owing to the particle-hole symmetry, the value of the second Chern number in the class D is even, i.e., $\mathrm{Ch}_{2}=2\mathbb{Z}$~\cite{teo}. Hence, the nontrivial value of $\mathrm{Ch}_{2}$ ensures the appearance of paired Majorana fermions at a topological line defect. It has also been pointed out that the second Chern number vanishes in the presence of the $P_{1}$ symmetry~\cite{tsutsumiPRB15}, and thus the $o$ vortex has $\mathrm{Ch}_{2}=0$. We also find that the Chern number in the other vortices is trivial, $\mathrm{Ch}_{2}=0$.

When the BdG Hamiltonian \eqref{eq:bdg2} satisfies Eq.~\eqref{eq:mirrorBdG} and keeps the mirror reflection symmetry, one can introduce a topological number called the mirror
$\mathbb{Z}_{2}$ number: Since the mirror invariant BdG Hamiltonian commutes with the mirror operator, it can be block diagonal by using the eigenvalues of the mirror operator. Here we should emphasize that the zero-energy vortex-bound state can be the Majorana zero mode only for $\check{\mathcal{M}}_{xy}^{\eta=-}$ while the mirror $\mathbb{Z}_{2}$ number can be defined for both of the two possible mirror symmetries $\check{\mathcal{M}}_{xy}^{\eta = \pm}$.
This is because the particle-hole symmetry is still supported within each subsector for $\check{\mathcal{M}}_{xy}^{-}$ but not for $\check{\mathcal{M}}_{xy}^{+}$.
In terms of the Altland-Zrinbauer symmetry classes,
each subsector for $\check{\mathcal{M}}_{xy}^{-}$ belongs to the class D as well as spinless chiral superconductors.
In contrast, for $\check{\mathcal{M}}_{xy}^{+}$, each mirror subsector does not maintain the particle-hole symmetry, and its Hamiltonian belongs to the class A, like a quantum Hall state. Thus, the zero-energy states behave as Majorana fermions only for $\check{\mathcal{M}}^{-}_{xy}$ and only Dirac fermions can be obtained for $\check{\mathcal{M}}^{+}_{xy}$. For $\check{\mathcal{M}}^{-}_{xy}$, if the $\mathbb{Z}_{2}$ invariant is odd, the vortex can host a single Majorana zero mode which behaves as a non-Abelian (Ising) anyon~\cite{ueno,sato14,tsutsumiJPSJ13}.

As mentioned in Eq.~\eqref{eq:mirror}, the BdG Hamiltonian for the $o$ vortex and the non-Abelian HQVs is invariant under $\check{\mathcal{M}}_{xy}^{-}$ if $\mathcal{A}_{xz} = \mathcal{A}_{yz}=0$, i.e., $\gamma_{M=\pm 1} = 0$. On the mirror reflection invariant plane at ${\bm k}_{\mathrm{M}}\equiv (k_{x},k_{y},k_{z}=0)$, the BdG Hamiltonian is commutable with $\check{\mathcal{M}}_{xy}^{-}$, $[\check{\mathcal{H}}({\bm k}_{\mathrm{M}},\theta),\check{\mathcal{M}}_{xy}^{-}]=0$. Hence, the BdG Hamiltonian is block-diagonal to the $2\times 2$ submatrices, $\tilde{\mathcal{H}}_{\lambda}({\bm k}_{\mathrm{M}},\theta)$,
in terms of the eigenvalues of the mirror operator $\lambda = \pm i$
as
\begin{align}
\check{\mathcal{H}}({\bm k}_{\mathrm{M}},\theta) = \bigoplus_{\lambda}\tilde{\mathcal{H}}_{\lambda}({\bm k}_{\mathrm{M}},\theta)
\end{align}
where $\tilde{\mathcal{H}}_{\lambda}({\bm k}_{\mathrm{M}},\theta)$ is still subject to the particle-hole symmetry with $\tilde{\mathcal{C}}=\tilde{\tau}_{x}K$ ($\tilde{\tau}_{\mu=x,y,z}$ are the $2\times2$ Pauli matrix in a reduced subspace) and belongs to the class D in each mirror subsector. Then, the BdG Hamiltonian, $\tilde{\mathcal{H}}_{\lambda}$, is obtained on the base space $({\bm k}_{\mathrm{M}},\theta) \in S^{2}\times S^{1}$, which is composed of the two-dimensional mirror-invariant momentum space and a loop enclosing the line defect on the mirror invariant plane in the real space. The topological invariant for the Altland-Zrinbauer symmetry class D is the $\mathbb{Z}_{2}$ number~\cite{teo,qiPRB08}. The $\mathbb{Z}_{2}$ number is obtained by the dimensional reduction of the second Chern number in the suspension of the base space, $\Sigma(S^{2}\times S^{1})$, which is given by the integral of the Berry curvature $\mathcal{F}\wedge\mathcal{F}$ over the suspension. The $\mathbb{Z}_{2}$ number in each mirror subsector is
\begin{align}
\nu_{\lambda} = \left(\frac{i}{\pi} \right)^{2} \int _{S^{2}\times S^{1}} Q_{3}~ \mod 2,
\end{align}
where $Q_{3}=\mathrm{tr}[\tilde{A}d\tilde{A} + \frac{2}{3}\tilde{A}^{3}]$ is the Chern-Simons form and the Berry connection $\tilde{A}$ is obtained from the eigenstates on the mirror reflection invariant plane.
For the vortex preserving the mirror symmetry, the $\mathbb{Z}_{2}$ invariant in the $\lambda$ subsector is
\begin{align}
\nu_{\lambda} = \ell \kappa_{\lambda}~ \mod 2,
\end{align}
where $\kappa_{\lambda}$ is the vorticity of the order parameter in the $\lambda$ subsector, and $\ell$ is the first Chern number characterizing the bulk topology of the mirror invariant plane and $\ell=\pm 1$ for $\lambda = \pm i$. On the basis of the total angular momentum $\Gamma_{M}$,  the vorticity $\kappa_{\lambda}$ is equivalent to the vorticity $\kappa_{M}$ of $J_{z}=M$ Cooper pairs. Hence, the mirror-protected $\mathbb{Z}_{2}$ invariants for an isolated HQV with $(\kappa,n)=(1/2,1/4)$ and $(1/2,-1/4)$ are $(\nu_{\lambda=+i},\nu_{\lambda=-i})=(0,1)$ and $(1,0)$, respectively. Hence, the zero energy state bound at each HQV is protected by the $\mathbb{Z}_{2}$ invariant regardeless of the intervortex distance $d_{\mathrm{V}}$. In Ref.~\cite{Masaki:2019rsz}, we found that a pair of the zero energy states exist in the $o$ vortex. The topological protection of a pair of zero energy states are also characterized by the $\mathbb{Z}_{2}$ invariants as $(\nu_{\lambda=+i},\nu_{\lambda=-i})=(1,-1)$.

Finally, we introduce another topological invariant associated with the chiral symmetry~\cite{tsutsumiJPSJ13,tsutsumiPRB15,Masaki:2019rsz,mizushimaJPSJ16}. Consider the vortex preserving the $P_{3}$ symmetry, that is, the magnetic $\pi$ rotation symmetry. Then, one can construct the chiral operator $\check{\Gamma}$ as a combination of $\mathcal{C}$ in Eq.~\eqref{eq:phs} and $P_{3}$ operator, and the BdG Hamiltonian $\check{\mathcal{H}}({\bm k},\theta)$ preserves the chiral symmetry,
\begin{align}
\{\check{\Gamma},\check{\mathcal{H}}({\bm k},\theta) \}=0, ~ \hat{\Gamma}^{2} = +1
\end{align}
for $k_{y}=k_{z}=0$. As long as the chiral symmetry is preserved, one can define the one-dimensional winding number for $\theta$ as
\begin{align}
w_{\mathrm{1d}}(\theta) = -\frac{1}{4\pi i} \int dk_{x} \mathrm{tr}\left[
\check{\Gamma}\check{\mathcal{H}}({\bm k},\theta)\partial _{k_{x}} \check{\mathcal{H}}({\bm k},\theta)
\right]_{k_{y}=k_{z}=0}.
\end{align}
The winding number for the $o$-vortex state is $w_{\mathrm{1d}}(\theta=0) = 2$ and $w_{\mathrm{1d}}(\theta=\pi) = -2$, regardless of the boundary condition. Then, the topological invariant is defined as the difference of $w_{\mathrm{1d}}(\theta)$, $w_{\mathrm{1d}} = \frac{w_{\mathrm{1d}}(0)-w_{\mathrm{1d}}(\pi)}{2} = 2$. This ensures the presence of the two zero energy states at $k_{z}=0$. Similarly, the winding number describes the topological protection of the zero energy state in an isolated HQV. We thus conclude that the zero energy state and its non-Abelian anyonic nature in the HQVs are protected by both the mirror $\mathbb{Z}_{2}$ invariants $\nu_{\lambda}$ and the winding number $w_{\mathrm{1d}}$.

In summary, a single Majorana zero mode bound at the HQV in the $D_4$-BN state is protected by the two topological invariants associated with the mirror reflection symmetry and chiral symmetry. These topological invariants ensure that the Majorana zero mode behaves as a non-Abelian (Ising) anyon. Therefore, the HQV hosts two-fold non-Abelian anyons characterized by both Majorana fermions and a non-Abelian first homotopy group. Both the symmetries can be preserved and topological invariants are unchanged even if two HQVs form a bound molecule and the magnetic field is applied along the vortex line. Therefore, the Majorana zero mode and its non-Abelian anyonic nature are tolerant against a magnetic field.

\bibliographystyle{apsrev4-2}

redpajama_set_name: RedPajamaArXiv


The National Mall is in need of a long overdue makeover, and the National Park Service wants your input on just what to change. The NPS has a plan that would include improved walkways, more food choices, and yes -- more bathrooms.
More than 25 million visitors flock to the Mall each year, and as you can imagine the 600 acres take a harsh daily beating.
"Many people go to the National Mall three or four times a year ... for a few people it may be a once-in-a-lifetime experience," Susan Spain, the National Mall Plan project executive, told the Washington Post.
So what should be improved? The National Park Service is taking suggestions from the public through March 18. Options can be read in a brief 600-page document, or viewed online.
The National Mall needs almost $500 million in repairs, so a private group that's trying to help raise the money held its second annual luncheon to draw attention to the issue.
Union Square: NPS would restore the Ulysses S. Grant Memorial to make it the focal point of Union Square. It would also be transformed into a larger venue able to accommodate more First Amendment demonstrations and events. The reflecting pool may also be downsized to make the space more versatile and reduce water use. The area would also get more public restrooms and drinking fountains.
The Mall: Gravel pathways would be paved to improve circulation. NPS would also replace all compacted soils with engineered soil capable of withstanding intensive use. A paved welcome plaza at 12th St and Jefferson Dr SW would also include a visitor contact station with "high-capacity" public restrooms, multiple orientation maps, and a large model or pavement map of the National Mall.
The Park Service says a new proposal for the National Mall's design would be easier for visitors to navigate.
Washington Monument: Replace the Sylvan Theater with a multipurpose performance space that would also serve food. It would also include more public restrooms.
Constitution Gardens: The current lake would be reconstructed to be self-sustainable, and the area would be rebuilt to provide food service and entertainment options.
The plan also calls for more seating near the Vietnam Veterans Memorial, expanded restrooms within the Lincoln Memorial, and widened walkways at the Korean War Veterans Memorial. NPS would also reconstruct the tidal basin area to accommodate wider walks and improve bicycle and vehicle circulation.
To get a CD version of the entire plan, complete wtih other options, send an e-mail request to nationalmallplan@nps.gov and put "Request copy of National Mall Plan DEIS" in the subject line. In the actual e-mail include your full name and complete mailing address.


Published 04/18/2019 06:42:09 pm at 04/18/2019 06:42:09 pm in My Home Thermostat.
my home thermostat why i no longer use nest auto away auto adjust your smart thermostat devices based on your location skylark changing my home thermostat.
my home thermostat says in recovery,replacing my home thermostat,my home thermostat is blank in house,my home thermostat is blank and ac,my home thermostat is blank carrier,my home thermostat is blank,my home thermostat reads the wrong temp on nest,my home thermostat reads the wrong temp on phone,why does my home thermostat keep clicking that pen,why does my home thermostat keep clicking text,why does my home thermostat keep clicking meme.


text:
Q: How do I join two tables in hibernate and Spring How do I join two tables in hibernate and Spring. below is my suto java code and I need to do a join on objectA where the name field is equal to the name field in objectB but I am going to be searching on ObjectA ID field but I need returned. ObjectA ID, ObjectA Name, ObjectA Regin, ObjectB Address.
//
// CLASS OBJECT A
//
@Entity
@Table(name = "tableA")
public class ObjectA {

    @Id
    @Column(name = "id")
    private String id;

    @Column(name = "name")
    private String name;

    @Column(name = "region")
    private String region;

}

//
// CLASS OBJECT B
//
@Entity
@Table(name = "tableB")
public class ObjectB {

    @Id
    @Column(name = "id")
    private String id;

    @Column(name = "name")
    private String name;

    @Column(name = "address")
    private String address;

}

can someone please tell me how to do this within the java code.

A: Add this to your A class:
@OneToOne
@JoinColumn(name="name")
private ObjectB objectB;

So that when you retrieve for A, you'll get inside corresponding B by name.

A: Use a cross join with a condition in the where clause to limit the join.  This is the only good way (other than native sql) that i know of, to join two objects when there is no mapped relationship between them.
You can do this easily with an hql query
select a.id, a.name, a.region, b. address
from ObjectA a, ObjectB b
where a.id = b.id

A: You can also use inner join
select A.ID,A.Name,A.Regin,B.Address
from ObjectA as A inner join  ObjectB as B

redpajama_set_name: RedPajamaStackExchange


text:
Vol. 4 No. 2 (2015): February /
Connecting Asian Heritage Conservation to the Idea of Performative Regionalism: A Case of Community-Enhancing Design Interventions in the Historical Art District of Liulichang Beijing
Diana Thamrin Petra Christian University
https://doi.org/10.18533/journal.v4i2.654
Community building, Design Interventions, Asian Heritage Conservation, Performative Regionalism
The active and sometimes ruthless modernisation in Asia has triggered an urgent need to secure the protection and continuation of its rich heritage and diverse regional attributes. However, as in the case of China, the Asian perspective of conservation is different from the West in terms of the nature or ways of design interventions produced and its purposes. This phenomenon has frequently triggered criticisms from heritage conservation professionals. Hence, the objective of this paper is to explore the interventions done on Asian heritage sites, taking the Liulichang Art District in Beijing as the case study, and analyze the positive influence they have brought. The paper starts by distinguishing the Asian concept and values of authenticity in conservation that differ from the West and how these principles have been applied in Liulichang, a famous ancient street known for the selling and practice of classical Chinese arts, mostly for Chinese painting. Using the phenomenological method of analysis, the paper further elaborates on the importance of community building in learning and appreciating the art of Chinese painting and discusses the positive impact made by the design interventions in Liulichang, particularly in terms of community engagement and creation of novel ways to accommodate traditional cultural practices of Chinese painting. Results reflect that the Asian perspective of conservation do not always follow the principle of minimum intervention favoured by the West, but how contemporary interventions could be merged into the heritage site to revive regional communities and cultural activities, connecting Asian architectural conservation with the design approach coined by Barbara Allen (2005) as Performative Regionalism, hence developing the idea and practice of this approach as a result of the discussion. Rather than merely following textual or scientific procedures like in the West, this approach requires a more experiential way of identifying with the regional qualities of a historical place through humanistic and participatory ways of interventions. Consequently, people can connect themselves with their cultural community, practice their culture with a much deeper and novel experience as well as communicate their unique cultural values to the contemporary society even in the face of globalization.
Diana Thamrin, Petra Christian University
Interior Design Department, Faculty of Art and Design, Petra Christian University
Allen, L. Barbara (2007).On Performative Regionalism. In Canizaro, Vincent B. (Ed.), Architectural Regionalism: Collected Writings on Place, Identity, Modernity and Tradition (p. 146-155). New York: Princeton Architectural Press.
Byrne, Denis (2014). Counterheritage: Critical Perspectives on Heritage Conservation in Asia. New York: Routeldge.
Kwanda, Timoticin (2010). Tradition of conservation: redefining authenticity in Javanese architectural conservation. In: Heritage 2010 – Portugal: International Conference on Heritage and Sustainable Development
Li, Xiaodong and Yang, Kang Shan (2007). The Chinese Conception of Space. Beijing: China Architecture and Building Press.
Lin, Ci (2010). Chinese Painting: Capturing the Spirit of Nature with Brushes. Beijing: China Intercontinental Press.
Loh, Laurence (2007). Conveying the Spirit of Place. In Engelhardt, R and Horayangura, M (Eds), Asia Conserved: Lessons Learned from the UNESCO Asia-Pacific Heritage Awards for Culture Heritage Conservation, Bangkok: UNESCO
Moustakas, Clark (1994). Phenomenological Research Methods, UK: Sage Publications
Pallasmaa, Juhani (2012). The Eyes of the Skin: Architecture and the Senses. United Kingdom: John Wiley and Sons Ltd.
Xu, Chenghei (2000). Old Beijing: People, Houses and Lifestyles. Jiangsu: Foreign Language Press
Yoo, Hyunjoon (2012). Modernism: A Hybrid of Eastern and Western Culture. Shanghai: Tongji University Press.
Yuen, Belinda (2005). Strengthening Urban Heritage in Singapore: building Economic Competitiveness and Civic Identity. Singapore: Global Urban Development Volume 8.
Vol. 4 No. 2 (2015): February

redpajama_set_name: RedPajamaCommonCrawl


Encompassing the natural beauty and life of Australia in a bottle of goodness.The Jack N' Jill Natural Bathtime Serenity Bubble Bath is naturally scented, plant-based, hypoallergenic and great for skin of all ages.
Containing a unique, soothing, aromatic blend of natural oils and extracts, it is the ideal choice for before-bed baths.With calming, relaxing essential oils of native Australian White Cypress, Australian Lavender, Clary Sage and Chamomile, this non-irritating formula also has antiseptic and anti-inflammatory properties (brought to you by Soap Bark and orange pearl) while being gentle on even the most sensitive of skin.
Glycerin provides deep hydration to the skin, while Quinoa Seed Extract and Panthenol enrich the skin with essential B vitamins and amino acids. Soaking in a warm bubble bath will leave skin feeling super soft and deeply cleansed (and the relaxing essential oils of White Cyprus and Lavender are perfect before bed time).
Jack N' Jill Natural Bathtime Serenity Bubble Bath creates rich, long-lasting bubbles that kids will love and comes in a handy 300 ml pump bottle (anything that helps manage bath time with one hand is a bonus!).


text:
Are These 90 Day Fiancé: The Other Way Season 1 Couples Still Together?
TLC's reality show ended its first season with some couples questioning their future
By Chris Harnick Oct 22, 2019 11:00 PMTags
TVReality TVEntertainment90 Day Fiancé
90 Day Fiancé: The Other Way followed six couples are they left family and friends and traveled to foreign countries all in the name of love.
Tiffany, along with her 8-year-old son, traveled to South Africa and married recovering gambling addict Ronald. Jenny left her family behind to move to India for Sumit, only to find out Sumit had one big secret: he's married. Corey did his best to get Evelin to agree to marriage with him in Ecuador. Paul moved to Brazil to be with his pregnant wife Karine. Laura returned to Qatar to be with Aladin, a man she married days after meeting in person. Deavan hit the road to South Korea to be with Jihoon, the father of her son. Not everything worked out.
The first season ended on Monday, Oct. 21 with, yep, some heartbreak, tears, talks of divorce and so much more.
So, who's still together?
ronald smith Instagram
Tiffany Franco & Ronald Smith
Status: Separated
The two, who met while Franco was on vacation in South Africa, documented their romance on the spinoff show, 90 Day Fiancé: The Other Way. They welcomed their daughter Carley Rose in July 2019. However, they split in January 2020, after Smith accused Franco of cheating on him.
Corey and Evelin
Status: Engaged
Despite voicing her desire not to get married, Evelin accepted Corey's marriage proposal. Rumors swirled after Corey was spotted with 90 Day veteran Larissa Dos Santos Lima, but he assured fans he and Evelin were still together.
Tiffany and Ronald
Status: Married, but living apart
Tiffany took her son back to the United States and had her daughter stateside as well. Ronald is still in South Africa and as of the "Tell All" he has yet to file the paperwork for his visa to come to America. Tiffany, however, said she's planning a trip to South Africa with her kids.
Paul and Karine
Despite Karine's absence from the "Tell All" reunion, and all of her divorce talk during the first season of The Other Way, Paul and Karine still seem very much together.
Laura and Aladin
Status: Split
During the "Tell All," Aladin said he wanted a divorce, and then later said he would consider marriage counseling. Laura seemed to think her marriage was over. On Instagram, she said she lost her marriage because of the show. Aladin was asked on Instagram his status with Laura and said they were "definitely not" together. "But I wish her no harm and wish her good luck with her future men," he wrote.
Deavan and Jihoon
Deavan revealed she left Korea because Jihoon didn't get his act together and she couldn't bring her daughter over to live at his parent's house. They're still married, and she does plan to return to Korea, but it's on Jihoon to get their living arrangements together.
Jenny and Sumit
Status: Living apart.
At the "Tell All," Sumit revealed he's separated from his wife and is still quite in love with Jenny. Jenny confirmed that she too would like to be back with Sumit, and the plan, once he's divorced, is for her to go back to India. Right now, she's living with her daughter.
90 Day Fiancé returns with new episodes on Sunday, Nov. 3 on TLC.
Too Hot to Handle's Francesca Farago and Demi Sims Share a Kiss


text:
Amir Kertes (; April 1964 - January 1, 2018) was an Israeli musician and singer.

Biography
Kertes is the lead singer and songwriter of the rock band Ra'ash (רעש). Ra'ash released their debut album Noise Only Noise. N. (רעש רק רעש. ק.) in 1994 to critical acclaim. Kertes wrote and sang most of the songs on the album, although the songs that were written and sung by the second singer Jonnie Shualy gained more popularity.

In 1995 Kertes and all of the members of Ra'ash participated in recording of Shualy's first solo album The Thousand and One (האלף ואחד).

In 1996 Ra'ash released their second album, "Tmimot" (תמימות) . All of the album was written and sung by Kertes. The group appeared on the TV and two songs received limited TV and radio play, but the sales were low. In the same year Kertes played in an album by the popular Israeli singer Yael Levi, which Shualy produced.

At that time Kertes moved from Tel-Aviv to Ezuz, a small moshav in the Negev desert.

In 1998 all members of Ra'ash played on the debut album of Adi Ran (עדי רן), a baal teshuva. The album became popular mostly in the Jewish religious communities.

In 2000 Ra'ash released their last album as a band, Ani Ze Lo' Ata (אני זה לא אתה). Singing and songwriting on this record were roughly divided between Kertes and Shualy. The album received positive reviews, but the band went on an indefinite hiatus shortly after its release.

In 2001 Ra'ash played their last show as a band at a two-day festival of Nana Disc artists.

In 2003 Kertes released his first solo album, Yellow Sea (ים צהוב).

Death
On January 1, 2018, Kertes died at the age of 53 from lung cancer. He was interred at Yarkon Cemetery.

External links
 Former rocker finds a quieter studio - Jerusalem Post
 Sounds of the 'yellow sea' - Jerusalem Post

1964 births
2018 deaths
21st-century Israeli male singers
20th-century Israeli male singers
Israeli male composers
Deaths from lung cancer in Israel
Burials at Yarkon Cemetery

redpajama_set_name: RedPajamaWikipedia


The Georgia 15 Contemporary Façade is a Brand New Design from Bellmarch. Specifically designed to fit most 15m wide blocks, or larger, to accommodate clients who are searching for a compact & functional good looking home around 27 squares. This home suits the first home buyer or second home buyer looking for a modern & easier to maintain home.
Open for viewing seven days a week from 9am - 5pm at 18 Clement Road, Edmondson Park.
See Brochure for Comprehensive List of Inclusions.
Disclaimer: All images, plans, 3D artists drawings are solely for the express purpose of illustration only and are to be used as a guide only. All prices are for brick finish only. Some images and floor plans may contain upgrades, please discuss any individual plan or design with your sales consultant for guidance.


text:
Third Space Launches Give20 Charitable Giving Program October 24 With Event Supporting Housing First Milwaukee
Local Brewer Kicks Off New Charitable Giving Program: Give20, With 20% of Proceeds Donated to Local Causes
Milwaukee, WI, October 16, 2019—Award-winning Milwaukee craft brewer, Third Space Brewing, has started a new charitable giving program to support local organizations working on Youth Development and Homelessness initiatives.
It is called the Give20 Program and it will include the brewery donating 20% of tap room sales one night per month to local nonprofits. Each month, Third Space will select a new charity partner for a Give20 Night. The goal of the Give20 Night is to help local organizations raise awareness and funds to further support their charitable efforts.
Third Space will host its first Give20 Night October 24th from 4:00-9:00 p.m. at the brewery's tap room at 1505. W. St. Paul. Ave. in Milwaukee's Menomonee River Valley. Third Space will donate 20% of the night's proceeds to Milwaukee County's Housing First Initiative.
Third Space announced its first Give20 partnership with Housing First at its 3rd Anniversary Party last month. To jump start the Give20 Program, Third Space committed to donate 20% of tap room sales of its 3rd Anniversary Triple IPA, Billy Mumphrey's Downfall to Housing First. The combined funds from 3rd Anniversary Beer sales and from the upcoming October 24th Give20 Night will be used to help transition residents of the make-shift tent community on the east end of the Menomonee River Valley into permanent housing before winter hits.
Give20 Program Details
Third Space will limit the Give20 Program to two types of charitable organizations to create a greater impact on causes most important to the company's employees. Those causes are Youth Development and Homelessness.
Third Space Co-Founder and Director of Sales & Marketing, Andy Gehl explained how the brewery chose these two causes: "Our motto at Third Space is that you have your home, you have your work, but everyone needs a 'third space'. However, it is difficult to enjoy a 'third space' if you don't have a first space, a home. Homelessness is also an issue directly facing our community in the Menomonee River Valley with the tent encampment at the east end of the valley. We want to do our part to help our neighbors there find permanent housing."
Gehl added: "Youth Development is also very important to us because my co-founder, Kevin Wright, and I met and worked together for many years as summer camp counselors where we witnessed the impact great youth programming can have on a child's life."
Organizations that work in these two areas that are interested in partnering with Third Space on the Give20 Program should send an inquiry via the brewery's donation portal at www.thirdspacebrewing.com/donations.
About Housing First
Milwaukee County Department of Health and Human Services' Housing First Initiative follows a best practice housing model that prioritizes providing people experiencing homelessness with affordable, independent and permanent housing as quickly as possible without pre-condition. Voluntary, community-based support services are provided as needed. Donations are needed for startup kits to assist individuals with moving into apartments.
All Articles Up Next: Get Your S'More On at Third Space Every Thursday in October


"From the Land of Sky Blue Waters" might bring back nostalgic scenes of Hamm's Beer commercials or family vacations on one of the nearly 12,000 lakes in Minnesota. With the prevailing Minnesota Nice perspective, Minnesotans also don't like to brag much, so they keep their slogan to the "Land of 10,000 Lakes," and it does look impressive with all those zeros. The state is also home to over 6,000 rivers and streams, including the mighty Mississippi River, which begins at Lake Itasca State Park in northern Minnesota and flows south to the Gulf of Mexico.
In early days, the state was inhabited by the Dakota and Ojibwe/Anishinaabe, before an influx of voyageur fur traders and European settlers. Many of these settlers came from New England and became farmers and loggers, using the riverways for transport. Later in the range country, underground and open-pit iron mining was booming, and the ore was sent by rail to the ports of Duluth and Two Harbors for shipping across the Great Lakes.
Now, the state consistently ranks well for its standard of living, low unemployment rate and lifestyle opportunities. In 2018, Minnesota rated #2 (behind Iowa) on the U.S. News and McKinsey & Company Best States report, largely because of its high rankings for quality of life, opportunity for its citizens, health care, infrastructure and education (see full report here).
You can find your favorite setting for work and play within the state's bountiful choices of urban, suburban, country or secluded locations. The Minneapolis/St. Paul area supports a large segment of the state's population and a wide variety of cultural, recreational, educational and business opportunities.
This Twin Cities area features the popular Mall of America, the Minneapolis–St. Paul International Airport (MSP), art museums, sporting events, including the Minnesota Vikings, Twins, Timberwolves, Wild, Lynx and college games, and an abundance of live theatre, including the Guthrie Theater situated on the banks of the Mississippi River. With its beautiful lakes, rivers, parks and bike trails, the metro offers outdoor activities for everyone.
In Greater Minnesota, you'll find open spaces, resort towns, farmland and rural communities. The state is home to a rich variety of parks, including national forests, the breath-taking Boundary Waters Canoe Area Wilderness and Voyagers National Park. You'll also find opportunities for music, birding, festivals, zoos, aquariums and amusement parks. There are casinos, shopping centers, quaint towns, antiques and boutiques.
Except for Alaska, Minnesota is the most northern state in the U.S. It borders Lake Superior and draws visitors to its northern region with attractions such as the Split Rock Lighthouse, Gooseberry Falls State Park, the Superior Hiking Trail, biking, boating and scenic views.
The state is known for its medical care industry with the distinguished Mayo Clinic and University of Minnesota Medical School. General Mills, 3M, Target, Best Buy, Cargill and Carlson Companies of Radisson Hotel fame are just a few of the well-known Minnesota businesses. The state has also produced celebrated musicians such as Prince, Bob Dylan, the Trashmen, The Andrews Sisters and Soul Asylum.
Many movies and TV shows have been filmed in Minnesota, including Purple Rain, North Country, Sweet Land, Airport, Drop Dead Gorgeous, A Serious Man and Untamed Heart—or have featured a Minnesota setting, such as in Grumpy Old Men, Grumpier Old Men, The Mighty Ducks, the Mary Tyler Moore Show and Little House on the Prairie.
A few of Minnesota's famous authors are Laura Ingalls Wilder, Sinclair Lewis, Garrison Keillor, LaVyrle Spencer, Joann Fluke, Tami Hoag, and William Kent Krueger who has written the popular Cork O'Connor series featuring the Minnesota north country and its original inhabitants, the Anishinaabe.
Although many people complain about the cold winters, snow and ice, the state has gorgeous variety with its seasons. In spring, the flowering trees are fragrantly beautiful, and the air is fresh. Bicyclists have options of many beautiful trails including the Mississippi River Trail and the North Star Route for energetic riders which spans from the Twin Cities to Duluth and ends along the Canadian border overlooking Pigeon Falls, Minnesota's highest waterfall. Fishing and baseball are also back in full swing.
Summer brings golf, festivals, garage sales, county fairs, outdoor concerts and annual running marathons like the Duluth-hosted Grandma's Marathon along the North Shore of Lake Superior. The lakes and rivers entice people for fishing, swimming, water skiing, boating, reunions and camping, and the Great American Get-Together, Minnesota's State Fair, closes out the summer, drawing thousands daily for the 12 event-filled days running through Labor Day.
In fall, Minnesotans are ready for football, and as the leaves turn color, it's time for a drive in the woods and along the rivers. Runners participate in the Twin Cities Marathon which charts a course around metro lakes and the Mississippi River. All seasons have festivals, and one of the largest in fall is the Renaissance Festival with all its bold adventures. It's also time for a trip to the apple orchard and cider mill, music and friends at street dances, and beer and brats at Oktoberfest.
Winter might be cold and snowy, but in Minnesota, it's a winter wonderland of beauty and activity. Minnesotans revel in it. From the Winter Carnival, snow sculptures and ice carvings to the opportunity for ice fishing, skating, skiing and snowmobiling, the fun continues. For some brave souls, the Polar Plunge is a daring and worthwhile event. Holidays also bring opportunity to cut down your own Christmas tree, gather with friends, shop, dine and celebrate, or view seasonal lights—maybe at the Duluth Bentleyville Tour of Lights.
In this state of 5.5 million people and land of opportunity, there are a lot of reasons to make it your home. Whether you prefer a single-family home, townhome or condo, there's a neighborhood waiting for you. As always with such an important transaction, if you're a buyer, it's equally as important to work with an experienced real estate agent who can help you prepare to move quickly in a high-demand market.
Currently in Minnesota, it's a seller's market. That spells a great time to sell your home or commercial building if you've been considering a change. The real estate business is always active as people buy and sell homes and business owners and investors look for commercial property opportunities. Wherever you would like to reside, retire or invest, you can find it in Minnesota.
To help you find the best source of local information and expertise, here is our recommended list of the top 25 real estate agents in the state of MN. Their years of experience and knowledge in their markets will provide you with the guidance needed for a smooth and successful real estate transaction. Contact one or more of these top 25 agents for an interview today!


text:
Big Breasts and Wide Hips is a novel by Mo Yan. It won the Dajia Honghe Literature Prize in 1997. The book tells the story of a mother and her eight daughters and one son, and explores Chinese history through the 20th century. The novel enthusiastically praises the original creator of life—the greatness, simplicity and selflessness of the mother, and the unparalleled significance of the inheritance of life. And in this flow chart of life, filled with the smoke of history and war, it is true, without any prejudice, and reproduces the history of a period of time. In 1997, Big Breasts and Fat Hips won China's Master Literature Award.

Characters
Shangguan Lushi, the mother
Shangguan Laidi, Eldest Sister, daughter of Lushi and Big Paw. Married to Sha Yueliang. Mother of Sha Zaohua.
Shangguan Zhaodi, Second Sister, daughter of Lushi and Big Paw. Married to Sima Ku. Mother of twins, Sima Feng and Sima Huang.
Shangguan Lingdi, Third Sister, also known as Bird Fairy. Daughter of Lushi and a peddler of ducks. First wife of Speechless Sun. Mother of Big Mute and Little Mute.
Shangguan Xiangdi, Forth Sister, daughter of Lushi and a doctor. Sold herself to a brothel during the famine in order to save her family.
Shangguan Pandi, Fifth Sister, daughter of Lushi and a butcher. Married to Lu Liren. Mother of Lu Shengli. Later changed her name to Ma Ruilian.
Shangguan Niandi, Sixth Sister, daughter of Lushi and a monk. Married to the American pilot Barbitt.
Shangguan Qiudi, Seventh Sister. Lushi gave birth to her after raped by deserts. Adopted by a Russian Duchess.
Shangguan Yunü, Eighth Sister, blind, daughter of Lushi and the Swedish missionary Maloja.
Shangguan Jintong, 'me' in the novel, son of Lushi and Maloja. Afflicted with breast fetishism.

Reception
Big Breasts and Wide Hips received near universal critical acclaim from Western literary critics who praised Mo Yan's inventive storytelling and use of his unique style of magical realism to describe the surrealism the average Chinese peasant felt living under the Japanese occupation.
Contributor for The Guardian, Paul Mason declared Mo Yan to be the Chinese equivalent of Thomas Pynchon, concluding that Mo Yan was "unlike any of the great living authors."

Jonathan Yardley of The Washington Post praised Mo Yan's dedication to feminism throughout the novel, but offered numerous reservations about the quality of the novel. Most of Yardley's criticism focuses on the stale prose and clumsy characterization of Jintong.

References

Chinese historical novels
Novels by Mo Yan
1996 Chinese novels
Feminist novels
Arcade Publishing books


text:
Q: Adding new cipher suites in SSL (TLS) using CNG As far as I know since Windows Vista CNG(Cryptography Next Generation), a personal user can add a new own cipher algorithm, which makes an own coded message (according information, for example, from http://technet.microsoft.com/en-us/library/cc730763(v=ws.10).aspx).
But CNG SDK has not commented whether we can also add new cipher suites in SSL.
Is it possible, IE (Internet Explorer) could use new algorithms for a
security connection through 'https'? What methods are possible to it
in CNG? I need assistance to add new chiper suites in ssl(tls), making a new
provider for ssl(tls) and so on.
Thanks for you help.


text:
Chemistry and Chemical Engineering (10)
"F15" x
Page:123456
Economic disintegration of the European Union: Not unavoidable, but probable
Acta Oeconomica
Volume 66: Issue s1
https://doi.org/10.1556/032.2016.66.s1.3
Author: Leon Podkaminer
It is argued that European integration has not fulfilled its chief economic promises. Output growth has been increasingly weak and unstable. Productivity growth has been following a decreasing trend. Income inequalities, both within and between the EU member states, have been rising. This sorry state of affairs is likely to continue — and likely to precipitate further exits, or eventually, the dissolution of the Union. However, this outcome is not unavoidable. A better integration in the EU is possible, at least in theory. Also, the negative consequences implicit in the existence of the common currency could be neutralised. However, the basic paradigms of the economic policies to be followed in the EU would have to be radically changed. First, the unconditional fiscal consolidation provisions still in force would have to be repelled. Second, "beggar-thy-neighbour" (or mercantilist) wage policies would have to be "outlawed".
European integration perspectives: From cohesion to divergence?
Authors: Vedran Recher and Nataša Kurnoga
This paper examines the impact of EU enlargement and the global economic crisis on the relative development of the EU countries. This effect is assessed by applying multivariate analysis to the whole set of 28 European countries at three representative points in time. The cluster analysis for the years 2002, 2007, and 2012 grouped the countries according to the range of economic development indicators showing within-EU cohesion before the EU enlargement, after the enlargement wave, and after the crisis. The findings show that a decrease in the development differences after the enlargement was replaced with an increase in these differences after the crisis, thus contributing to the existing debate about the success of cohesion and future of European integration. These results are somewhat worrying for the new member states of the EU as well as for EU membership candidates and their prospective development within the integration.
Globalization, secular stagnation, and soft national balances: A pro-equilibrium manifesto
https://doi.org/10.1556/032.2018.68.s.11
It is argued that increased freedom to run economic activities combined with the growing impotence of national governments (i.e., globalization) have contributed to the secular growth slowdown at the global level. Fast globalisation-driven growth of international trade has unleashed the global race for economic surpluses. The process involves the suppression of wages and widening income inequalities – restricting aggregate demand globally. A "beggar-thy-neighbor" tactics of keeping large trade surpluses by countries successfully suppressing wages and domestic demand is likely to be unproductive. Overcoming the secular stagnation may not be possible without safeguarding equilibrium (or balance) in international transactions between major industrial countries – even if this may necessitate that in most (or all) of them the public sectors run large fiscal deficits permanently.
Central and Eastern Europe: Trapped in integration?
https://doi.org/10.1556/032.65.2015.s1.6
The Central and Eastern European new Member States of the European Union (CEECs) went through the transition process following the commandments of the Washington Consensus, which gradually evolved into the "integrative growth model". External liberalisation exposed the CEECs to recurring problems over external imbalances, bubbles driven by capital inflows, and resulting growth instabilities. Large foreign direct investment inflows attracted by repressed wages and low taxes do not accelerate growth. Arguably, real convergence would be much faster under a system with built-in limitations to free trade, free capital movements – and with more scope for traditional industrial, trade, incomes, and fiscal policies.
Crisis and economic growth in the EU
Medium and long-term trends
https://doi.org/10.1556/aoecon.61.2011.4.4
Authors: P. Halmai and V. Vásáry
The study analyses the impacts of the financial and economic crisis on potential growth in the European Union. It identifies the main channels of impact mechanism and carries out quantitative estimations in order to reveal the medium and long-term trends. According to over findings the impacts of the crisis are significantly different in the main country-groups of the EU. The basic structural problem of the EU is considered the decreasing trend in potential growth which might be further strengthened through the lasting consequences of the crisis.
The effects of the economic crisis on income convergence in the European Union
Author: Nenad Stanišić
This paper evaluates income convergence in the European Union, between "old" (EU15) and "new" member states from Central and East Europe (CEE10), and among the countries within these two groups. The GDP per capita convergence should be expected according to the exogenous economic growth model and neoclassical trade theory. The presence of σ-convergence and both absolute and conditional β-convergence is tested for on a sample of 25 European Union countries (EU25). Results confirm the existence of β-convergence of GDP per capita at purchasing power parity among EU25, but not among EU15 and CEE10 countries. σ-convergence has been confirmed among EU25 and CEE10 countries, while GDP per capita has been diverging in the EU15 group of countries. Moreover, the results reveal that recent economic crisis has reversed long-term tendencies and led to income convergence within EU15 and divergence within CEE10. During the crisis, the income differences among the EU25 countries have increased, but the scope and duration of this effect has been limited and has not affected the long term convergence path. However, the obtained long term speed of convergence is significantly lower compared with the previous researches.
EURO zone crisis and EU governance: Tackling a flawed design and inadequate policy arrangements
(An essay)
Author: Daniel Dăianu
This paper focuses on the roots of strain in the European Monetary Union (EMU). It argues that there is need for a thorough reform of the EU governance structure in conjunction with radical changes in the regulation and supervision of financial markets. The EMU was sub-optimal from its debut and competitiveness gaps did not diminish against the backdrop of its inadequate policy and institutional design. The euro zone crisis is not related to fiscal negligence only; over-borrowing by the private sector and poor lending by banks, as well as a one-sided monetary policy also explain this debacle. The EMU needs to complement its common monetary policy with solid fiscal/budget underpinnings. Fiscal rules and sanctions are necessary, but not sufficient. A common treasury (a federal budget) is needed in order to help the EMU absorb shocks and forestall confidence crises. A joint system of regulation and supervision of financial markets should operate. Emergency measures have to be comprehensive and acknowledge the necessity of a lender of last resort; they have to combat vicious circles. Structural reforms and EMU level policies are needed to enhance competitiveness in various countries and foster convergence.
Comparative advantages, job destruction and the regional pattern of polish unemployment
Authors: A. Newell, F. Pastore, and M. Socha
This paper investigates the relationship between industrial restructuring and regional unemployment in Poland. Poland's regional unemployment broke out of nothing at the beginning of the 1990s decade. Since then, it has remained remarkably unchanged over the decade for a variety of factors, such as the gradual restructuring process, labour supply rigidities and technological differences. The role of each of these factors is assessed within the framework of hazard functions applied to the inflow to unemployment from a job, computed using Polish Labour Force Survey data. When voivodships are grouped according to their unemployment rate it can be seen that low unemployment voivodships form a heterogeneous group, including both rural and urban areas. Applying a new method of analysis of the labour market effects of trade integration, the paper reveals circumstantial evidence on how Poland's international comparative advantages in labour-intensive manufacturing combine with the economic advantages of urbanised regions to play a significant role in shaping the regional distribution of Poland's unemployment.
Relocation, standardization and vertical specialization: Core–periphery relations in the European automotive value chain
Society and Economy
https://doi.org/10.1556/204.2019.001
Authors: Tamás Gerőcs and András Pinkasz
The global automotive industry has been exposed to an overproduction crisis for several decades. Under the pressure of restructuring, automotive companies renew both the geographical scope and the technological standardization of their production processes. We analyze the effects this restructuring had on the development of European economies in order to understand whether vertical specializations in the automotive value chain can lead to Central and Eastern European countries' catching up to advanced economies, or whether such specializations reproduce new forms of core-periphery relations. In order to answer this question, we introduce a new methodological approach to understand vertical specialization in the global value chain from a semi-peripheral perspective. We combine the theory of global value chains with Vernon's product life-cycle theory. In the research we focus on the standardization of the production of electric engines behind the geographical relocation of production between core and periphery.
The European Union's failed "Lisbon strategy"
https://doi.org/10.1556/socec.32.2010.1.8
Author: Arno Tausch
Is Europe becoming the world's leading knowledge-based economic area of the world, as European leaders planned at their Lisbon meeting in 2000? In this article, we analyze the Lisbon performance of the countries of the European Union from a long-term, structural perspective. We examine performance in the Lisbon indicators by factor analytical means. To measure progress, we observe contradictions between some of the indicators, chosen by the member governments and the European Commission. Finally, we conclude that only a Schumpeterian vision of capitalism as a process of "creative destruction," or rather "destructive creation," can explain these contradictions, which we empirically reveal in this analysis, and which beset the "Lisbon strategy" from the very beginning. European decision-makers often seem to be unaware of these underlying contradictions, which is why the goal of our paper is to clarify the processes involved. In Schumpeter's elitist-conservative visions of society, the decay of values in the capitalist society was an all-important element in his pessimistic theory developed in "Capitalism, Socialism, and Democracy". For Schumpeter the disappearance of the enterprising, male-dominated capitalist family was a critical element in his theory. But it is not the disappearance of the enterprising capitalist family that threatens the future of capitalism in Europe, but the often still existing incompatibility of work and family life, which explains more than 60% of the Lisbon process failure.


I have highlighted Michael Yon's work many times on this blog. Back in the day, he was taking great pictures and telling great stories. I, like many milbloggers and our readers were impressed with his quality of work and his inside track to get the stories told.
However he has now morphed into a combination of Dennis Hopper and Marlon Brando's characters from Apocalypse Now. He is so in love with himself that he must embarrass Afghans on a Thursday night. The guy drinks his own kool-aid and believes himself the savior of Afghanistan or any other war or conflict that he finds himself in.
I don't know him personally, but run in the same circles as he used to and I know some that were very close to him the last time he was in Afghanistan before being thrown out of country. The common opinion from all is that he has lost his marbles, has no sense of reality anymore and does nothing but spout the great things he does and how he is the poor little victim. And, Michael if you are reading this I am not even talking about other milbloggers like the ones you recently have been going after in your Facebook rantings. None of the people I speak of are milbloggers, per se.
Michael recently posted on his facebook account a copy of a letter sent to him by a supposed soldier from in Afghanistan. The letter highlights so many OPSEC (Operational Security) violations, it isn't funny. For Michael to post such a letter highlighting supposed vulnerabilities and weaknesses in certain Afghanistan perimeter defenses is inexcusable. For a guy that I guess was a Special Forces SGM at one time, he, like the famed COL Kurtz has lost his way when it comes to the safety of American Soldiers.
Shame on you Michael and for the lies you continue to tell people to this day as you pursue you own little hate-filled agenda. You are violating the trust and readership of those who have become fans of your past work in order to focus the attention on you as you throw your little temper tantrum from Thailand. You remind me of a toddler in the grocery store line who throws a tantrum at their parent (McChrystal) because he/she won't give you a toy or a piece of candy. So you are going to make a scene in order to embarrass them. Do us all a favor and grow a pair, grow up and then STFU.
To read Michael's posting on Facebook, click HERE.
Bouhammer.com retracts all support it had for Michael Yon. I apologize for mis-leading my readers to the fact that he was one person to read and I hope you did not provide him any financial support. If you did, I am truly sorry for that too.
Well, Troy, I did (in a modest way) financially support Yon back in the day when he was posting great stuff from Iraq. I've watched recent developments with horror, like watching a car accident happen. I'm sure his donations and influence with readers are drying up – he's certainly lost me.
Much like the Main stream Media, Micheal Yon, has forgotten the fact that he/they are reporters. They do not make policy for the units they are embeded with. Those units are charged with protecting them and They should stick to the facts and yes drop a story if it endangers people. He has lost my resepect and I am sure that of those who's trust he comprimized.
I think maybe all along –people gave Michael Yon far more credit than he deserved.


Pie Five Pizza to Add Vegan Cheese in All 87 Locations by End of March!
What's the second best thing to a celebrity chef opening an all-vegan pizzeria? Pizza chains including vegan options in their menu due to increasing demand!
Many of Pie Five Pizza's crusts and sauces are already vegan, so customers can customize a perfect completely plant-based pizza! In addition to Daiya's Classic Blend being vegan, it is also soy-free, gluten-free, dairy-free, and tree-nut free!
With locations in 24 states, offering completely vegan pizza options to their standard menu is a very significant move, and shows the importance of customer trends and preferences!